# Random Tensor Networks with Non-trivial Links

Newton Cheng, Cécilia Lancien, Geoff Penington, Michael Walter, Freek Witteveen

► To cite this version:

Newton Cheng, Cécilia Lancien, Geoff Penington, Michael Walter, Freek Witteveen. Random Tensor Networks with Non-trivial Links. Annales Henri Poincaré, 2023, 25 (4), pp.2107-2212. 10.1007/s00023-023-01358-2. hal-04285851

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# Random Tensor Networks with Non-trivial Links

Newton Cheng, Cécilia Lancien, Geoff Penington, Michael Walter and Freek Witteveen

<figure><img src="image_3.png" /></figure>

**Abstract.** Random tensor networks are a powerful toy model for understanding the entanglement structure of holographic quantum gravity. However, unlike holographic quantum gravity, their entanglement spectra are flat. It has therefore been argued that a better model consists of random tensor networks with link states that are not maximally entangled, i.e., have non-trivial spectra. In this work, we initiate a systematic study of the entanglement properties of these networks. We employ tools from free probability, random matrix theory, and one-shot quantum information theory to study random tensor networks with bounded and unbounded variation in link spectra, and in cases where a subsystem has one or multiple minimal cuts. If the link states have bounded spectral variation, the limiting entanglement spectrum of a subsystem with two minimal cuts can be expressed as a free product of the entanglement spectra of each cut, along with a Marchenko-Pastur distribution. For a class of states with unbounded spectral variation, analogous to semiclassical states in quantum gravity, we relate the limiting entanglement spectrum of a subsystem with two minimal cuts to the distribution of the minimal entanglement across the two cuts. In doing so, we draw connections to previous work on split transfer protocols, entanglement negativity in random tensor networks, and Euclidean path integrals in quantum gravity.

## Contents

1. Introduction 2108

1.1. Notation and Conventions 2115

2. Random Tensor Network States 2116

2.1. The Replica Trick for Random Tensor Networks 2117

2.2. Maximally Entangled Link States and Minimal Cuts 2119

2.3. The Replica Trick for General Background States 2121

<figure><img src="image_4.png" /></figure>
<table><tbody><tr><td>2.3.1.</td><td>Normalization of Random Tensor Network States</td><td>2123</td></tr><tr><td>3.</td><td>Link States with Bounded Spectral Variation</td><td>2123</td></tr><tr><td>3.1.</td><td>Random Matrices, Free Probability, and Non-crossing Partitions</td><td>2124</td></tr><tr><td>3.1.1.</td><td>Random Matrix Theory and Wishart Matrices</td><td>2124</td></tr><tr><td>3.1.2.</td><td>Free Probability</td><td>2125</td></tr><tr><td>3.1.3.</td><td>Non-crossing Partitions</td><td>2128</td></tr><tr><td>3.2.</td><td>Entanglement Spectrum of Random Tensor Network States as a Free Product</td><td>2129</td></tr><tr><td>3.3.</td><td>Non-trivial Link States and Entanglement Negativity</td><td>2136</td></tr><tr><td>4.</td><td>Link States with Unbounded Spectral Variation</td><td>2142</td></tr><tr><td>4.1.</td><td>One-Shot Entropies</td><td>2142</td></tr><tr><td>4.2.</td><td>Recovery Isometries</td><td>2145</td></tr><tr><td>4.3.</td><td>One Minimal Cut</td><td>2151</td></tr><tr><td>4.4.</td><td>Two Competing Minimal Cuts</td><td>2153</td></tr><tr><td>4.5.</td><td>Computing Entropies with Two Minimal Cuts</td><td>2173</td></tr><tr><td colspan="2">Acknowledgements</td><td>2181</td></tr><tr><td>A.</td><td>Euclidean Gravity Path Integrals and Entanglement Spectra</td><td>2182</td></tr><tr><td>A.1.</td><td>The Replica Trick and Euclidean Path Integrals</td><td>2182</td></tr><tr><td>A.1.1.</td><td>Fixed-Area States</td><td>2184</td></tr><tr><td>A.2.</td><td>States at a Minimal Surface Phase Transition</td><td>2185</td></tr><tr><td>A.2.1.</td><td>Fixed-Area States with Two Minimal Surfaces</td><td>2185</td></tr><tr><td>A.2.2.</td><td>General States at the Minimal Surface Phase Transition</td><td>2186</td></tr><tr><td>A.3.</td><td>Replica Wormholes and JT Gravity</td><td>2188</td></tr><tr><td>A.3.1.</td><td>A Recursion Relation for the Resolvent</td><td>2191</td></tr><tr><td>B.</td><td>Random Tensor Network States and Split Transfer Protocols</td><td>2191</td></tr><tr><td>B.1.</td><td>Split Transfer and Recovery in Holography</td><td>2194</td></tr><tr><td>C.</td><td>Joint Smoothing of Link States</td><td>2195</td></tr><tr><td>D.</td><td>A Family of Metrics on the Symmetric Group</td><td>2205</td></tr><tr><td colspan="2">References</td><td>2207</td></tr></tbody></table>

# 1. Introduction

More than twenty years after its discovery, the AdS/CFT correspondence [49] remains the only known example of a theory of quantum gravity.<fnref n="1" /> A crucial feature of this correspondence is that the emergence of a (classical) spacetime is closely related to the entanglement structure of the boundary theory. Tensor networks appear to provide useful toy models for this aspect of AdS/CFT, mirroring many of its expected properties in a setting that can be made completely mathematically rigorous [40, 61, 70, 71]. A particularly powerful model is given

<footnote n="1">¹Here, we are requiring any putative theory of quantum gravity to (a) be defined non-perturbatively and (b) have strong evidence for the existence of a semiclassical limit consisting of Einstein gravity coupled to quantum field theory.</footnote>
by random tensor networks, which have the advantage of being highly analytically tractable, while exhibiting remarkably precise agreement with gravitational calculations (even including certain exponentially small corrections) [29, 40, 42, 60, 62–64, 80]. Random tensors and tensor networks also arise in a number of other fields of physics, including quantum information, where they have been used to explore generic entanglement properties of quantum states [2, 5, 9–11, 17, 18, 20–22, 37, 39, 46, 50, 57, 79] and condensed matter physics, e.g., in the study of random circuits and measurements [44, 47, 48, 53, 55, 77, 81, 82].

The most basic version of a random tensor network is characterized by a choice of bond dimension $D$ and a graph $G = (V, E)$, where the vertices $V = V_b \sqcup V_\partial$ of $G$ are partitioned into “bulk” vertices $V_b$ and “boundary” vertices $V_\partial$. To each edge $e \in E$, we associate a maximally entangled state

$$ \frac{1}{\sqrt{D}} \sum_{i=1}^{D} |ii\rangle \qquad (1.1) $$

on two $D$-dimensional Hilbert spaces, one of which is associated with each endpoint of $e$; each vertex $v \in V$ is therefore associated with a Hilbert space $\mathcal{H}_v$ of dimension $D^{\deg(v)}$. Finally, we project each bulk vertex $v_b \in V_b$ onto a Haar random state $|\psi_{v_b}\rangle \in \mathcal{H}_{v_b}$. The resulting “random tensor network state” lives in the Hilbert space $\mathcal{H}_\partial = \otimes_{v_\partial} \mathcal{H}_{v_\partial}$ associated with the boundary vertices $v_\partial \in V_\partial$, as shown in Fig. 1. Such states, obtained by projecting maximally entangled edge states onto (not necessarily random) bulk vertex states, are also known as projected entangled pair states (PEPS) in the condensed matter literature [23, 75, 76].

To characterize the typical entanglement structure of random tensor network states, we can compute the von Neumann entropy $H(\rho_A)$ of the reduced density matrix $\rho_A$ on a subset $A \subset V_\partial$ of the boundary vertices. In the limit where the bond dimension $D$ is very large, this entropy can be shown to converge with high probability to $\log(D)|\gamma_A|$, where $\gamma_A$ is the set of edges

<figure><img src="image_5.png" /><figcaption>(a) The skeleton of a random tensor network. We take the green-colored vertices to be the boundary vertices $V_\partial$ and the remaining, orange-colored vertices to be the bulk vertices $V_b$. We use this network for illustration throughout the remainder of this paper.</figcaption></figure>

<figure><img src="image_6.png" /><figcaption>(b) A close-up picture of a random tensor network. We first associate each vertex $v \in V$ with a Hilbert space $\mathcal{H}_v$ of dimension $D^{\deg(v)}$ (here, $\deg(v) = 3$). Then maximally entangled states are distributed according to the graph’s edges, after which the state at each bulk vertex $v_b \in V_b$ is projected onto a Haar random state $|\psi_{v_b}\rangle \in \mathcal{H}_v$.</figcaption></figure>

<caption>FIGURE 1. The basic structure of a random tensor network</caption>
crossing the minimal cut (for the moment, assumed to be the unique such cut) in the graph separating A from its boundary complement $V_\partial\setminus A$ (see Fig. 2a). This formula is closely analogous to the Ryu-Takayanagi (RT) formula and its generalizations in AdS/CFT, in which entropies are given by the area of minimal surfaces homologous to a subregion of the conformal boundary [32, 33, 41, 45, 65, 66]. Indeed, this connection is one of the primary reasons for studying tensor networks as a toy model of quantum gravity. However, if one goes beyond the von Neumann entropy and studies finer details of the entanglement spectrum of random tensor network states, significant divergences from holography begin to appear, as we will see shortly.

When studying entanglement in either random tensor networks or quantum gravity, or more generally in quantum field theory, it is often convenient to study $k$th Rényi entropies $H_k(\rho_A) = (1-k)^{-1} \log \text{tr}[\rho_A^k]$. For integer $k > 1$, these are more amenable to direct computation than the von Neumann entropy, and one can extract the von Neumann entropy by analytic continuation to $k=1$. The computation of Rényi entropies in random tensor network models is very similar to holographic computations. In both cases, the idea is to use the *replica trick*—essentially, this is the observation that $\text{tr}[\rho_A^k] = \text{tr}[\tau \rho_A^{\otimes k}]$ where $\tau$ is an operator which permutes the $k$ copies of $A$ cyclically. In the holographic computation, this can be written as a path integral, on $k$ copies of the theory, glued together in an appropriate way. By the holographic dictionary, this path integral can then be computed by the action of a bulk geometry with certain boundary conditions [45]. For random tensor networks, one finds that $\text{tr}[\rho_A^k]$ concentrates around its expectation and can be computed as the partition function of a classical spin model on the bulk vertices, with boundary conditions dictated by the choice of boundary subsystem [40]. This computation will be explained in detail in Sect. 2.1. From these computations, one finds that holographic CFT states and random tensor network states behave quite differently when $k \neq 1$. For random tensor network states, the Rényi entropies are approximately independent of $k$ in the large $D$ limit, meaning their entanglement spectrum is close to “flat”; the boundary state $\rho_A$ is approximately maximally mixed within a certain subspace. On the other hand, CFT states that are dual to semiclassical spacetime geometries have Rényi entropies that vary non-trivially with $k$, meaning their entanglement spectrum contains a wide range of eigenvalues that contribute significantly to the state. Recently, it has been argued that the class of “fixed-area states” in AdS/CFT do have flat spectra and more generally have an entanglement structure that closely matches random tensor network states [8, 14, 27, 29, 54]. Fixed-area states have a well-defined semiclassical geometry associated with a fixed spatial slice; however, thanks to the uncertainty principle, they cannot describe a single semiclassical spacetime geometry [14]. We discuss the connection between these states and random tensor networks in more detail in “Appendix A.”

In the random tensor network model, the flatness of the spectrum can be traced to the maximally entangled states used as “link states” (see Eq. (1.1) and Fig. 1b) on the edges of the graph, which themselves have flat entanglement spectra. To take results about random tensor networks beyond
the fixed-area state regime, it is natural—see, e.g., discussion in [14,40]—to replace the maximally entangled link states by general states

$$|\phi_e\rangle = \sum_{i=1}^{D} \sqrt{\lambda_{e,i}} |ii\rangle. \qquad (1.2)$$

The variation in the entanglement spectrum $\lambda_{e,i}$ represents the fluctuations in area in semiclassical gravitational states. We introduce this model in Sect. 2. The goal of this paper will be to understand the entanglement spectra of random tensor networks with such non-trivial link states and spectra in a number of different regimes. In fact, a number of our results apply in an even more general setting, where the product of link states $\otimes_e|\phi_e\rangle$ is replaced by a completely general “background state” density matrix $\phi_V$. From a quantum gravity perspective, random tensor networks with general background states are needed to model bulk quantum fields in AdS/CFT, which yield significant physical consequences when the bulk entropies are large [6,7]. Beyond holography, they also play a central role in the quantum information processing tasks of multiparty state merging split transfer [26], a connection we elaborate on in “Appendix B.”

If one considers a random tensor network with non-trivial link states, if there is a single minimal cut $\gamma_A$ for a subsystem A, then the resulting density matrix $\rho_A$ will have an entanglement spectrum that converges to that of $|\gamma_A|$ copies of the link state along the minimal cut as $D \to \infty$; indeed, this was implicit in [40]. A more complex question, and the main focus of this work, is the case where there are two minimal cuts, as in Fig. 2b. This situation is motivated by questions in holography: It can be used to study the phase transition at the point where there are two competing minimal surfaces [6,54], which has been relevant to recent advances on the black hole information paradox [1,4,51,59,60].

For our first main result, in Sect. 3, we consider a family of link states with increasing bond dimension D as in Eq. (1.2). For each D, the link state has an associated distribution

$$\mu_e^{(D)} = \frac{1}{D} \sum_{i=1}^{D} \delta_{D\lambda_{e,i}},$$

where $\delta_x$ is a $\delta$-distribution centered at $x$, so this is the discrete probability distribution given by a uniform distribution over the spectrum of the link state. Note that $\lambda_{e,i} = \lambda_{e,i}^{(D)}$ also depends on D. We then require that the moments

$$m_k^{(D)} = D^{k-1} \sum_{i=1}^{D} \lambda_{e,i}^k$$

of the distributions $\mu_e^{(D)}$ converge to a finite limit as $D \to \infty$ for all positive integer $k$. We refer to this as the bounded spectral variation limit. This means, in particular, that we must have $\lambda_{e,i} = O(1/D)$ for all but a vanishing fraction of the eigenvalues $\lambda_{e,i}$. If we let $\gamma_A$ denote a minimal cut for a boundary
<figure><img src="image_7.png" /><figcaption>FIGURE 2. Tensor networks with one and two minimal cuts</figcaption></figure>

domain A, then we may similarly define the associated distribution

$$ \mu_{\gamma_A}^{(D)} = \frac{1}{D^{|\gamma_A|}} \sum_{\{i_e\}_{e \in \gamma_A}} \delta_{D^{|\gamma_A|}} \prod_{e \in \gamma_A} \lambda_{e, i_e}. $$

By assumption, the moments of the distribution $\mu_{\gamma_A}^{(D)}$ converge to a finite limit (because those of each distribution $\mu_e^{(D)}$ do), implying that $\mu_{\gamma_A}^{(D)}$ converges weakly to some distribution $\mu_{\gamma_A}$. Now, consider the empirical distribution of the spectrum of reduced state $\rho_A$, which is the (random) distribution

$$ \mu_A^{(D)} = \frac{1}{D^{|\gamma_A|}} \sum_{\lambda \in \text{spec}(\rho_A)} \delta_{D^{|\gamma_A|} \lambda}. $$

In the case where there are two non-intersecting minimal cuts $\gamma_{A,1}$ and $\gamma_{A,2}$, we find that $\mu_A^{(D)}$ converges weakly, in probability, to a limiting distribution $\mu_A$ given by a free product MP(1) $\boxtimes \mu_{\gamma_{A,1}} \boxtimes \mu_{\gamma_{A,2}}$, a notion from the theory of free probability. Here, MP(1) is the Marchenko-Pastur distribution of parameter 1. The situation is summarized by our first main result, which we state more precisely as Theorem 3.4:

**Theorem (Informal).** Consider a family of link states in the bounded spectral variation limit. If there is a unique minimal cut $\gamma_A$ for a boundary subsystem A, then $\mu_A^{(D)}$ converges weakly, in probability, to $\mu_{\gamma_A}$, while if there are exactly two non-intersecting minimal cuts $\gamma_{A,1}$ and $\gamma_{A,2}$, it converges to MP(1) $\boxtimes \mu_{\gamma_{A,1}} \boxtimes \mu_{\gamma_{A,2}}$.

In Sect. 3.3, we briefly discuss the closely related problem of computing the entanglement negativity spectrum in the same regime.
For our second main result, in Sect. 4, we investigate a different regime, in which link states are allowed to have *unbounded spectral variation* in the large *D* limit. This is the more relevant regime for holography, where fluctuations in the area of a surface (in Planck units) grow sublinearly but without bound in the semiclassical limit. When the spectral variation is unbounded, there still exists a reasonable notion of a minimal cut that determines the entanglement spectrum of the boundary state, but the key difference is that minimality must now be defined entropically, rather than geometrically. In fact, the underlying graph essentially plays no role in this regime. A sensible way to formalize this would be to use one-shot entropies: We might say that a cut is “minimal” if the rank of the state along the cut is smaller than the inverse of the largest element in the entanglement spectrum along any other cut. This condition, while intuitive, is a little too restrictive, and one can use smooth conditional entropies to get a weaker, but still meaningful, condition. In Definition 4.6, following [6] we introduce the notion of a *unique* $(\epsilon, K)$-minimal cut $\Gamma_A$, where $\Gamma_A \subseteq V$ is a subset of vertices such that the $\epsilon$-smooth conditional min-entropy of $\Gamma_A$ compared to competing cuts either contained in $\Gamma_A$ or containing $\Gamma_A$ is lower bounded by $K$. Intuitively, we want $K$ to be as large as possible, and indeed, we show in Theorem 4.7 that the spectrum of a reduced density matrix $\rho_A$ will be close to the spectrum along a unique $(\epsilon, K)$-minimal cut with an error exponentially small in $K$.

The situation is more complicated if there are two non-intersecting $(\epsilon, K)$-minimal cuts, defined in Definition 4.10 as both cuts satisfying an $(\epsilon, K)$-minimality property for the same $\epsilon$ and $K$. Here, we need to impose a regularity condition on the link states, motivated by the example of a link state that is a (large) number of copies of a fixed state:

$$|\phi_e\rangle = |\phi_0\rangle^{\otimes n} \qquad (1.3)$$

where $|\phi_0\rangle$ is a bipartite state with local dimension $d$, so the total bond dimension is $D = d^n$. In this case, if $\phi_0$ is not maximally entangled, the measure $\mu_e^{(D)}$ will not converge with increasing $n$ as the spectrum is not concentrated around $1/D$. However, using a different measure, the entanglement spectrum of $|\phi_e\rangle$ satisfies a central limit theorem. Namely, if $|\phi_e\rangle$ has Schmidt coefficients $\{\lambda_i\}$, and $|\phi_0\rangle$ has entanglement entropy $H_0$, then the distribution of the random variable $X^{(n)}$ which takes values $\frac{1}{\sqrt{n}}(\log(\frac{1}{\lambda_i}) - nH_0)$ with probability $\lambda_i$, converges weakly to a centered Gaussian distribution as $n \to \infty$. Since we subtracted the entropy $nH_0$, the random variable $X^{(n)}$ has expectation zero. Its variance can be thought of as a measure of the fluctuation of $\log(\frac{1}{\lambda_i})$ around the entropy and is relevant for second-order asymptotic rates in quantum information processing tasks [72]. We take this central limit theorem as motivation for a regularity condition on the spectra of general link and background states, and we allow the states to have varying bond dimensions $D(n)$, e.g., $D(n) \sim d^n$. To be more precise, we define the following measure
along a cut $\gamma_A$:

$$ \nu_{\gamma_A}^{(n)} = \sum_{\{i_e\}_{e \in \gamma_A}} \prod_{e \in \gamma_A} \lambda_{e,i_e} \delta_{\frac{1}{\sqrt{n}}(\sum_{e \in \gamma_A} \log \frac{1}{\lambda_{e,i_e}} - H(n))}, $$

where $H(n)$ is a function of $n$ (which one can think of as being approximately equal to the entanglement entropy along the cut $\gamma_A$), and we assume that $\nu_{\gamma_A}^{(n)}$ converges weakly to a continuous distribution. Note that the distribution described above reduces to the distribution of $X^{(n)}$ if the link state is of the form in Eq. (1.3) and is very different from the distribution $\mu_A^{(D)}$, we study for link states with bounded spectral variation. Similarly, we let

$$ \nu_A^{(n)} = \sum_{\lambda \in \text{spec}(\rho_A)} \lambda \delta_{\frac{1}{\sqrt{n}}(\log(\frac{1}{\lambda}) - H(n))} $$

be the corresponding (random) distribution for the boundary spectrum. Knowledge of this distribution allows computation of the entropy of $\rho_A$ (and fluctuations) as a correction to $H(n)$. In the random tensor network setting, we find that in a situation with two competing minimal cuts, the random tensor network will 'select' the minimal parts of each cut, in the following sense:

**Theorem (Informal).** Assume that we have a family of (states with) two non-intersecting $(\varepsilon(n), K(n))$-minimal cuts $\gamma_{A,1}$ and $\gamma_{A,2}$, as defined in Definition 4.10. Suppose the entanglement spectra along the two minimal cuts are such that $\nu_{\gamma_{A,1}}^{(n)}$ and $\nu_{\gamma_{A,2}}^{(n)}$ converge weakly to continuous measures $\nu_1$ and $\nu_2$, respectively, as $n \to \infty$. Then, $\nu_A^{(n)}$ converges weakly, in probability, to $\min_*(\nu_1, \nu_2)$ which is the pushforward of $\nu_1$ and $\nu_2$ along the function $\min: \mathbb{R} \times \mathbb{R} \to \mathbb{R}$. In other words, for any bounded continuous function $f \in C_b(\mathbb{R})$

$$ \sum_{\lambda \in \text{spec}(\rho_A)} \lambda f \left( \frac{\log(\frac{1}{\lambda}) - H(n)}{\sqrt{n}} \right) \to \iint f(\min(x_1, x_2)) \, d\nu_1(x_1) d\nu_2(x_2) \quad (1.4) $$

in probability.

We also show in Corollary 4.14 that, up to an error of size $O(\log(n))$, this allows us to compute the entropy of $\rho_A$.

An analogous statement to (1.4) was previously conjectured in [54] to be valid in quantum gravity and justified at a physics level of rigor in [6]. Our proof of (1.4) is closely related to the arguments in [6], but converting the physical arguments into a mathematical proof and careful controlling the relevant sources of error requires significant technical work, and constitutes the majority of Sect. 4.

In “Appendix A,” we relate our results to the study of holographic gravity computations, particularly in situations with competing minimal surfaces. This is not needed to understand the results of this work, but provides additional motivation for the relevance of our results and clarifies the way in which random tensor networks provide a useful toy model for holographic quantum gravity. Then, in “Appendix B,” we discuss the relation of our results to split
transfer and its relevance in holography. This is again not needed to understand the main text, but rather pointing at topics our work is connected to. Next, in “Appendix C,” we prove two technical lemmas on joint smoothing that are necessary to analyze competing minimal cuts in the unbounded spectral variation regime. Finally, in “Appendix D,” we prove that a certain function on the symmetric group is a metric; this is not directly used in the current work, but may be of independent interest for the study of random tensor networks.

After the completion of this manuscript, we became aware of independent work by Jinzhao Wang [78] on the use of free products to describe entanglement in the toy model of quantum gravity introduced in [60] that has strong overlap with the ideas in Sect. 3.2 and “Appendix A.”

## 1.1. Notation and Conventions

For $k \in \mathbb{N}$, we let $[k] = \{1, \dots, k\}$, and we denote by $S_k$ the group of permutations of this set. We denote by $\|a\|_p$ the $l_p$-norm of a vector $a$, defined by $\|a\|_p = \sum_i |a_i|^p$. If $a$ and $b$ are vectors of different dimension, we extend the shorter vector by zeros and still write $\|a - b\|_p$ for their distance. For example, if $a \in \mathbb{C}^{d_1}$ and $b \in \mathbb{C}^{d_2}$ with $d_2 > d_1$, we write $\|a - b\|_1 = \sum_{i=1}^{d_1} |a_i - b_i| + \sum_{i=d_1+1}^{d_2} |b_i|$. We also denote by $\|A\|_p$ the Schatten $p$-norm of an operator $A$, defined as the $l_p$-norm of the singular values $\{s_i\}$ of $A$; it can also be computed by $\|A\|_p = \text{tr}((A^\dagger A)^{p/2})$. The operator norm is given by $\|A\|_\infty = \max\{s_i\}$. If $\mathcal{H}$ is a Hilbert space, we introduce the notation $\mathcal{P}(\mathcal{H})$ for the set of positive semidefinite operators on $\mathcal{H}$. We often refer to positive semidefinite operators as “density operators” or “states,” without requiring them to be normalized to unit trace. We write $\mathcal{P}_-(\mathcal{H})$ for the set of $\rho \in \mathcal{P}(\mathcal{H})$ with unit trace, $\text{tr}[\rho] = 1$, and we denote by $\mathcal{P}_-(\mathcal{H})$ the set of subnormalized states, that is, $\rho \in \mathcal{P}(\mathcal{H})$ with $\text{tr}[\rho] \le 1$. We use the convention that for a vector $|\phi\rangle$, we denote the corresponding pure state by $\phi$, so $\phi = |\phi\rangle\langle\phi|$. Given a positive semidefinite operator $\rho$, we denote by $\text{spec}(\rho)$ the vector containing its spectrum in non-increasing order, and we write $\text{spec}_+(\rho)$ for the nonzero part of the spectrum. It is a well-known fact that

$$ \|\text{spec}(\rho) - \text{spec}(\sigma)\|_1 = \|\text{spec}_+(\rho) - \text{spec}_+(\sigma)\|_1 \le \|\rho - \sigma\|_1 \quad (1.5) $$

(In the second expression, we use the convention for the distance of vectors of possibly different dimension introduced above.) If $A$ is a quantum system with Hilbert space $\mathcal{H}_A$, we write $\mathcal{P}(A) = \mathcal{P}(\mathcal{H}_A)$, $\mathcal{P}_-(A) = \mathcal{P}_-(\mathcal{H}_A)$, and $\mathcal{P}_-(A) = \mathcal{P}_-(\mathcal{H}_A)$, and we use subscripts, e.g., $\rho_A \in \mathcal{P}(A)$, to indicate which system and Hilbert space a quantum state is associated with. For a bipartite state $\rho_{AB} \in \mathcal{P}(AB)$ defined on a tensor product of Hilbert spaces $\mathcal{H}_{AB} = \mathcal{H}_A \otimes \mathcal{H}_B$, we obtain the reduced state or reduced density operator $\rho_A \in \mathcal{P}(A)$ by taking the partial trace over the complement: $\rho_A = \text{tr}_B[\rho_{AB}]$, and similarly in multipartite situations. Finally, we adopt the standard notation that if $\mu_n$ is some sequence of finite measures, we write $\mu_n \Rightarrow \mu$ if $\mu_n$ converges weakly (or in distribution) to a finite measure $\mu$, meaning that for any bounded continuous
function $f \in C_b(\mathbb{R})$,

$$ \int f(x)d\mu_n(x) \rightarrow \int f(x)d\mu(x). \qquad (1.6) $$

If $\mu_n$ is a sequence of random finite measures on $\mathbb{R}$, we say that the sequence $\mu_n$ converges weakly, in probability, to a finite measure $\mu$, if, for any bounded continuous function $f \in C_b(\mathbb{R})$, Eq. (1.6) converges in probability, i.e., if for every $\varepsilon > 0$ we have that

$$ \lim_{n \to \infty} \mathrm{Pr} \left( \left| \int f(x)d\mu_n(x) - \int f(x)d\mu(x) \right| \ge \varepsilon \right) = 0. $$

In this situation, we will also write $\mu_n \Rightarrow \mu$, in probability. All logarithms are to base 2.

## 2. Random Tensor Network States

We first review the random tensor network model, closely following [29, 40]. Let $G = (V, E)$ be a connected undirected graph, and let $V = V_\partial \sqcup V_b$ be a partition of the vertices into a set of boundary vertices $V_\partial$ and bulk vertices $V_b$. If $A \subseteq V_\partial$, we write $\bar{A} = V_\partial \setminus A$. We assign a bond dimension $D_e$ to each edge, and we will consider families of states with increasing bond dimensions; for example, we may take $D_e = D$ for all edges and let $D$ increase. For each vertex $x \in V$, let $\partial\{x\}$ denote the set of edges $e = (xy) \in E$ connecting $x$ to some $y \in V$. We define Hilbert spaces $\mathcal{H}_{e,x} = \mathbb{C}^{D_e}$ for $e \in \partial\{x\}$, and $\mathcal{H}_x := \bigotimes_{e \in \partial\{x\}} \mathcal{H}_{e,x}$. We call the pair $(e, x)$ a half-edge. Moreover, we write $\mathcal{H}_e = \mathcal{H}_{e,x} \otimes \mathcal{H}_{e,y}$ for an edge $e = (xy) \in E$. Let $D_x = \dim(\mathcal{H}_x)$. For a subset $A \subseteq V$, we write $\mathcal{H}_A = \bigotimes_{x \in A} \mathcal{H}_x$, and similarly, for a subset $S \subseteq E$ we write $\mathcal{H}_S = \bigotimes_{e \in S} \mathcal{H}_e$. Similarly, for a set $T$ of half-edges we write $\mathcal{H}_T = \bigotimes_{(e,x) \in T} \mathcal{H}_{e,x}$. At each edge $e = (xy) \in E$, we place a pure state $|\phi_e\rangle \in \mathcal{P}_-(\mathcal{H}_e)$

$$ |\phi_e\rangle = \sum_{i=1}^{D_e} \sqrt{\lambda_{e,i}} |ii\rangle \in \mathcal{H}_e = \mathcal{H}_{e,x} \otimes \mathcal{H}_{e,y}, \qquad (2.1) $$

that we call a link state. Then, $\phi_{e,x} = \phi_{e,y} = \sum_{i=1}^D \lambda_{e,i} |i\rangle\langle i|$ is the reduced density matrix of the link state on either of the two subsystems. We refer to the vector spec($\phi_{e,x}$) = spec($\phi_{e,y}$), which is ordered in non-increasing fashion, as the entanglement spectrum of $\phi_e$. Let $\phi \in \mathcal{P}_-(V)$ be the full state on edges given by the tensor product of link states

$$ |\phi\rangle = \bigotimes_{e \in E} |\phi_e\rangle. \qquad (2.2) $$

At every bulk vertex $x \in V_b$, we place a random vector $|\psi_x\rangle \in \mathcal{H}_x$, where the entries of $|\psi_x\rangle$ are independent standard (circularly symmetric) complex Gaussian random variables: Each entry of the tensor can be written as $\frac{1}{\sqrt{2}}(x + iy)$ where $x$ and $y$ are independent real Gaussian random variables of mean 0 and unit variance. We note that, in the model of [40], the tensors $|\psi_x\rangle$ were not chosen as random Gaussian vectors, but as uniformly random vectors on
the unit sphere. However, for our choice of Gaussian $|\psi_x\rangle$, the norm $|||\psi_x\rangle||$ is independent of the normalized vector $|\psi_x\rangle/|||\psi_x\rangle||$, and $|\psi_x\rangle/|||\psi_x\rangle||$ will be a uniformly random vectors on the unit sphere. Therefore, these two models only differ by their normalization. We write $|\psi\rangle = \bigotimes_{x \in V_b} |\psi_x\rangle$. The resulting random tensor network state $\rho \in \mathcal{P}(V_\partial)$ is defined by

$$|\rho\rangle = (I_{V_\partial} \otimes \langle\psi|)|\phi\rangle. \qquad (2.3)$$

The random tensor network state is obtained by projecting the link states onto random vectors, so that the final state lives in the boundary Hilbert space. We can make this manifest by using the cyclicity of the trace to write the density matrix:

$$\rho = (I_{V_\partial} \otimes \langle\psi|) \phi (I_{V_\partial} \otimes |\psi\rangle) = \text{tr}_{V_b} [(I_{V_\partial} \otimes \psi) \phi]. \qquad (2.4)$$

Note that this state need not be normalized, but we chose the standard deviation of the $|\psi_x\rangle$ such that $\rho$ is normalized on average, given that the link state $\phi$ is normalized:

$$\mathbb{E} \text{tr}[\rho] = \text{tr}[\phi]. \qquad (2.5)$$

In Sect. 2.3.1, we prove the stronger statement that $\rho$ is normalized with high probability for appropriately connected tensor networks and large bond dimension. Note also, that in Eq. (2.1), we have chosen states which have a Schmidt decomposition in a fixed basis (the standard basis). Since we project onto uniformly random tensors, we can choose to do so without loss of generality.

## 2.1. The Replica Trick for Random Tensor Networks

We now consider a boundary subset $A \subseteq V_\partial$ and use the replica trick to study the Rényi entropies of the reduced density matrix $\rho_A$. The replica trick for random tensor network models was first studied in [40], and it is the key tool we apply throughout this work. Let $\mathcal{H}$ be a Hilbert space. The Rényi entropies of a (normalized) density matrix $\rho \in \mathcal{P}_-(\mathcal{H})$ are defined by

$$H_k(\rho) = \frac{1}{1-k} \log(\text{tr}[\rho^k])$$

for $k \in (0, 1) \cup (1, \infty)$. For $k = 0, 1, \infty$, there are well-defined limits, given by

$$\begin{align}
H_0(\rho) &:= \log(\text{rank}(\rho)) \nonumber \\
H_1(\rho) &:= -\text{tr}[\rho \log(\rho)] \tag{2.6} \\
H_\infty &:= -\log(\|\rho\|_\infty). \nonumber
\end{align}$$

In particular, we see that $H(\rho) = H_1(\rho)$ is the von Neumann entropy. We will also write $H(A)_\rho := H(\rho_A)$ and $H_k(A)_\rho := H_k(\rho_A)$ for reduced density matrices. If $\rho \in \mathcal{P}_-(\mathcal{H})$ is subnormalized, we let

$$H_k(\rho) = \frac{1}{1-k} \log \frac{\text{tr}[\rho^k]}{\text{tr}[\rho]}. \qquad (2.7)$$
Denote by $R$ the representation of $S_k$ on $\mathcal{H}^{\otimes k}$ which permutes the $k$ copies of $\mathcal{H}$ according to the action of $S_k$. We will write $R_x(\pi)$ when $\mathcal{H} = \mathcal{H}_x$ and $R_A(\pi)$ if $\mathcal{H} = \mathcal{H}_A$ for $A \subseteq V$. We let $\tau$ denote the standard $k$-cycle in $S_k$, i.e.,

$$ \tau = (12\dots k). $$

The key idea of the replica trick is the observation that the $k$th moment of $\rho \in \mathcal{P}(\mathcal{H})$ can be written as

$$ \mathrm{tr} [\rho^k] = \mathrm{tr} [R(\tau) \rho^{\otimes k}]. \qquad (2.8) $$

Recall the notion of the cycle type of a permutation $\pi$: If $\pi$ can be written as a product of $m$ disjoint cycles of lengths $l_1, \dots, l_m$, then $\pi$ has cycle type $C(\pi) = \{l_1, \dots, l_m\}$. Then, for an arbitrary $\pi \in S_k$,

$$ \mathrm{tr} [R(\pi) \rho^{\otimes k}] = \prod_{l \in C(\pi)} \mathrm{tr} [\rho^l]. $$

Note that this is the generalization of the well-known swap trick for two copies of a state $\rho$. The other crucial ingredient is a property of the Gaussian random vectors:

$$ \mathbb{E}[\psi_x^{\otimes k}] = \sum_{\pi \in S_k} R_x(\pi). \qquad (2.9) $$

Using Eq. (2.4), we may then compute

$$ \begin{aligned} \mathbb{E} \mathrm{tr} [\rho_A^k] &= \mathbb{E} \mathrm{tr} [R_A(\tau) \rho_A^{\otimes k}] \\ &= \mathbb{E} \mathrm{tr} [((R_A(\tau) \otimes R_{V_\partial \setminus A}(\mathrm{id})) \rho^{\otimes k})] \\ &= \mathbb{E} \mathrm{tr} [((R_A(\tau) \otimes R_{V_\partial \setminus A}(\mathrm{id})) (I_{V_\partial} \otimes \psi)^{\otimes k}) \phi^{\otimes k}] \\ &= \mathrm{tr} [((R_A(\tau) \otimes R_{V \setminus A}(\mathrm{id})) \mathbb{E} [(I_{V_\partial} \otimes \psi)^{\otimes k}] \phi^{\otimes k}]. \end{aligned} \qquad (2.10) $$

To further simplify this expression, we define the following set:

$$ S_{A,\sigma} = \{\{\pi_x\}_{x \in V} : \pi_x \in S_k, \text{ where } \pi_x = \sigma \text{ for } x \in A \text{ and } \pi_x = \mathrm{id} \text{ for } x \in \bar{A}\}, \qquad (2.11) $$

for any $\sigma \in S_k$ and $A \subseteq V_\partial$. An element of $S_{A,\sigma}$ assigns a permutation to each vertex in $V$ subject to a “boundary condition.” Now, using Eq. (2.9), we find that

$$ \mathbb{E} \mathrm{tr} [\rho_A^k] = \sum_{\{\pi_x\} \in S_{A,\tau}} \mathrm{tr} \left[ \bigotimes_{x \in V} R_x(\pi_x) \phi^{\otimes k} \right]. $$

Finally, we observe that for $e = (xy)$

$$ \mathrm{tr} [R(\pi_x) \otimes R(\pi_y) \phi^{\otimes k}] = \prod_{l \in C(\pi_x^{-1} \pi_y)} \mathrm{tr} [\phi_{e,x}^l], $$

where we recall that $\phi_{e,x}$ is the reduced density matrix of the link state on edge $e = (xy)$. Thus, we conclude that

$$ \mathbb{E} \mathrm{tr} [\rho_A^k] = \sum_{\{\pi_x\} \in S_{A,\tau}} \prod_{e=(xy) \in E} \prod_{l \in C(\pi_x^{-1} \pi_y)} \mathrm{tr} [\phi_{e,x}^l]. \qquad (2.12) $$
We can interpret the expectation as the partition function of a classical spin model

$$ \mathbb{E} \operatorname{tr} [\rho_A^k] = \sum_{\{\pi_x\} \in S_{A, \tau}} 2^{-\sum_{e=(xy) \in E} J_e(\pi_x, \pi_y)}, \quad (2.13) $$

where the site variables in the spin model are permutations $\pi_x \in S_k$, and the interaction at the edges between sites is given by

$$ J_e(\pi_x, \pi_y) = - \sum_{l \in C(\pi_x^{-1} \pi_y)} \log(\operatorname{tr}[\phi_{e,x}^l]) = \sum_{l \in C(\pi_x^{-1} \pi_y)} (l-1) H_l(\phi_{e,x}), $$

with $H_l$ being the $l$th Rényi entropy, and the model as boundary conditions such that the permutation must be $\tau$ on $A$ and id on $\bar{A}$. It turns out that $J_e$ is a metric on the symmetric group $S_k$—see “Appendix D.” Similarly, we may place an arbitrary permutation $\pi$ on $A$ instead of $\tau$, which yields (by exactly the same reasoning)

$$ \mathbb{E} \operatorname{tr} [R(\pi) \rho^{\otimes k}] = \sum_{\{\pi_x\} \in S_{A, \pi}} \prod_{e=(xy) \in E} \prod_{l \in C(\pi_x^{-1} \pi_y)} \operatorname{tr} [\phi_{e,x}^l]. \quad (2.14) $$

## 2.2. Maximally Entangled Link States and Minimal Cuts

We will now discuss the special case where all the link states are maximally entangled states of dimension $D$, which has been studied extensively in [40]. We will generalize the results we discuss here to a wider class of link states in Sect. 3. In this case, the entanglement spectra of the link states are flat: For $e \in E$, we have $\lambda_{e,i} = \frac{1}{D}$ for $i = 1, \dots, D$. In particular, for all $l \in \mathbb{N}$ we have $H_l(\phi_e) = \log(D)$ and hence

$$ J_e(\pi_x, \pi_y) = \log(D) \sum_{l \in C(\pi_x^{-1} \pi_y)} (l-1). $$

This leads to the so-called *Cayley distance* on $S_k$:

$$ d(\pi_x, \pi_y) = \sum_{l \in C(\pi_x^{-1} \pi_y)} (l-1) = k - |C(\pi_x^{-1} \pi_y)|, \quad (2.15) $$

where $|C(\pi)|$ is the number of cycles in $\pi$. Moreover, $d(\pi_x, \pi_y)$ is a metric and equals the minimal number of transpositions needed to transform $\pi_x$ into $\pi_y$. We say that $\pi \in S_k$ is on a geodesic between $\pi_1$ and $\pi_2$ if $d(\pi_1, \pi) + d(\pi, \pi_2) = d(\pi_1, \pi_2)$. (Recall that $d$ is a metric.) We can rewrite the spin model in terms of this distance:

$$ \mathbb{E} \operatorname{tr} [\rho_A^k] = \sum_{\{\pi_x\} \in S_{A, \sigma}} 2^{-\log(D) \sum_{e=(xy) \in E} d(\pi_x, \pi_y)}. \quad (2.16) $$

The physically inclined reader may observe that the logarithm of the bond dimension has the role of an inverse temperature, and for large $D$, the dominant contribution to the partition function will be the ground state of the spin model, subject to the relevant boundary conditions.

To describe the dominant contribution to the sum in Eq. (2.16) for large $D$, we need the *minimal cuts* for $A$ in $G$. A cut for $A$ is a subset of
the vertices $\Gamma_A \subset V$ such that $\Gamma_A \cap V_\partial = A$. Throughout this work, we will denote the set of all cuts for $A$ by $C(A)$. We will use the convention of denoting cuts (i.e., subsets of vertices) by capital Greek letters. Given a cut $\Gamma_A \in C(A)$, we will denote the set of edges crossing the cut, that is, edges connecting a vertex in $\Gamma_A$ with a vertex in $V \setminus \Gamma_A$, by lowercase Greek letters $\gamma_A$. (And by an abuse of language, also refer to this set as a “cut.”) A minimal cut for $A$ is a cut such that the number of edges $|\gamma_A|$ is minimal. We write $m(A) = |\gamma_A|$ for a minimal cut $\gamma_A \in C(A)$. If $\Gamma_A \in C(A)$, we write $\Gamma_A^c = V \setminus \Gamma_A$. Note that $\Gamma_A^c$ is a cut for $\bar{A} = V_\partial \setminus A$.

In the simplest case, there is a unique minimal cut $\gamma_A$. For this case, one can show that the dominant configuration is the one in which $\pi_x = \tau$ for $x \in \Gamma_A$ and $\pi_x = \text{id}$ for $x \in V \setminus \Gamma_A$, see [39], or Proposition 3.3. That is, there are two domains in the spin model corresponding to $\tau$ and id, and the minimization of the domain wall corresponds to the minimal cut in the graph.

We will also be interested in the case of exactly two non-intersecting minimal cuts $\Gamma_{A,1}$ and $\Gamma_{A,2}$. In this case, we have that $\Gamma_{A,1} \subset \Gamma_{A,2}$, or $\Gamma_{A,2} \subset \Gamma_{A,1}$. After relabeling, we may assume that the first is the case, and define three domains in the graph: $V = V_1 \sqcup V_2 \sqcup V_3$ given by $V_1 = \Gamma_{A,1}$, $V_2 = \Gamma_{A,2} \setminus \Gamma_{A,1}$ and $V \setminus \Gamma_{A,2}$. If there are exactly two minimal cuts, then multiple dominant configurations contribute equally to the partition function Eq. (2.16). These dominant configurations can be constructed as follows: For each $\pi$ on a geodesic between $\tau$ and id, set $\pi_x = \tau$ for $x \in V_1$, $\pi_x = \pi$ for $x \in V_2$ and $\pi_x = \text{id}$ for $x \in V_3$. That these are the dominant configurations follows immediately from the fact that $d(\tau, \pi) + d(\pi, \text{id}) \ge d(\tau, \text{id})$, with equality if and only if $\pi$ is on a geodesic between $\tau$ and id.

To understand this degeneracy, we use the following fact [56]: the set of permutations $\pi$ on a geodesic between $\tau$ and id is in a one-to-one correspondence with the set of non-crossing partitions $NC(k)$ of $[k]$. See Sect. 3.1 for a definition and properties of $NC(k)$. Thus, the degeneracy for the $k$th moment is $|NC(k)| = C_k$ where

$$C_k = \frac{1}{k+1} \binom{2k}{k}$$

is the $k$th Catalan number. These are the moments of the Marchenko-Pastur distribution MP($t$)

$$MP(t) = \max(1-t, 0)\delta_0 + \nu_t \\ d\nu_t(x) = \frac{\sqrt{4t - (x-1-t)^2}}{2\pi x} \mathbf{1}_{(x-1-t)^2 \le 4t} dx. \quad (2.17)$$

This allows one to show the folklore result (which we prove and extend to more general link states in Theorem 3.4) that upon an appropriate rescaling, the empirical distribution of the spectrum of $\rho_A$ converges to a Marchenko-Pastur distribution. This is in line with the case of a single random tensor, which precisely yields a Wishart matrix (see Sect. 3.1.1 for a brief introduction to these objects). In the first case, where there is a unique minimal cut, the
entanglement spectrum of $\rho_A$ is flat, while, as we have seen, in the second case, the degeneracy gives rise to a non-trivial spectrum in the right scaling limit.

## 2.3. The Replica Trick for General Background States

In Eq. (2.13), we computed the result of the replica trick for the kth moment for a random tensor network state. We will also consider the more general setting where the link state is replaced by some arbitrary state $\phi_V$. In this setting, there need not be a graph structure, and the Hilbert space at each vertex $x \in V$ can be some arbitrary Hilbert space, rather than a tensor product of Hilbert spaces labeled by half-edges. We will refer to $\phi_V$ as a “background state” instead of a “link state” (as the interpretation of links along the edges does not necessarily make sense in this situation). That is, where before we had a link state

$$|\phi\rangle = \bigotimes_{e \in E} |\phi_e\rangle,$$

we will now consider some arbitrary possibly mixed and subnormalized $\phi_V \in \mathcal{P}_{\le}(V)$ in the tensor network construction. We can generalize Eq. (2.4) to also apply for general background states to obtain a state $\rho \in \mathcal{P}(V_{\partial})$ given by

$$\rho = \text{tr}_{V_b} [(I_{V_{\partial}} \otimes \psi) \phi_V] \qquad (2.18)$$

where $|\psi\rangle$ is a tensor product of random states at the bulk vertices. If $\phi$ is pure, then so is $\rho$, since in that case

$$|\rho\rangle = (I_{V_{\partial}} \otimes \langle\psi|) |\phi\rangle.$$

If $\phi$ is not pure, we can consider a purification $\phi_{VR} \in \mathcal{P}_{\le}(VR)$ and consider $R$ as an additional boundary system; this leads to a random tensor network state $\rho_{V_{\partial}R}$ which is a purification of $\rho_{V_{\partial}}$. This setup is illustrated in Fig. 3, while formally very similar, the resulting state is no longer a PEPS tensor network state in general.

<figure><img src="image_8.png" /><figcaption>FIGURE 3. The structure of a (purified) random tensor network with a general background state</figcaption></figure>
There are multiple reasons to also allow general background states. The first reason is of a technical nature: They are useful for estimates based on smooth entropies, which we discuss in Sect. 4. In this application, the full state on edges is still pure, but is no longer a tensor product of link states along the edges. A second motivation for considering general background states is that they can be used as a toy model for holographic systems where there is “bulk entropy” present. Finally, these states are closely related to protocols for the quantum information processing task of split transfer [26]. We comment on this connection in “Appendix B.”

Even for a general background state, a version of the replica trick still applies. Consider a boundary subsystem $A \subseteq V_\partial$ with corresponding boundary state $\rho_A$. Then, the computation in Eq. (2.10) is still valid, and we find

$$ \mathbb{E} \operatorname{tr}[\rho_A^k] = \sum_{\{\pi_x\} \in S_{A,\tau}} \operatorname{tr}_V \left[ \bigotimes_{x \in V} R_x(\pi_x) \phi_V^{\otimes k} \right] \quad (2.19) $$

where $\tau = (12...k)$. However, Eq. (2.19) no longer has the interpretation of a spin model with local interactions.

For general background states, we will only need the replica trick for $k=2$. Since $S_2$ has only two elements, each configuration of permutations is completely characterized by the domain $\Delta_A = \{x \in V \text{ such that } \pi_x = \tau\}$. Because of the boundary conditions in $S_{A,\tau}$, the collection of these sets coincides with $C(A)$, and hence,

$$ \mathbb{E} \operatorname{tr}[\rho_A^2] = \sum_{\Delta_A \in C(A)} \operatorname{tr}[\phi_{\Delta_A}^2] = \sum_{\Delta_A \in C(A)} \operatorname{tr}[\phi] 2^{-H_2(\Delta_A)_\phi}. \quad (2.20) $$

Another useful fact is that by Eq. (2.9),

$$ \mathbb{E}\rho_{V_\partial} = \phi_{V_\partial}. \quad (2.21) $$

We remark that if one only uses the $k=2$ replica trick, one could also use tensors which are drawn from a projective 2-design, a distribution which produces tensors with the same first and second moments as uniformly random tensors of unit norm [35, 43]. An example of a projective 2-design is the set of uniformly random stabilizer states. For tensors $|\psi_x\rangle$ drawn from a projective 2-design of dimension $D_x$, it holds that

$$ \mathbb{E}\psi_x^{\otimes 2} = \frac{1}{D_x(D_x-1)} I + \frac{1}{D_x(D_x-1)} R_x(\tau), $$

and hence,

$$ \mathbb{E} \operatorname{tr}[\rho_A^2] = \frac{D_x}{D_x+1} \sum_{\Delta_A \in C(A)} \operatorname{tr}[\phi_{\Delta_A}^2], $$

which is close to Eq. (2.20) for large $D_x$. Thus, it is not hard to see that all random tensor network results which only use the $k=2$ replica trick are also valid for states with tensors drawn from projective 2-designs. This was already observed in [40], and random tensor networks with random stabilizer tensors were further studied in [57]. The results of Sect. 4 only use the $k=2$
replica trick and thus will extend to states with tensors drawn from projective 2-designs. This will not be true for the results in Sect. 3, which requires usage of the replica trick for all $k \in \mathbb{N}$.

**2.3.1. Normalization of Random Tensor Network States.** One immediate consequence of the replica trick for $k = 2$ is that the random tensor network state $\rho$ will be approximately normalized with high probability, so long as a mild condition on the background state is satisfied: The bulk needs to be connected, with sufficiently entangled edges. Let

$$ \eta = \max_{\Delta \subseteq V_b, \Delta \neq \emptyset} \mathrm{tr}[\phi_{\Delta}^2] = \max_{\Delta \subseteq V_b, \Delta \neq \emptyset} \mathrm{tr}[\phi] 2^{-H_2(\Delta)}_{\phi}. \quad (2.22) $$

If the state has enough correlations along each cut (or more precisely, if $H_2(\Delta)_{\phi}$ is large for each $\Delta$), then $\eta$ is small. Concretely, if we consider a random tensor network state with maximally entangled link states of bond dimension $D$, we will have $\eta \le \frac{1}{D}$. We then have

**Lemma 2.1.** For any background state $\phi \in \mathcal{P}_{\le}(V)$, with associated $\rho \in \mathcal{P}(V_{\partial})$ as in Eq. (2.18), it holds that for any $\varepsilon > 0$

$$ \mathrm{Pr}(|\mathrm{tr}[\rho] - \mathrm{tr}[\phi]| \ge \varepsilon) \le 2^{|V_b|} \frac{\eta}{\varepsilon^2} $$

where $\eta$ is defined in Eq. (2.22).

*Proof.* This follows from a special case of Eq. (2.20). In this case, the empty cut contributes $\mathrm{tr}[\phi]^2$, so we find

$$ \mathrm{Var}(\mathrm{tr}[\rho]) = \mathbb{E} |\mathrm{tr}[\rho] - \mathrm{tr}[\phi]|^2 = \mathbb{E} |\mathrm{tr}[\rho]|^2 - |\mathrm{tr}[\phi]|^2 \le 2^{V_b} \max_{\Delta \subseteq V_b, \Delta \neq \emptyset} \mathrm{tr}[\phi_{\Delta}^2], $$

where we have used the normalization of $\rho$ in expectation $\mathbb{E} \mathrm{tr}[\rho] = \mathrm{tr}[\phi]$, as in Eq. (2.5). The result follows by an application of Chebyshev's inequality. $\square$

We can improve this result by taking advantage of the fact that our random projectors are random Gaussian vectors, allowing us to use Gaussian concentration of measure rather than the Chebyshev's inequality. For instance, using a concentration bound for Gaussian polynomials (see [9], Corollary 5.49) one can show that for any $\varepsilon \ge (\sqrt{2e})^{2V_b}\eta$:

$$ \mathrm{Pr}(|\mathrm{tr}[\rho] - \mathrm{tr}[\phi]| \ge \varepsilon) \le \exp \left( - \frac{|V_b|}{2e} \varepsilon^{\frac{1}{|V_b|}} \eta^{-\frac{1}{|V_b|}} \right), $$

where $\eta$ is defined as in Eq. (2.22). We will not need this refinement.

## 3. Link States with Bounded Spectral Variation

In this section, we study random tensor network states with link states that have bounded spectral variation, meaning that there is an effective bond dimension $D$ such that the Schmidt coefficients of the link state are of the order $\frac{1}{D}$.

We start by providing background material on random matrix theory and free probability, which is a key tool in the study of products of random
matrices. In Sect. 3.2, we will precisely define the notion of bounded spectral variation and generalize the results in Sect. 2.2 for random tensor network states with maximally entangled link states to this wider class of link states. This leads to the main result of this section, Theorem 3.4, which shows that the asymptotic entanglement spectrum can be expressed in terms of a free product of distributions. We will see that the results are similar to the quantum gravity setup described in “Appendix A.3.” Finally, in Sect. 3.3, we investigate the entanglement negativity for random tensor network states with link states of bounded spectral variation.

## 3.1. Random Matrices, Free Probability, and Non-crossing Partitions

**3.1.1. Random Matrix Theory and Wishart Matrices.** We start by reviewing relevant concepts from probability and random matrix theory that are relevant for our analyses. This material can be found in any introduction to random matrix theory, e.g., [3, 15, 58].

A fundamental question in random matrix theory is as follows: Given a family of $n \times n$ matrices with entries selected according to some distribution, what is the asymptotic distribution of the eigenvalues as $n \to \infty$? This question has been extensively studied and in many cases has an elegant and concise answer. We discuss a basic example which is closely related to our purposes: *Wishart matrices*. Consider an $n \times m$ matrix $X$ whose entries are drawn i.i.d. from a Gaussian distribution with mean zero and unit variance. The sample covariance matrix of $X$ is the $n \times n$ matrix defined as

$$Y_{n,m} = \frac{1}{m}XX^T. \qquad (3.1)$$

Such random matrices are called (real) *Wishart matrices* and can be thought of as a sample second moment matrix (where one has $m$ realizations of an $n$-dimensional random variable). One can also consider *complex* Wishart matrices: In this case, the entries of the $n \times m$ matrix $X$ are complex i.i.d. standard (circularly symmetric) complex Gaussian random variables. We then let $Y_{n,m} = \frac{1}{m}XX^†$. We would like to understand the spectrum of $Y_{n,m}$, and to that end, we consider the empirical distribution of the eigenvalues. This empirical distribution is itself random, depending on the particular realization of $Y_{n,m}$. To characterize the convergence, we recall that if $\{\mu_n\}_{n \in \mathbb{N}}$ is a sequence of random finite measures on $\mathbb{R}$, we say that the sequence $\mu_n$ converges weakly, in probability, to a finite measure $\mu$, if, for any bounded continuous function $f \in C_b(\mathbb{R})$, it holds that for every $\varepsilon > 0$

$$\lim_{n \to \infty} \mathrm{Pr} \left( \left| \int f(x) \mathrm{d}\mu_n(x) - \int f(x) \mathrm{d}\mu(x) \right| \ge \varepsilon \right) = 0.$$

The asymptotic distribution of the eigenvalues of Wishart matrices is known to obey the *Marchenko-Pastur law* (see, for instance, Theorem 3.6 and Theorem 3.7 in [15]):
**Theorem 3.1.** Consider (real or complex) Wishart matrices $Y_{n,m}$, and let

$$ \mu_{n,m} = \frac{1}{n} \sum_{\lambda \in \text{spec}(Y_{n,m})} \delta_{\lambda} $$

be the empirical distribution of its eigenvalue spectrum. Suppose that the ratio of dimensions $n/m$ converges to a constant $t > 0$ as $n \to \infty$. Then, $\mu_{n,m}$ converges weakly, in probability, to the Marchenko-Pastur distribution MP(t) with parameter $t > 0$, as defined in Eq. (2.17).

Generalizations to this result are possible. For example, one still has convergence if the entries of $X$ are chosen according to non-Gaussian distributions with mean zero and unit variance. Also, one can prove weak convergence, almost surely (rather than just in probability); see [15].

If $Y_{n,m} = \frac{1}{m}XX^\dagger$ is a complex Wishart matrix, $X$ can also be interpreted as a uniformly random pure quantum state on $C^n \otimes C^m$, and $Y_{n,m}$, up to normalization, as the reduced density matrix on $C^n$ [39]. Note that $\frac{1}{n}Y_{n,m}$ is normalized in expectation in the sense that $\mathbb{E}\frac{1}{n}Y_{n,m} = 1$. So, complex Wishart matrices can be used as a model for the reduced state of a random bipartite quantum state, and this allows one to quantify the “typical entanglement” of a random state. Equivalently, in the tensor network setting, $\frac{1}{\sqrt{n}}X$ can be thought of as a random tensor network state with a single bulk vertex, two boundary vertices, and maximally entangled link states. We can then can interpret $\frac{1}{n}Y_{n,m}$ as the reduced density matrix on one of the boundary vertices. We will provide a generalization of Theorem 3.1 for the entanglement spectrum of random tensor network states in Theorem 3.4.

**3.1.2. Free Probability.** The topic of probability distributions in random matrix theory is closely related to free probability and, in particular, to the notion of the free product. We provide a brief introduction here; the material in this section is very standard, and we only review a few relevant aspects. For an extensive treatment, see, for instance, Chapter 5 in [3] or the books [52, 56, 58]. As we will see later, the free product will allow us to concisely formulate replica trick results involving multiple minimal cuts.

A non-commutative probability space is a pair $(\mathcal{A}, \omega)$, where $\mathcal{A}$ is a $C^*$-algebra and $\omega$ is a state on $\mathcal{A}$. An element $a \in \mathcal{A}$ is called a non-commutative random variable. The key example to have in mind is the space of $n \times n$ random matrices, where the matrix entries are distributed according to some probability distribution, and $\omega(a) = \mathbb{E}\frac{1}{n}\text{tr}[a]$ defines a tracial state. If $a \in \mathcal{A}$, the distribution (or law) $\mu_a$ of $a$ is defined as a map on polynomials, which evaluates on a polynomial $p$ as $\mu_a(p) = \omega(p(a))$. If $a$ is self-adjoint, it has real spectrum and we can extend the domain of $\mu_a$ to all bounded continuous functions $f \in C_b(\mathbb{R})$, using the functional calculus to define $f(a)$ and letting $\mu_a(f) = \omega(f(a))$. In this case, we can identify $\mu_a$ with a distribution such that, for $f \in C_b(\mathbb{R})$, we have $\mu_a(f) = \int f(x)d\mu_a(x)$. In particular, if $a$ is an $n \times n$ self-adjoint random matrix, then $\mu_a(f) = \frac{1}{n}\mathbb{E}\sum_{\lambda \in \text{spec}(a)} f(\lambda)$, and we may identify $\mu_a$ with the empirical measure of the eigenvalues of $a$. If $\mathcal{A}$ is a
commutative algebra, these notions reduce to the usual notions of probability theory, where $\omega$ is the expectation.

We call a set of $n$ non-commutative random variables $\{a_i\}$ on a non-commutative probability space $(\mathcal{A}, \omega)$ freely independent or just free if, for any set of $k \ge 2$ polynomials $\{p_j\}$, the variables satisfy

$$ \omega(p_1(a_{i_1}) \dots p_k(a_{i_k})) = 0 $$

whenever $\omega(p_m(a_{i_m})) = 0$ for all $1 \le m \le k$ and no two adjacent indices $i_m$ and $i_{m+1}$ for $1 \le m \le k-1$ are equal. One can see that two freely independent variables $a_1, a_2$ satisfy:

$$ 0 = \omega((a_1 - \omega(a_1))(a_2 - \omega(a_2))) = \omega(a_1 a_2) - \omega(a_1)\omega(a_2), \quad (3.2) $$

which, in the commutative case with random variables $x_1, x_2$, is the classical bivariate independence condition $\mathbb{E}[x_1x_2] = \mathbb{E}[x_1]\mathbb{E}[x_2]$. The definition of free independence does not specialize to independence in the commutative case. (Commuting independent random variables are only free when they are constant.) However, the role of free independence is analogous to the role of classical independence for commuting random variables: It allows one to, in principle, compute the joint mixed moments of the variables.

We will be interested in the multiplicative free convolution or free product (there also exists an additive convolution or just free convolution) of distributions. Suppose $a, b$ are non-commutative self-adjoint free random variables on $(\mathcal{A}, \omega)$ with distributions $\mu_a$ and $\mu_b$. Then, we denote the distribution of $ab$ by $\mu_{ab} = \mu_a \boxtimes \mu_b$. Note that, generally, $ab$ need not be self-adjoint. However, if $\omega$ is tracial (as in the random matrix case) and $a$ is positive, the distribution of $ab$ coincides with that of $\sqrt{ab}\sqrt{a}$ which is self-adjoint, and we can identify $\mu_{ab}$ with a distribution on $\mathbb{R}$. If $\mu_a$ and $\mu_b$ are compactly supported distributions, then so is $\mu_a \boxtimes \mu_b$.

As a concrete example of the freeness and the free product, let $X_n$ and $Y_n$ be two families of random $n \times n$ positive diagonal matrices with uniformly bounded norm, such that their spectrum converges weakly to probability distributions $\mu$ and $\nu$, respectively. Let $U_n$ be a family of Haar random unitary $n \times n$ matrices. Then, as $n$ goes to infinity, $X_n$ and $Y'_n = U_n Y_n U_n^\dagger$ will be freely independent (so they are asymptotically free), and we would like to study their product. The product of positive matrices need not be self-adjoint, so we consider $Z_n = \sqrt{X_n} Y'_n \sqrt{X_n}$ which is a positive matrix. One may then show that the distribution of the spectrum of $Z_n$ weakly converges in probability to $\mu \boxtimes \nu$. See Corollary 5.4.11 in [3] for a precise statement and proof.

The free product may be analyzed using generating functions: Given a (non-commutative) random variable $a$ with distribution $\mu_a$, let

$$ m_{a,k} = \int x^k d\mu_a(x) $$
be the kth moment of $\mu_a$. Then, the moment-generating function is the formal power series

$$M_{\mu_a}(z) = \sum_{k=1}^{\infty} m_{a,k} z^k. \qquad (3.3)$$

We define the S-transform to be the formal power series

$$S_{\mu_a}(z) = \frac{1+z}{z} M_a^{-1}(z),$$

where $M_a^{-1}(z)$ is the power series corresponding to the formal inverse of $M_\mu(z)$ under composition, which is well defined as long as $m_{a,1} \neq 0$. For compactly supported distributions, the moment-generating function, and hence the S-transform, uniquely determines the distribution.

If a and b are non-commutative self-adjoint free random variables, then

$$S_{\mu_a \boxtimes \mu_b}(z) = S_{\mu_a b}(z) = S_{\mu_a}(z)S_{\mu_b}(z). \qquad (3.4)$$

This also provides a completely combinatorial interpretation of the free product, without reference to the associated non-commutative probability spaces. That is, given compactly supported distributions $\mu$ and $\nu$, we can define $\mu \boxtimes \nu$ by Eq. (3.4): It is the compactly supported distribution with moments prescribed by $S_{\mu_a \boxtimes \mu_b}(z)$, and hence, $M_{\mu_a \boxtimes \mu_b}(z)$. The free product is commutative and associative.

As an example, we compute the S-transform of the Marchenko-Pastur distribution $\mu \sim \text{MP}(1)$. The distribution is given by

$$d\mu(x) = \frac{1}{2\pi} \sqrt{4x^{-1} - 1} dx.$$

The moments can be computed directly:

$$m_k = \sum_{i=0}^{k-1} \frac{1}{i+1} \binom{k}{i} \binom{k-1}{i} \qquad (3.5)$$

After some work, one can show that the moments above lead to a closed-form moment-generating function

$$M(z) = \frac{2z - 1 - \sqrt{1 - 4z}}{2z}.$$

One may then invert the expression and obtain the S-transform

$$S(z) = \frac{1}{1+z}.$$

Similarly, for the Marchenko-Pastur distribution $\text{MP}(t)$ with parameter $t$, which has distribution as given in Eq. (2.17), we find that

$$S(z) = \frac{1}{t+z}.$$

See, for instance, [12].
**3.1.3. Non-crossing Partitions.** Given $k \in \mathbb{N}$, let $NC(k)$ denote the set of non-crossing partitions of $[k]$. A non-crossing partition of $[k]$ is a partition $[k] = X_1 \cup \dots \cup X_m$ which is such that if $i < j \in X_\alpha$, then there are no $k, l \in X_\beta$ for $\beta \neq \alpha$ with $k < i < l < j$ or $i < k < j < l$. To any non-crossing partition, we associate a permutation $\pi \in S_k$ by mapping each subset $\{i_1, \dots, i_l\}$ to the cycle $(i_1, \dots, i_l)$ with $i_1 < \dots < i_l$. In a slight abuse of notation, we will write $\pi \in NC(k)$. For any $\pi \in S_k$, and for a sequence of numbers $f_k$ for $k = 1, 2, \dots$, we write

$$f_{\pi} = \prod_{l \in C(\pi)} f_l \qquad (3.6)$$

where $C(\pi)$ is the cycle type of $\pi$. We will need the following result, which is a straightforward consequence of the combinatorics of the S-transform.

**Theorem 3.2.** *Consider compactly supported probability distributions $\mu, \nu, \eta$. Suppose that the moments of $\eta$ are given by*

$$m_k^{\eta} = \sum_{\pi \in NC(k)} m_{\pi}^{\mu} m_{\pi^{-1}\tau_k}^{\nu}$$

where $\tau_k = (12\dots k)$ is the full cycle. Then,

$$\eta = \mathrm{MP}(1) \boxtimes \mu \boxtimes \nu.$$

*Proof.* We let $\mathcal{F}$ be the transformation that sends a formal power series $f(z)$ to the power series $\frac{1}{z}f^{-1}(z)$. This is such that for some distribution $\mu$, the S-transform is given by $S_{\mu}(z) = (1+z)\mathcal{F}(M_{\mu})(z)$. Moreover, given power series $f(z) = \sum_k f_k z^k$ and $g(z) = \sum_k g_k z^k$, define a convolution operation $\otimes$ by

$$(f \otimes g)(z) = \sum_k \left( \sum_{\pi \in NC(k)} f_{\pi} g_{\pi^{-1}\tau_k} \right) z^k$$

where $\tau_k$ is the full cycle in $S_k$. Then, Theorem 18.14 in [56] states that for any two $f$ and $g$ with $f_1 \neq 0$ and $g_1 \neq 0$, it holds that

$$\mathcal{F}(f \otimes g)(z) = \mathcal{F}(f)(z)\mathcal{F}(g)(z).$$

Then, the S-transform of $\eta$ can be written:

$$S_{\eta}(z) = (1+z)\mathcal{F}(M_{\eta})(z) = (1+z)\mathcal{F}(M_{\mu})(z)\mathcal{F}(M_{\nu})(z) = \frac{1}{1+z}S_{\mu}(z)S_{\nu}(z).$$

This implies the desired result, as the S-transform of $\mathrm{MP}(1)$ is given by $\frac{1}{1+z}$, and the S-transform uniquely determines a compactly supported distribution. $\square$

We remark briefly that free independence can equivalently be formulated in terms of the vanishing of *free cumulants*, which are themselves defined in terms of sums over non-crossing partitions. We refer the interested reader to any of the previously cited references for a more in-depth discussion on the role of non-crossing partitions in free probability. For our purposes, the fact that non-crossing partitions are intimately related to free independence will allow us to later phrase random tensor network results in terms of free probability.
## 3.2. Entanglement Spectrum of Random Tensor Network States as a Free Product

We now return to studying random tensor network states. Consider a family of states in $P_-(V)$ composed of the tensor product of link states $|\phi_e\rangle$ along the edges $e \in E$ as in Eq. (2.1), and assume that along each edge, the bond dimensions scale with a parameter $D$, so $D_e = \Theta(D)$. Our key assumption is that the link states have bounded spectral variation—by this we mean that the empirical distribution of the rescaled entanglement spectrum of the link states

$$ \mu_e^{(D)} := \sum_{i=1}^{D_e} \frac{1}{D_e} \delta_{D_e \lambda_{e,i}} \qquad (3.7) $$

has all moments converging to the moments $m_{e,k}$ of a compactly supported probability distribution $\mu_e$, as $D$ goes to infinity. We assume that the link states are normalized, so $m_{e,1} = 1$. This condition implies that, up to a vanishing fraction as $D \to \infty$, the elements of the entanglement spectrum of the link state are of order $D^{-1}$.

For a minimal cut $\gamma_A$, let $\mu_{\gamma_A}^{(D)}$ be the distribution for the spectrum of the tensor product of the link states in $\gamma_A$:

$$ \mu_{\gamma_A}^{(D)} = \bigotimes_{e \in \gamma_A} \mu_e^{(D)} = \frac{1}{D_{\gamma_A}} \sum_{\{i_e\}} \delta_{D_{\gamma_A} \prod_{e \in \gamma_A} \lambda_{e,i_e}} $$

where $i_e = 1, \dots, D_e$ and $D_{\gamma_A} = \prod_{e \in \gamma_A} D_e$. We define the tensor product of distributions as follows: If $X_1$ and $X_2$ are independent real valued random variables with distributions $\mu_{X_1}$ and $\mu_{X_2}$, then $\mu_{X_1} \otimes \mu_{X_2}$ is defined as the joint distribution of $(X_1, X_2)$. The distribution $\mu_{\gamma_A}^{(D)}$ has $k$th moment given by $m_{\gamma_A,k}^{(D)} = \prod_{e \in \gamma_A} m_{e,k}^{(D)}$, and we can see that $m_{\gamma_A,k}^{(D)}$ converges to $m_{\gamma_A,k}$, the moments of the distribution

$$ \mu_{\gamma_A} := \bigotimes_{e \in \gamma_A} \mu_e. $$

Let $\text{spec}(\rho_A) = \{\lambda_{A,i}\}$. (Recall that $\text{spec}(\rho_A)$ is ordered in non-increasing order.) Let $\gamma_A$ be a cut for $A$. By a standard argument, the number of nonzero eigenvalues of $\rho_A$ (that is, $\text{rank}(\rho_A)$) is upper bounded by $D_{\gamma_A}$. If $\gamma_A$ is the unique minimal cut, then we define

$$ \mu_A^{(D)} := \frac{1}{D_{\gamma_A}} \sum_{i=1}^{D_{\gamma_A}} \delta_{D_{\gamma_A} \lambda_{A,i}}. \qquad (3.8) $$

If there are multiple minimal cuts, it is ambiguous which $\gamma_A$, and hence, which $D_{\gamma_A}$, we should pick; we choose the cut for which $D_{\gamma_A}$ is minimal in Eq. (3.8), and we will denote this minimal cut by $\gamma_{A,1}$. The moments of $\mu_A^{(D)}$ are given by

$$ m_{A,k}^{(D)} := \int z^k d\mu_A(z) = D_{\gamma_A}^{k-1} \sum_{i=1}^{D_{\gamma_A}} (\lambda_{A,i})^k. $$
Note that the distribution $\mu_A^{(D)}$ is random, and correspondingly, the moments $m_{A,k}^{(D)}$ are random variables. In contrast, the moments $m_{e,k}^{(D)}$ and $m_{\gamma_A,k}^{(D)}$ are numbers depending only on the bond dimension.

The theorem we want to prove will follow straightforwardly from a key intermediate result: As $D$ goes to infinity, all the moments of the boundary distribution $\mu_A^{(D)}$ converge to the moments of $\mu_{\gamma_A}$. We use the notation in Eq. (3.6) to write expressions like

$$m_{\gamma_A, \pi} = \prod_{l \in C(\pi)} m_{\gamma_A, l}$$

for a permutation $\pi \in S_k$. We will then apply the method of moments to show that convergence of moments implies convergence in distribution. As a remark on notation, in the error bounds in both the current section and Sect. 4, when we use $\mathcal{O}$-notation, the constants may depend on the graph underlying the tensor network. (Typically our bounds scale as $2^{|V_b|}$, where $V_b$ is the set of bulk vertices.)

**Proposition 3.3.** If there exists a unique minimal cut $\gamma_A$ for $A$, then

$$\lim_{D \to \infty} \mathbb{E}m_{A,k}^{(D)} = m_{\gamma_A, k}. \qquad (3.9)$$

If there exist exactly two minimal cuts $\gamma_{A,1}$ and $\gamma_{A,2}$, which do not intersect (so $\gamma_{A,1} \cap \gamma_{A,2} = \emptyset$) and for which $\frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}}$ converges to a constant $t \le 1$, then

$$\lim_{D \to \infty} \mathbb{E}m_{A,k}^{(D)} = \sum_{\pi \in NC(k)} t^{d(\pi, \text{id})} m_{\gamma_{A,1}, \tau^{-1}\pi} m_{\gamma_{A,2}, \pi}. \qquad (3.10)$$

Moreover, in both cases the variance goes to zero as $D$ goes to infinity: for every $k$

$$\mathbb{E} \left[ \left( m_{A,k}^{(D)} - \mathbb{E} \left[ m_{A,k}^{(D)} \right] \right)^2 \right] = \mathcal{O} \left( \frac{1}{D} \right). \qquad (3.11)$$

*Proof.* We first provide a sketch of the proof. It proceeds via the following steps:

1. Write the expectation of the moments of $\mu_A^{(D)}$ as the partition function for a classical spin model, as in Sect. 2.1.

2. Show that the contributions from terms of the form given in the statement of the proposition dominate the partition function by carefully tracking the powers of $D$, and showing that all other contributions are suppressed polynomially in $D$.

3. Show that the variance of the moments vanishes in the limit $D \to \infty$ by direct computation.

We begin with Step 1. First, we observe that the $k$th moment of $\mu_A^{(D)}$ is given by $m_{A,k}^{(D)} = D_{\gamma_A}^{k-1} \text{tr}[\rho_A^k]$. Consider the expression in Eq. (2.14) for the replica trick with permutation $\pi$ on $A$:

$$Z_{k,\pi} := \mathbb{E} \text{tr} [R_A(\pi) \rho_A^{\otimes k}] = \sum_{\{\pi_x\} \in S_{A,\pi}} \prod_{e=(xy) \in E} \prod_{l \in C(\pi_x^{-1} \pi_y)} \text{tr}[\phi_{e,x}^l]. \qquad (3.12)$$
Recall that the set $S_{A,\pi}$, as defined in Eq. (2.11), consists of assignments of permutations to each $x \in V$, subject to $\pi_x = \pi$ for $x \in A$ and $\pi_x = \text{id}$ for $x \in \bar{A}$. As in Eq. (2.12), if $\pi = \tau$, then we indeed have $Z_{k,\pi} = \mathbb{E} \text{tr} [\rho_A^k]$, so

$$ \mathbb{E}m_{A,k}^{(D)} = D_{\gamma_A}^{k-1} Z_{k,\tau}. \qquad (3.13) $$

On the other hand, if we let $k = 2n$ and $\pi = \tilde{\tau} = (12\dots n)(n+1n+2\dots 2n)$, then $Z_{k,\pi} = \mathbb{E} [\text{tr} [\rho_A^n]^2]$, and hence,

$$ \mathbb{E} \left[ \left( m_{A,n}^{(D)} \right)^2 \right] = D_{\gamma_A}^{2n-2} Z_{k,\tilde{\tau}}. \qquad (3.14) $$

Recall that $m_{e,l}^{(D)} = D_e^{l-1} \text{tr} [\phi_{e,x}^l]$, and write

$$ Z_{k,\pi} = \sum_{\{\pi_x\} \in S_{A,\pi}} Z_k(\{\pi_x\}) $$

where

$$ \begin{aligned} Z_k(\{\pi_x\}) &:= \prod_{e=(xy) \in E} \prod_{l \in C(\pi_x^{-1} \pi_y)} \text{tr}[\phi_{e,x}^l] \\ &= \prod_{e=(xy) \in E} D_e^{|C(\pi_x^{-1} \pi_y)|-k} \prod_{l \in C(\pi_x^{-1} \pi_y)} m_{e,l}^{(D)} \qquad (3.15) \\ &= \prod_{e=(xy) \in E} D_e^{-d(\pi_x, \pi_y)} m_{e, \pi_x^{-1} \pi_y}^{(D)}. \end{aligned} $$

This accomplishes Step 1: We have recast the problem of computing moments into a question of computing a partition function for a classical spin model with fixed boundary conditions.

For Step 2, we want to show that the dominant contribution(s) to $Z_{k,\pi}$ as $D$ goes to infinity are those given in the statement of the proposition. This will simply be a matter of checking powers of $D$, and using the triangle inequality property of the Cayley distance. If $\Gamma_A$ is the unique minimal cut, then we let $\pi_x^{\min} = \pi$ for $x \in \Gamma_A$ and $\pi_x^{\min} = \text{id}$ for $x \in V \setminus \Gamma_A$, and we have

$$ Z_k(\{\pi_x^{\min}\}) = D_{\gamma_A}^{-d(\pi, \text{id})} \prod_{e \in \gamma_A} m_{e, \pi}^{(D)} = D_{\gamma_A}^{-d(\pi, \text{id})} m_{\gamma_A, \pi}^{(D)}. \qquad (3.16) $$

If there are exactly two minimal cuts $\Gamma_{A,1} \subset \Gamma_{A,2}$, we let $V = V_1 \sqcup V_2 \sqcup V_3$, with $V_1 = \Gamma_{A,1}$, $V_2 = \Gamma_{A,2} \cap \Gamma_{A,1}^c$ and $V_3 = \Gamma_{A,2}^c$. Now, consider the permutations $\sigma \in S_k$ that are on a geodesic between $\pi$ and $\text{id}$ (recall this implies $d(\pi, \sigma) + d(\sigma, \text{id}) = d(\pi, \text{id})$), and consider the configuration given by $\pi_x^{\sigma} = \pi$ for $x \in V_1$, $\pi_x^{\sigma} = \sigma$ for $x \in V_2$, and $\pi_x^{\sigma} = \text{id}$ for $x \in V_3$. By hypothesis, $\gamma_{A,1}$ and $\gamma_{A,2}$ do not intersect, and hence, the edges in each cut
are distinct. Then, this configuration has weight

$$
\begin{align}
Z_k(\{\pi_x^\sigma\}) &= \prod_{e_1 \in \gamma_{A,1}} D_{e_1}^{-d(\pi, \sigma)} \prod_{l_1 \in C(\pi^{-1}\sigma)} m_{e_1, l_1}^{(D)} \prod_{e_2 \in \gamma_{A,2}} D_{e_2}^{-d(\sigma, \mathrm{id})} \prod_{l_2 \in C(\sigma)} m_{e_2, l}^{(D)} \nonumber \\
&= D_{\gamma_{A,1}}^{-d(\pi, \mathrm{id})} \left(\frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}}\right)^{d(\sigma, \mathrm{id})} \prod_{e_1 \in \gamma_{A,1}} m_{e_1, \pi^{-1}\sigma}^{(D)} \prod_{e_2 \in \gamma_{A,2}} m_{e_2, \sigma}^{(D)} \nonumber \\
&= D_{\gamma_{A,1}}^{-d(\pi, \mathrm{id})} \left(\frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}}\right)^{d(\sigma, \mathrm{id})} m_{\gamma_{A,1}, \pi^{-1}\sigma}^{(D)} m_{\gamma_{A,2}, \sigma}^{(D)}, \tag{3.17}
\end{align}
$$

where $D_{\gamma_{A,1}}/D_{\gamma_{A,2}}$ converges to $t$, by assumption. Now, to show that these configurations yield the dominant contributions, we will need to use that $D_e = \Theta(D)$, so let us write $\frac{D}{D_e} = C_e^{(D)} = \Theta(1)$. Then for general configurations labeled by $\pi_x$, we may rewrite Eq. (3.15) as

$$
Z_k(\{\pi_x\}) = \prod_{e=(xy) \in E} D^{-d(\pi_x, \pi_y)} (C_e^{(D)})^{d(\pi_x, \pi_y)} m_{e, \pi_x^{-1} \pi_y}^{(D)}.
$$

The configurations we claimed to be dominant satisfy $Z_k(\{\pi\}) = \Theta(D^{-m(A)d(\pi,id)})$,
where we recall that $m(A)$ is the size of a minimal cut for $A$. Now, we will
show that all other configurations satisfy $Z_k(\{\pi\}) = \mathcal{O}(D^{-m(A)d(\pi,id)^{-1}})$. To
this end, consider some arbitrary configuration $\{\pi_x\} \in S_{A,\pi}$. Let $P$ be a max-
imal set of edge-disjoint paths in $G$ from $A$ to $\bar{A}$. It is a well-known fact that
such a set has size $m(A)$, by the max-flow min-cut theorem. Let

$$
C_k^{(D)} := \left( \max_{e \in E, l=1,\dots,k} (C_e^{(D)})^{l-1} \right) \left( \max_{e \in E, \pi \in S_k} m_{e,\pi}^{(D)} \right).
$$

Then, we may bound

$$
Z_k(\{\pi_x\}) \le (C_k^{(D)})^{|E|} \prod_{e=(xy) \in E} D^{-d(\pi_x, \pi_y)} \le (C_k^{(D)})^{|E|} \prod_{p \in P} D^{-\sum_{e=(xy) \in p} d(\pi_x, \pi_y)}. \tag{3.18}
$$

The first inequality is clear from the definition of $C_k^{(D)}$, and in the second
inequality, we simply restrict to a subset of the edges we multiply over. Note
that $C_k^{(D)} = \mathcal{O}(1)$. Then, by the triangle inequality for the Cayley distance $d$,
it holds that

$$
\sum_{e=(xy) \in p} d(\pi_x, \pi_y) \geq d(\pi, \mathrm{id})
$$

with equality if and only if the only edges (xy) for which $\pi_x \neq \pi_y$ are on a
path in P, and each of the paths is a geodesic. Then, we conclude

$$
Z_k(\{\pi_x\}) \le C_k^{(D)} \prod_{p \in P} D^{-d(\pi, \mathrm{id})} = C_k^{(D)} D^{-m(A)d(\pi, \mathrm{id})},
$$

and we see that the weight of every configuration can be bounded by the
product of a $O(1)$ number and a polynomial in $D$.
Now, as promised, we show that if {$\pi_x$} is not one of the minimal configurations described above, we actually have

$$Z_k(\{\pi_x\}) = \mathcal{O}(D^{-m(A)d(\pi, \mathrm{id})-1}). \qquad (3.19)$$

To see this, we rewrite the triangle inequality for the Cayley distance as:

$$\prod_{e=(xy) \in E} D^{-d(\pi_x, \pi_y)} \le \prod_{p \in P} D^{-\sum_{e=(xy) \in p} d(\pi_x, \pi_y)} \le D^{-m(A)d(\pi, \mathrm{id})} \qquad (3.20)$$

with equality if and only if the $\pi_x$ are on a geodesic path in P. We now show that this is satisfied only for the configurations we claimed to be minimal. Assume that {$\pi_x$} $\in S_{A,\pi}$ is such that the inequalities in Eq. (3.20) are equalities and let

$$\Delta_n = \{x \in V \text{ such that } d(\pi_x, \pi) \le n\}.$$

Then, $\Delta_n \in C(A)$ for $0 \le n < d(\pi, \mathrm{id})$, and we denote by $\delta_n$ the associated set of edges crossing the cut. Each edge $(xy) \in \delta_n$ must be such that $\pi_x \ne \pi_y$, so it must be on a path in P, and because the permutations are geodesics along the paths, they must be on different paths. Hence $|\delta_n| \le |P| = m(A)$, implying each $\Delta_n$ is a minimal cut. This immediately implies the claim if there is a unique minimal cut, since we must have $\Delta_{d(\pi, \mathrm{id})-1} = \Delta_0 = \Gamma_A$. If there are exactly two minimal cuts, then we must have $\pi_x = \pi$ for $x \in V_1$, $\pi_x = \mathrm{id}$ for $x \in V_3$, and there must be some $l$ such that for all $x \in V_2$ we have $d(\pi, \pi_x) = l$ and $d(\pi_x, \mathrm{id}) = d(\pi, \mathrm{id}) - l$. Then in order to have equality in Eq. (3.20), we must have that for all $x \in V_2$, $\pi_x$ equals some fixed permutation $\sigma$, because the assumption of having exactly two cuts implies that $V_2$ is connected, and we must have $d(\pi_x, \pi_y) = 0$ for all $(xy) \in E$ with $x, y \in V_2$. This proves Eq. (3.19).

In conclusion, if there is a unique minimal cut, then by Eqs. (3.16) and (3.19), we find

$$Z_{k, \pi} = D_{\gamma_A}^{-d(\pi, \mathrm{id})} m_{\gamma_A, \pi}^{(D)} + \mathcal{O}(D^{-m(A)d(\pi, \mathrm{id})-1}), \qquad (3.21)$$

and if there are exactly two (non-intersecting) cuts, then by Eqs. (3.17) and (3.19), we find

$$Z_{k, \pi} = \sum_{\sigma, d(\pi, \sigma) + d(\sigma, \mathrm{id}) = d(\pi, \mathrm{id})} D_{\gamma_{A,1}}^{-d(\pi, \mathrm{id})} \left( \frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}} \right)^{d(\sigma, \mathrm{id})} m_{\gamma_{A,1}, \pi^{-1}\sigma}^{(D)} m_{\gamma_{A,2}, \sigma}^{(D)} + \mathcal{O}(D^{-m(A)d(\pi, \mathrm{id})-1}). \qquad (3.22)$$

Finally, we set $\pi = \tau$ for the full cycle $\tau$ and we use Eq. (3.13). For a unique minimal cut $\gamma_A$, by Eq. (3.21)

$$\begin{aligned} \mathbb{E}m_{\gamma_A,k} &= D_{\gamma_A}^{k-1} Z_{k,\tau} \\ &= m_{\gamma_A,\pi}^{(D)} + \mathcal{O}(D_{\gamma_A}^{k-1} D^{-m(A)(k-1)-1}) \\ &= m_{\gamma_A,k}^{(D)} + \mathcal{O}\left(\frac{1}{D}\right). \end{aligned} \qquad (3.23)$$
using $d(\tau, \text{id}) = k - 1$ and $D_{\gamma_A} = \Theta(D^{m(A)})$. This proves Eq. (3.9) as $m_{\gamma_A, k}^{(D)}$ converges to $m_{\gamma_A, k}$.

For two non-intersecting minimal cuts, we saw that the dominant contribution is due to configurations $\{\pi_x^\sigma\}$ for $\sigma$ on a geodesic between $\tau$ and id. Then, applying the observation that $\sigma$ is on such a geodesic if and only if $\sigma$ is a non-crossing partition similarly yields that by Eq. (3.22)

$$ 
\begin{aligned}
\mathbb{E}m_{\gamma_A, k} &= D_{\gamma_A}^{k-1} Z_{k, \tau} \\
&= D_{\gamma_A}^{k-1} \sum_{\sigma \in NC(k)} \left(\frac{D_{\gamma_A, 1}}{D_{\gamma_A, 2}}\right)^{d(\sigma, \text{id})} m_{\gamma_A, 1, \pi^{-1}\sigma}^{(D)} m_{\gamma_A, 2, \sigma}^{(D)} \\
&\quad + \mathcal{O}(D_{\gamma_A}^{k-1} D^{-m(A)(k-1)-1}) \\
&= \sum_{\sigma \in NC(k)} \left(\frac{D_{\gamma_A, 1}}{D_{\gamma_A, 2}}\right)^{d(\sigma, \text{id})} m_{\gamma_A, 1, \tau^{-1}\sigma}^{(D)} m_{\gamma_A, 2, \sigma}^{(D)} + \mathcal{O}\left(\frac{1}{D}\right).
\end{aligned}
\quad (3.24) $$

Since $m_{\gamma_A, 1, \tau^{-1}\sigma}^{(D)} \to m_{\gamma_A, 1, \tau^{-1}\sigma}$, $m_{\gamma_A, 2, \sigma}^{(D)} \to m_{\gamma_A, 2, \sigma}$ and $D_{\gamma_A, 1}/D_{\gamma_A, 2} \to t$, this proves Eq. (3.10).

This accomplishes Step 2: We have shown that the configurations $\{\pi_x^{\min}\}$ (in case of a unique minimal cut for A) and $\{\pi_x^\sigma\}$ (in case there are exactly two non-intersecting minimal cuts for A) dominate in the computation of the expectation of the kth moment of $\mu_A$ in terms of powers of D.

We complete the proof by showing that the variance of $m_{A,k}$ vanishes as $D \to \infty$. We use the observation in Eq. (3.14), applying the analysis of $Z_{2k, \pi}$ to the case where $\pi = \tilde{\tau} = (12...k)(k+1k+2...2k)$. If there is a unique minimal cut, then using Eq. (3.21) and the fact that $d(\tilde{\tau}, \text{id}) = 2k-2$, we find

$$ 
\begin{aligned}
\mathbb{E}\left[(m_{A,k}^{(D)})^2\right] &= D_{\gamma_A}^{2k-2} Z_{2k, \tilde{\tau}} = \prod_{l \in C(\tilde{\tau})} m_{\gamma_A, l}^{(D)} + \mathcal{O}(D_{\gamma_A}^{2k-2} D^{-m(A)(2k-2)-1}) \\
&= (m_{\gamma_A, k}^{(D)})^2 + \mathcal{O}\left(\frac{1}{D}\right).
\end{aligned}
$$

By Eq. (3.23), we know that $(\mathbb{E}m_{A,k}^{(D)})^2 = (m_{\gamma_A, k}^{(D)} + \mathcal{O}(\frac{1}{D}))^2$, and we conclude that the variance obeys

$$ \mathbb{E}\left[(m_{A,k}^{(D)} - \mathbb{E}[m_{A,k}^{(D)}])^2\right] = \mathbb{E}\left[(m_{A,k}^{(D)})^2\right] - (\mathbb{E}m_{A,k}^{(D)})^2 = \mathcal{O}\left(\frac{1}{D}\right). $$

For the case with exactly two minimal cuts, a similar argument holds. Here, the key observation is that $\sigma$ is on a geodesic between $\tilde{\tau}$ and id if and only if $\sigma = \sigma_1\sigma_2$ where $\sigma_1$ is on a geodesic between (12...k) and id and $\sigma_2$ is on a
geodesic between $(k + 1 k + 2 \dots 2k)$ and id. Using Eq. (3.22), this implies

$$
\begin{align*}
\mathbb{E}(m_{A,k}^{(D)})^2 &= D_{\gamma_A}^{2k-2} Z_{2k,\bar{\tau}} \\
&= \sum_{\sigma_1, \sigma_2 \in NC(k)} \left( \frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}} \right)^{d(\sigma_1, \mathrm{id})+d(\sigma_2, \mathrm{id})} m_{\gamma_{A,1}, \tau^{-1}\sigma_1}^{(D)} \\
&\qquad m_{\gamma_{A,1}, \tau^{-1}\sigma_2}^{(D)} m_{\gamma_{A,2}, \sigma_1}^{(D)} m_{\gamma_{A,2}, \sigma_2}^{(D)} + \mathcal{O}\left(\frac{1}{D}\right) \\
&= \left( \sum_{\sigma \in NC(k)} \left( \frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}} \right)^{d(\sigma, \mathrm{id})} m_{\gamma_{A,1}, \tau^{-1}\sigma}^{(D)} m_{\gamma_{A,2}, \sigma}^{(D)} \right)^2 + \mathcal{O}\left(\frac{1}{D}\right).
\end{align*}
$$

By Eq. (3.24), we see that this coincides with $(\mathbb{E}m_{A,k}^{(D)})^2$, up to $\mathcal{O}(\frac{1}{D})$, and hence, Eq. (3.11) holds. $\square$

We now have the ingredients to prove that the entanglement spectrum of random tensor networks with link states with bounded spectral variation can be written in a simple fashion. We will use the method of moments to translate the above result on convergence of moments to convergence in distribution. The basic statement is that, given certain conditions on the distributions in question, if the moments of a sequence of distribution $\mu_n$ converge to those of $\mu$, then $\mu_n \Rightarrow \mu$—see, for instance, Theorem 30.8 in [13].

The method of moments is valid, so long as a distribution $\mu$ is completely determined by its moments. This occurs if, for all $k$, the $k$th moment $m_{\mu,k}$ is bounded as

$$m_{\mu,k} \leq AB^k k! \qquad (3.25)$$

for constants $A, B$ independent of $k$. If the distributions have compact support, as in Proposition 3.3, then this condition is satisfied.<fnref n="2" />

Now that we have established the convergence of moments in Proposition 3.3, we have our main result of the (conditional) convergence in distribution. As in Proposition 3.3, we consider a family of random tensor network states with link states with bounded spectral variation with increasing $D$, as defined in the beginning of this section.

**Theorem 3.4.** If there exists a unique minimal cut $\gamma_A$ for $A$, then $\mu_A^{(D)} \Rightarrow \mu_{\gamma_A}$, in probability, as $D \to \infty$. If there exist exactly two minimal cuts $\gamma_{A,1}$ and $\gamma_{A,2}$, which do not intersect and for which $\lim_{D \to \infty} \frac{D_{\gamma_{A,1}}}{D_{\gamma_{A,2}}} = t \le 1$, then $\mu_A^{(D)} \Rightarrow$ MP(1) $\boxtimes$ $\mu_{\gamma_{A,1}} \boxtimes \mu_{\gamma_{A,2}}(t)$, in probability, where $\mu_{\gamma_{A,2}}(t) = (1-t)\delta_0 + t\mu_{\gamma_{A,2}}$

<footnote n="2">²A basic example of a distribution which does not have compact support, but is nevertheless uniquely determined by its moments, is a standard Gaussian distribution. On the other hand, a standard example of distributions that are not determined by their moments is the densities on $\mathbb{R}_{\ge 0}$ with $d\mu_1(x) = \sqrt{2\pi x^{-1}}e^{-(\log x)^2/2}dx$ and $d\mu_2(x) = (1 + \sin(2\pi \log x))d\mu_1(x)$, for which it can be verified that the $n$th moments of both distributions are equal to $e^{-n^2/2}$, while the distributions are clearly not identical.</footnote>
**Proof.** It is straightforward to see that the kth moment of $\mu_{\gamma_{A,2}}(t)$ is given by $t^{k-1}m_{\gamma_{A,2},k}$, and then, the result follows immediately from Proposition 3.3, Theorem 3.2, and the method of moments. Because we assumed that for any minimal cut $\gamma_A$ for A, the limiting distributions $\mu_{\gamma_A}$ are compactly supported, they are uniquely determined by their moments. Hence, the method of moments is valid, and the convergence of moments implies convergence in distribution. $\square$

**Remark 3.5.** In Theorem 3.4, we assumed that the two cuts were non-intersecting. What happens if there are still only exactly two minimal cuts, but $\gamma_{A,1} \cap \gamma_{A,2}$ is non-empty? This extension is straightforward. Let $\gamma_A^{(a)} := \gamma_{A,1} \cap \gamma_{A,2}$ and let $\gamma_{A,i}^{(b)} = \gamma_{A,i} \setminus \gamma_A^{(a)}$ for $i = 1, 2$. In line with previous notation, let $\mu_{\gamma_A^{(a)}}$ and $\mu_{\gamma_{A,i}^{(b)}}$ denote the corresponding limiting distributions of the entanglement spectra along these sets, with moments $m_{\gamma_A^{(a)},k}$ and $m_{\gamma_{A,i}^{(b)},k}$. The only step in the proof of Proposition 3.3 where we used that the cuts were non-intersecting is when we computed the value of $Z_k(\{\pi_x\})$ for the optimal configuration. If the cuts do intersect, and we consider the configuration with $\pi_x = \tau$ for $x \in V_1$ with $\tau$ the complete cycle, $\pi_x = \sigma$ for $x \in V_2$ and $\sigma \in NC(k)$, and $\pi_x = \text{id}$ for $x \in V_3$, then a quick calculation shows

$$ Z_k(\{\pi_x\}) \rightarrow D_{\gamma_{A,1}}^{-d(\pi, \text{id})} (D_{\gamma_{A,1}}/D_{\gamma_{A,2}})^{d(\sigma, \text{id})} \prod_{e \in \gamma_A^{(a)}} m_{e,k} \\ \prod_{e_1 \in \gamma_{A,1}^{(b)}} m_{e_1, \pi^{-1}\sigma} \prod_{e_2 \in \gamma_{A,2}^{(b)}} m_{e_2, \sigma}. $$

Apart from this modification, the proof of Proposition 3.3 is still valid, leading to

$$ Z_{k, \tau} = m_{\gamma_A^{(a)}, k} \sum_{\sigma \in NC(k)} t^{d(\sigma, \text{id})} m_{\gamma_{A,1}^{(b)}, \tau^{-1}\sigma} m_{\gamma_{A,2}^{(b)}, \sigma}. $$

If, in Theorem 3.4, we do not assume that the cuts are non-intersecting, then the partition function above leads to a limiting distribution given by

$$ \mu_{\gamma_A^{(a)}} \otimes (MP(1) \boxtimes \mu_{\gamma_{A,1}^{(b)}} \boxtimes \mu_{\gamma_{A,2}^{(b)}}(t)). $$

### 3.3. Non-trivial Link States and Entanglement Negativity

As another application of the theory of free probability, we will compute the entanglement negativity spectrum for random tensor network states with link states with bounded spectra. In [29], it was shown how to compute the entanglement negativity spectrum for a random tensor network state with maximally entangled link states using a replica trick. Using the methods from the previous subsection, we can analyze the negativity for entangled link states with bounded spectral variation. We remark that similar computations have recently been performed in [28] in the context of replica wormholes, and our assumption on the link states is a generalization of the “pairwise connected regime” in [28]. Another work investigating non-trivial entanglement negativity spectra in random tensor networks is [42], where they focus on the effect of
having multiple minimal cuts in the network. As our analysis will be a straightforward combination of the arguments in [29] and Sect. 3.2, we will be rather concise; the main message of this section is to show that the language of free probability applies to other random tensor network computations as well.

We first recall how negativity functions as an entanglement measure for mixed states. Let $\mathcal{T}$ be the superoperator which maps an operator $X$ to its transpose $X^T$, and $\mathcal{I}$ be the identity superoperator. For $\rho_{AB} \in \mathcal{P}(AB)$,

$$ \rho_{AB}^{TB} := (\mathcal{I}_A \otimes \mathcal{T}_B)(\rho_{AB}) $$

is the partial transpose of $\rho_{AB}$ on the $B$ system. The logarithmic or entanglement negativity is given by

$$ E_N(\rho_{AB}) = \log \frac{\|\rho_{AB}^{TB}\|_1}{\text{tr}[\rho]} $$

It is a measure for the entanglement of the mixed state $\rho_{AB}$: if $E_N(\rho_{AB}) > 0$ the state must be entangled. We call spec($|\rho_{AB}^{TB}|$) the entanglement negativity spectrum. In analogy to the Rényi entropies, we can generalize the logarithmic negativity to a one-parameter family of negativities. The $k$th Rényi negativity is given by

$$ N_k(\rho_{AB}) = \text{tr} \left[ (\rho_{AB}^{TB})^k \right]. $$

If we let $N_m^{(\text{even})}(\rho_{AB}) = N_{2m}(\rho_{AB})$, then the logarithmic negativity is obtained as an analytic continuation in the Rényi index $m \to \frac{1}{2}$ of $\log(N_m^{(\text{even})}(\rho_{AB}))$. More precisely, in the expression

$$ \log \sum_{\lambda \in \text{spec}(\rho_{AB}^{TB})} |\lambda|^{\alpha}, $$

we may take $\alpha \to \frac{1}{2}$ to obtain $E_N(\rho_{AB}) + \log \text{tr}[\rho]$.

In the context of random tensor networks, we partition the boundary in three regions: $V_\partial = A \sqcup B \sqcup C$, and we would like to compute the Rényi negativities of the reduced state $\rho_{AB}$. We will then use this to determine the entanglement negativity spectrum and compute the entanglement negativity. The idea is that the $k$th Rényi negativity can be computed using a replica trick, by placing the full cycle $\tau_k = (12\dots k) \in S_k$ on $A$ and $\tau_k^{-1} = (kk^{-1}\dots 1)$ on $B$:

$$ \begin{aligned} N_k(\rho_{AB}) &= \text{tr} \left[ \rho_{AB}^{\otimes k} (R_A(\tau) \otimes R_B(\tau^{-1})) \right] \\ &= \text{tr} \left[ \rho_{ABC}^{\otimes k} (R_A(\tau) \otimes R_B(\tau^{-1}) \otimes R_C(\text{id})) \right]. \end{aligned} $$

Let us first discuss the case with maximally entangled link states, following [29]. The same arguments as in Sect. 2.2 show that one can compute the expectation of $N_k(\rho_{AB})$ for a random tensor network state using a spin model, now with boundary conditions of $\tau_k$ on $A$, $\tau_k^{-1}$ on $B$ and id on $C$. We will assume that the minimal cuts $\Gamma_A, \Gamma_B$ and $\Gamma_C$ are unique. Note that the minimal cut for $AB$ is given by $\Gamma_{AB} = \Gamma_C^c$. From the theory of multi-commodity flows, it is known that there exist sets of edge-disjoint paths $P = P_{AB} \cup P_{AC} \cup P_{BC}$,
<figure><img src="image_9.png" /><figcaption>(a) Illustration of the case where $\gamma_C = \gamma_A \cup \gamma_B$, where the dominant configuration is given by $\tau_k$ on $\Gamma_A$, $\tau_k^{-1}$ on $\Gamma_B$ and id on $\Gamma_C$.</figcaption></figure>

<figure><img src="image_10.png" /><figcaption>(b) Illustration of the case where $\gamma_C \neq \gamma_A \cup \gamma_B$, where the dominant configuration is given by $\tau_k$ on $\Gamma_A$, $\tau_k^{-1}$ on $\Gamma_B$ and id on $\Gamma_C$ and some non-crossing pairing $\pi_1$ on the domain $V_1$.</figcaption></figure>

<caption>FIGURE 4. Tensor networks with one and two minimal cuts. The relevant ground state configuration domains are denoted by $\Gamma_A$.</caption>

where $P_{AB}$ consists of paths from A to B, and similarly for $P_{AC}$ and $P_{BC}$, and which are such that

$$|P_{AB}| + |P_{AC}| = |\gamma_A|, \quad |P_{AB}| + |P_{BC}| = |\gamma_B|, \quad |P_{AC}| + |P_{BC}| = |\gamma_C|.$$

This can be used to show (in analogous fashion to the proof of Proposition 3.3) that if $k = 2n$ is even, any spin model configuration contributing to $\mathbb{E}N_k(\rho_{AB})$ is of order $O(D^{-(n-1)(|\gamma_A|+|\gamma_B|)-n|\gamma_C|})$. If $k = 2n + 1$ is odd, any spin model configuration contributing to $\mathbb{E}N_k(\rho_{AB})$ is of order $O(D^{-n(|\gamma_A|+|\gamma_B|+|\gamma_C|)})$.

In order to determine what happens as $D \to \infty$, we need to determine the dominant configurations. Let $r$ be the number of connected components of $V \setminus (\Gamma_A \cup \Gamma_B \cup \Gamma_C)$. There are two distinct cases. The first is when the minimal cut for AB (which is the complement of the minimal cut for C) is the union of the minimal cuts for A and B, so $\Gamma_{AB} = \Gamma_A \cup \Gamma_B$ and hence $\gamma_{AB} = \gamma_A \cup \gamma_B$. Then, the minimal cuts naturally partition the bulk vertices into three cuts $\Gamma_A$, $\Gamma_B$, and $\Gamma_C$, and we have $r = 0$. In this case, the dominant configurations in the spin model are those where the vertices in $\Gamma_A$ are assigned $\tau_k$, those in $\Gamma_B$ are assigned $\tau_k^{-1}$ and those in $\Gamma_C$ are assigned id. This is illustrated in Fig. 4a.

The second case is when $\Gamma_A \cup \Gamma_B \subsetneq \Gamma_{AB}$ and hence $\gamma_{AB} \neq \gamma_A \cup \gamma_B$. Now, we have again the domains $\Gamma_A$, $\Gamma_B$ and $\Gamma_C$, but upon removing these vertices, there may also be connected components $V_1, \dots, V_r$ which are not connected to A, B or C. Here, the minimal configurations are those for which, again, the vertices in $\Gamma_A$ are assigned $\tau_k$, those in $\Gamma_B$ are assigned $\tau_k^{-1}$ and those in $\Gamma_C$ are assigned id, and where in each component $V_i$ the vertices are assigned a permutation $\pi_i$ which is such that it satisfies three conditions: It must be on a geodesic between $\tau_k$ and $\tau_k^{-1}$, on a geodesic between $\tau_k$ and id and on a geodesic
between $\tau_k^{-1}$ and id. If $k = 2n$ is even, such permutations are given by non-crossing pairings: permutations corresponding to non-crossing partitions in which each cycle has length 2. The set of non-crossing pairings on $2n$ elements is in bijection with the set of non-crossing partitions on $n$ elements, so the number of non-crossing pairings on $2n$ elements is given by $|NC(n)| = C_n$. One way to obtain this correspondence is as follows. If $\pi$ is a non-crossing pairing, $\tau_{2n}\pi$ will map even numbers to even numbers, and restricting to the even numbers and relabeling $2i \mapsto i$ yields a non-crossing partition $\sigma \in NC(n)$. Moreover, restricting to the odd numbers and relabeling $2i + 1 \mapsto i$ yields the non-crossing partition $\sigma^{-1}\tau \in NC(n)$. This leads to $C_n^r$ dominant contributions to $\mathbb{E}N_{2n}(\rho_{AB})$ of size $D^{-(n-1)(|\gamma_A|+|\gamma_B|)-n|\gamma_C|}$ since we can choose a non-crossing pairing $\pi_i$ for each component. Such a configuration is illustrated in Fig. 4b.

For odd $k = 2n + 1$, we similarly have permutations which correspond to a non-crossing partition, and which have a single fixed point and all other cycles with length 2. This leads to $((2n + 1)C_n)^r$ dominant contributions to $\mathbb{E}N_{2n}(\rho_{AB})$, of size $D^{-(n-1)(|\gamma_A|+|\gamma_B|)-n|\gamma_C|}$. We also note that $\text{rank}(\rho_{AB}^{TB}) \le D^{|\gamma_A|+|\gamma_B|}$. If $\text{spec}(\rho_{AB}^{TB}) = \{s_i\}$, then we define the measure

$$ \mu_{AB}^{(D)} = \frac{1}{D^{|\gamma_A|+|\gamma_B|}} \sum_{i=1}^{D^{|\gamma_A|+|\gamma_B|}} \delta_{D^{\frac{1}{2}}(|\gamma_A|+|\gamma_B|+|\gamma_C|)s_i} \quad (3.26) $$

This has moments given by

$$ m_{AB,k}^{(D)} = \int x^k d\mu_{AB}^{(D)}(x) = D^{(\frac{k}{2}-1)(|\gamma_A|+|\gamma_B|)+\frac{k}{2}|\gamma_C|} N_k(\rho_{AB}). $$

If we take the expectation of the moments, we again need to distinguish the two cases. If $|\gamma_A| + |\gamma_B| = |\gamma_C|$, we see that the powers of $D$ cancel for the dominant configurations, so $m_{AB,k}^{(D)} \to 1$ for all $k$. On the other hand, for $|\gamma_A| + |\gamma_B| > |\gamma_C|$, we see that for $D \to \infty$ with odd $k$, we have $\mathbb{E}m_{AB,k}^{(D)} \to 0$. For even $k$, we recover the degeneracy of the dominant configurations, leading to

$$ \lim_{D \to \infty} m_{AB,k}^{(D)} = \begin{cases} 1 & \text{if } |\gamma_A| + |\gamma_B| = |\gamma_C|, \\ 0 & \text{if } k \text{ odd and } |\gamma_A| + |\gamma_B| > |\gamma_C|, \\ C_{k/2}^r & \text{if } k \text{ even and } |\gamma_A| + |\gamma_B| > |\gamma_C|, \end{cases} \quad (3.27) $$

where $r$ is the number of connected components of $V \setminus (\Gamma_A \cup \Gamma_B \cup \Gamma_C)$. In fact, one can show that, as in Proposition 3.3, the variance goes to zero as well, and hence, the method of moments allows one to conclude that $\mu_{AB}^{(D)} \Rightarrow \mu_{AB}$, in probability, where

$$ \mu_{AB} = \begin{cases} \sigma^{\otimes r} & \text{if } r > 0, \\ \frac{1}{2}\delta_1 + \frac{1}{2}\delta_{-1} & \text{if } r = 0 \text{ and } |\gamma_A| + |\gamma_B| > |\gamma_C|, \\ \delta_1 & \text{if } r = 0 \text{ and } |\gamma_A| + |\gamma_B| = |\gamma_C|, \end{cases} \quad (3.28) $$
where $\sigma$ is the semicircle distribution with density

$$d\sigma(x) = \frac{1}{2\pi} \sqrt{4 - x^2} \mathbb{1}_{|x| \le 2} dx$$

Alternatively, one may study the empirical distribution of the squared entanglement negativity spectrum

$$\nu_{AB}^{(D)} = \frac{1}{D|\gamma_A| + |\gamma_B|} \sum_i \delta_{D|\gamma_A| + |\gamma_B| + |\gamma_C|} s_i^2. \qquad (3.29)$$

This distribution has kth moment given by $m_{AB,2k}^{(D)}$, and in comparison with the limiting moments in Eq. (3.27), one can conclude that $\nu_{AB}^{(D)} \Rightarrow \nu_{AB}$, in probability, where

$$\nu_{AB} = MP(1)^{\otimes r}. \qquad (3.30)$$

The logarithmic negativity can be computed using the distribution $\mu_{AB}^{(D)}$ or $\nu_{AB}^{(D)}$ as

$$E_N(\rho_{AB}) = \log \int |\lambda| d\mu_{AB}^{(D)}(\lambda) + \frac{\log D}{2} (|\gamma_A| + |\gamma_B| - |\gamma_C|) - \log \text{tr}[\rho] \quad (3.31)$$

$$= \log \int \sqrt{\lambda} d\nu_{AB}^{(D)}(\lambda) + \frac{\log D}{2} (|\gamma_A| + |\gamma_B| - |\gamma_C|) - \log \text{tr}[\rho]. \qquad (3.32)$$

The convergence of $\nu_{AB}^{(D)}$ to $\nu_{AB}$ implies<fnref n="3" /> that $E_N(\rho_{AB}) - \frac{\log D}{2} (|\gamma_A| + |\gamma_B| - |\gamma_C|)$ converges in probability to

$$\log \int \sqrt{\lambda} d\nu_{AB}(\lambda) = r \log \frac{8}{3\pi}.$$

See Appendix D of [29] for details and proofs.

A straightforward combination of the arguments in Sect. 3.2 and [29] shows that the same configurations are the dominant contributions for link states with bounded spectral variation as in Sect. 3.2. To determine the limiting distribution in this case, we can generalize Eq. (3.28) in the same fashion as in Sect. 3.2. We assume the minimal cuts $\Gamma_A$, $\Gamma_B$ and $\Gamma_C$ are unique. We also assume that $\gamma_A \cap \gamma_B = \emptyset$, and in the case where $\gamma_C = \gamma_{AB} \neq \gamma_A \cup \gamma_B$ (so $|\gamma_A| + |\gamma_B| > |\gamma_C|$), all pairwise intersections between $\gamma_A$, $\gamma_B$ and $\gamma_C$ are empty. This excludes the case where $|\gamma_A| + |\gamma_B| > |\gamma_C|$, but $r = 0$. We let $\gamma_{A,i}$ and $\gamma_{B,i}$ denote the components of $\gamma_A$ and $\gamma_B$ which are connected to $V_i$, and we let $\mu_{\gamma_{A,i}}^{(D)}$ and $\mu_{\gamma_{B,i}}^{(D)}$ denote the distribution of the spectrum along these sets, with associated kth moments $m_{\gamma_{A,i},k}^{(D)}$, $m_{\gamma_{B,i},k}^{(D)}$, which we assume to converge to the moments $m_{\gamma_{A,i},k}$, $m_{\gamma_{B,i},k}$ of compactly supported distributions $\mu_{\gamma_{A,i}}$ and $\mu_{\gamma_{B,i}}$. For convenience, we assume $D_e = D$ for all edges $e \in E$.

We can now compute the dominant contributions to $\mathbb{E}N_k(\rho_{AB})$. If $\gamma_C = \gamma_A \cup \gamma_B$, then there is a unique dominant configuration, which contributes

<footnote n="3">³The function $f(\lambda) = \sqrt{\lambda}$ is not in $C_b(\mathbb{R})$, but the method of moments actually shows a stronger convergence, allowing test functions to have polynomial growth.</footnote>
$D^{-(k-1)|\gamma_C|}m_{\gamma_C,k}$. If $|\gamma_A| + |\gamma_B| > |\gamma_C|$ and $k = 2n$ is even, consider the configuration which assigns $\pi_i$ to $V_i$, where each $\pi_i$ is a non-crossing pairing. For each edge $e \in \gamma_C$, we have $m_{e,\pi_i}^{(D)} = (m_{e,2}^{(D)})^n$, so this configuration contributes

$$D^{-(n-1)(|\gamma_A|+|\gamma_B|)-n|\gamma_C|} \left(m_{\gamma_C,2}^{(D)}\right)^n \prod_{i=1}^{r} \left(m_{\gamma_{A,i},\tau_{2n}^{-1}\pi_i}^{(D)} m_{\gamma_{B,i},\tau_{2n}\pi_i}^{(D)}\right).$$

Recalling the construction of the equivalence between $NC(n)$ and non-crossing pairings on $2n$ elements, we see that

$$m_{\gamma_{B,i}, \tau_{2n} \pi_i}^{(D)} = m_{\gamma_{B,i}, \sigma_i}^{(D)} m_{\gamma_{B,i}, \sigma_i^{-1} \tau_n}^{(D)}$$

for some unique $\sigma_i \in NC(n)$. Similarly, one may verify

$$m_{\gamma_{A,i}, \tau_{2n}^{-1} \pi_i}^{(D)} = m_{\gamma_{A,i}, \sigma_i}^{(D)} m_{\gamma_{A,i}, \sigma_i^{-1} \tau_n}^{(D)}.$$

This implies that the contribution of all dominant configurations is given by

$$\left(m_{\gamma_C,2}^{(D)}\right)^n \prod_{i=1}^{r} \left( \sum_{\sigma \in NC(n)} m_{\gamma_{A,i},\sigma}^{(D)} m_{\gamma_{B,i},\sigma}^{(D)} m_{\gamma_{A,i},\sigma^{-1}\tau_n}^{(D)} m_{\gamma_{B,i},\sigma^{-1}\tau_n}^{(D)} \right)$$

As in the maximally entangled case, upon rescaling, the odd moments vanish as $D \to \infty$. In conclusion, the resulting asymptotic moments are given by

$$\lim_{D \to \infty} \mathbb{E} m_{AB,k}^{(D)} = \begin{cases} m_{\gamma_C,k} & \text{if } |\gamma_A| + |\gamma_B| = |\gamma_C|, \\ 0 & \text{if } k \text{ odd and } |\gamma_A| + |\gamma_B| > |\gamma_C|, \\ m_k & \text{if } k \text{ even and } |\gamma_A| + |\gamma_B| > |\gamma_C| \end{cases} \quad (3.33)$$

with

$$m_{2n} = m_{\gamma_C,2}^n \prod_{i=1}^{r} \left( \sum_{\sigma \in NC(n)} m_{\gamma_{A,i},\sigma} m_{\gamma_{B,i},\sigma} m_{\gamma_{A,i},\sigma^{-1}\tau_n} m_{\gamma_{B,i},\sigma^{-1}\tau_n} \right).$$

As before, one can also show, in similar fashion to the proof of Proposition 3.3, that the variance of the moments goes to zero as $D \to \infty$. For the case $|\gamma_A| + |\gamma_B| > |\gamma_C|$, we consider $\nu_{AB}^{(D)}$ similar to Eq. (3.29), but with an additional rescaling by $m_{\gamma_C,2}$:

$$\nu_{AB}^{(D)} = \frac{1}{D|\gamma_A|+|\gamma_B|} \sum_i \delta_{D|\gamma_A|+|\gamma_B|+|\gamma_C|} m_{\gamma_C,2s_i^2}^{-1}$$

This has moments, which compute $N_k^{(\text{even})}(\rho_{AB})$, converging to

$$\lim_{D \to \infty} \mathbb{E} \int x^k d\nu_{AB}^{(D)}(x) = \prod_{i=1}^{r} \left( \sum_{\sigma \in NC(n)} m_{\gamma_{A,i},\sigma} m_{\gamma_{B,i},\sigma} m_{\gamma_{A,i},\sigma^{-1}\tau_n} m_{\gamma_{B,i},\sigma^{-1}\tau_n} \right).$$

Thus, by the method of moments and Theorem 3.2, it holds that $\nu_{AB}^{(D)} \Rightarrow \nu_{AB}$, in probability, where

$$\nu_{AB} = \begin{cases} \bigotimes_{i=1}^{r} \nu_i & \text{if } r > 0, \\ \mu_{\gamma_C} & \text{if } r = 0, \end{cases} \quad (3.34)$$
and where $\nu_i$ is given by

$$ \nu_i = (\mu_{\gamma_{A,i}} \otimes \mu_{\gamma_{B,i}})^{\otimes 2} \boxtimes \mathrm{MP}(1). $$

This reduces to Eq. (3.30) if the link states are maximally entangled. We can use this to compute the logarithmic negativity, as we did previously. For $r > 0$,

$$ E_N(\rho_{AB}) = \log \int \sqrt{\lambda} d\nu_{AB}^{(D)}(\lambda) + \frac{\log D}{2} (|\gamma_A| + |\gamma_B| - |\gamma_C|) \\ + \frac{1}{2} \log m_{\gamma_{C,2}} - \log \mathrm{tr}[\rho], $$

from which we find that $E_N(\rho_{AB}) - \frac{\log D}{2}(|\gamma_A| + |\gamma_B| - |\gamma_C|)$ converges in probability to

$$ \log \int \sqrt{\lambda} d\nu_{AB}(\lambda) + \frac{1}{2} \log m_{\gamma_{C,2}}. $$

For the case $|\gamma_A| + |\gamma_B| = |\gamma_C|$, it is more elegant to use the limiting distribution of $\mu_{AB}^{(D)}$, as defined in Eq. (3.26). By the method of moments and Eq. (3.33), $\mu_{AB}^{(D)} \Rightarrow \mu_{\gamma_C}$, in probability. We may then compute the entanglement negativity as

$$ E_N(\rho_{AB}) = \log \int |\lambda| d\mu_{AB}^{(D)}(\lambda) + \frac{\log D}{2} (|\gamma_A| + |\gamma_B| - |\gamma_C|) - \log \mathrm{tr}[\rho], $$

and hence $E_N(\rho_{AB}) - \frac{\log D}{2}(|\gamma_A| + |\gamma_B| - |\gamma_C|)$ converges in probability to $\log \int |\lambda| d\mu_{AB}(\lambda)$.

# 4. Link States with Unbounded Spectral Variation

We will now consider a different regime, where the link states have unbounded spectral variation. Our methods in this section are distinct from the previous one, and the two sections can be considered separately.

## 4.1. One-Shot Entropies

We begin by introducing one of our main tools for studying entanglement spectra in random tensor network states: one-shot entropies. In quantum information theory, the rates of certain important protocols, such as compression or state merging can be expressed as entropic quantities. One-shot entropies are the appropriate analogs for settings where one would like to analyze a task for a single or finite number of copies of the relevant state. Asymptotic rates in terms of ordinary von Neumann entropies are then recovered in the limit of infinitely many independent copies. For an extensive introduction to this point of view, see [74]; here, we provide the basic definitions and introduce the relevant concepts.

A random tensor network built from link states that are maximally entangled (or more generally have bounded spectral variation) can be analyzed using asymptotic tools. Indeed, if we have a maximally entangled state of large dimension $D = 2^n$, then this is equal to the $n$th tensor power of a qubit maximally entangled state, so we are effectively in an asymptotic situation.
However, if we allow for link states with unbounded spectral variation or even completely general background states, as in Sect. 2.3, then it is more natural to use tools from one-shot quantum information theory.

We take the Rényi entropies as a starting point, which we defined in Eq. (2.7) for subnormalized states. Let $\mathcal{H}$ be some Hilbert space and for $\rho \in \mathcal{P}_{\le}(\mathcal{H})$ we define the (unconditional) min-entropy and the max-entropy by

$$H_{\min}(\rho) = -\log \|\rho\|_{\infty} \\ H_{\max}(\rho) = \log (\text{tr}[\sqrt{\rho}]^2)$$

which coincide with the Rényi entropies $H_{\infty}(\rho)$ and $H_{\frac{1}{2}}(\rho)$ for $\rho \in \mathcal{P}_{=}(\mathcal{H})$. As usual, if $\rho_A$ is the reduced density matrix on a system $\hat{A}$, we write $H_{\min}(A)_{\rho} = H_{\min}(\rho_A)$ and $H_{\max}(A)_{\rho} = H_{\max}(\rho_A)$.

Often, when applied to study quantum information processing tasks, it is useful to allow a small error. This leads to the introduction of smooth entropies. To define these, we use a distance measure known as the purified distance, which is given for $\rho, \sigma \in \mathcal{P}_{\le}(\mathcal{H})$ by

$$P(\rho, \sigma) = \sqrt{1 - F_{*}(\rho, \sigma)^2}$$

where $F_{*}(\rho, \sigma)$ is the generalized fidelity between $\rho$ and $\sigma$, which is defined by

$$F_{*}(\rho, \sigma) = F(\rho, \sigma) + \sqrt{(1 - \text{tr}[\rho])(1 - \text{tr}[\sigma])}$$

in terms of the ordinary fidelity $F(\rho, \sigma) = \|\sqrt{\rho}\sqrt{\sigma}\|_1$. We define the smooth min- and max-entropies of $\rho \in \mathcal{P}_{\le}(\mathcal{H})$ as

$$H_{\min}^{\epsilon}(\rho) = \sup_{\rho^{\epsilon} \in \mathcal{P}_{\le}(\mathcal{H}), P(\rho^{\epsilon}, \rho) \le \epsilon} H_{\min}(\rho^{\epsilon}) \\ H_{\max}^{\epsilon}(\rho) = \inf_{\rho^{\epsilon} \in \mathcal{P}_{\le}(\mathcal{H}), P(\rho^{\epsilon}, \rho) \le \epsilon} H_{\max}(\rho^{\epsilon}).$$

The smooth entropies are such that one recovers the usual von Neumann entropies in the limit of many independent copies. Indeed, the following asymptotic equipartition property holds:

$$\lim_{n \to \infty} \frac{1}{n} H_{\min}^{\epsilon}(\rho^{\otimes n}) = H(\rho) = \lim_{n \to \infty} \frac{1}{n} H_{\max}^{\epsilon}(\rho^{\otimes n})$$

for any $0 < \epsilon < 1$. Variations on this definition are possible. For instance, one can choose a different distance measure, which will yield different entropies. However, for the usual choices, the differences go to zero as $\epsilon$ goes to zero, so the particular choice is often immaterial. For instance, consider the trace distance between $\rho, \sigma \in \mathcal{P}_{\le}(\mathcal{H})$, which is defined by

$$T(\rho, \sigma) = \frac{1}{2} \|\rho - \sigma\|_1 + \frac{1}{2} |\text{tr}[\rho - \sigma]|,$$

where the last term, which is absent in usual definitions of the trace distance, accounts for subnormalized states. It is easy to see that $T(\rho, \sigma) \le \|\rho - \sigma\|_1 \le 2T(\rho, \sigma)$. The Fuchs-van de Graaff inequalities (see Lemma 3.17 in [74]) relate the trace distance and purified distance:

$$T(\rho, \sigma) \le P(\rho, \sigma) \le \sqrt{2T(\rho, \sigma)} \quad (4.1)$$
for $\rho, \sigma \in \mathcal{P}_{\leq}(\mathcal{H})$.

There are also conditional versions of the Rényi entropies. Consider a bipartite quantum state $\rho_{AB} \in \mathcal{P}_{=}(AB)$. For the von Neumann entropy, the conditional entropy can simply be defined as an entropy difference, namely $H(A|B)_{\rho} = H(AB)_{\rho} - H(B)_{\rho}$. However, it turns out that this is not a good definition in the Rényi case. There are various ways to define a Rényi conditional entropy $H_k(A|B)$; we use a version based on the so-called sandwiched Rényi relative entropy. For $k=2$, this gives a quantum conditional collision entropy, which will be useful for defining minimal cuts and which is defined as follows. For $\rho_{AB} \in \mathcal{P}_{\leq}(AB)$, let

$$H_2(A|B)_{\rho|\rho} := -\log \operatorname{tr} \left[ \left( (I \otimes \rho_B)^{-\frac{1}{4}} \rho_{AB} (I \otimes \rho_B)^{-\frac{1}{4}} \right)^2 \right] + \log \operatorname{tr}[\rho]. \quad (4.2)$$

Finally, there are also conditional versions of the min- and max-entropy. For $\rho_{AB} \in \mathcal{P}_{\leq}(AB)$ and $\sigma_B \in \mathcal{P}_{\leq}(B)$, we define

$$H_{\min}(A|B)_{\rho|\sigma} = -\inf\{\lambda : \rho_{AB} \le 2^{\lambda} I_A \otimes \sigma_B\}$$

$$H_{\max}(A|B)_{\rho|\sigma} = \log \| \sqrt{\rho_{AB}} \sqrt{I \otimes \sigma_B} \|_1^2$$

and we let

$$H_{\min}(A|B)_{\rho} = \sup_{\sigma \in \mathcal{P}_{\leq}(B)} H_{\min}(A|B)_{\rho|\sigma}$$

$$H_{\max}(A|B)_{\rho} = \sup_{\sigma \in \mathcal{P}_{\leq}(B)} H_{\max}(A|B)_{\rho|\sigma}.$$

We can also define their smoothed versions

$$H_{\min}^{\epsilon}(A|B)_{\rho} = \sup_{\rho^{\epsilon} \in \mathcal{P}_{\leq}(AB), P(\rho^{\epsilon}, \rho) \leq \epsilon} H_{\min}(A|B)_{\rho^{\epsilon}}$$

$$H_{\max}^{\epsilon}(A|B)_{\rho} = \inf_{\rho^{\epsilon} \in \mathcal{P}_{\leq}(AB), P(\rho^{\epsilon}, \rho) \leq \epsilon} H_{\max}(A|B)_{\rho^{\epsilon}}.$$

There is a duality between (smooth) max- and min-entropies. If $\rho \in \mathcal{P}_{\leq}(ABC)$ is a pure state, it holds that

$$H_{\min}^{\epsilon}(A|B)_{\rho} = -H_{\max}^{\epsilon}(A|C)_{\rho}. \quad (4.3)$$

We will use the fact that for a normalized state $\rho_{AB} \in \mathcal{P}_{=}(AB)$ (Corollary 5.10 in [74])

$$H_{\min}(A|B)_{\rho} \le H_2(A|B)_{\rho|\rho}. \quad (4.4)$$

A final important property of conditional smooth entropies is the data processing inequalities. Let $\Phi$ and $\Psi$ be completely positive and trace-preserving (CPTP) maps, mapping systems $A$ to $A'$ and $B$ to $B'$, respectively, and let $\sigma = (\Phi \otimes \Psi)(\rho)$. If $\Phi$ is also subunitary, and $0 \le \epsilon \le \sqrt{\operatorname{tr} \rho}$, then Theorem 6.2 of [74] states

$$H_{\min}^{\epsilon}(A'|B')_{\sigma} \ge H_{\min}^{\epsilon}(A|B)_{\rho} \quad \text{and} \quad H_{\max}^{\epsilon}(A'|B')_{\sigma} \ge H_{\max}^{\epsilon}(A|B)_{\rho}.$$

In fact, for the smooth min-entropy the data processing inequality is also valid if $\Phi$ is only trace non-increasing rather than trace-preserving, see [73].
## 4.2. Recovery Isometries

Recall that we study random tensor network states with link states, pure states placed on each edge whose tensor product forms the full state on edges $\phi = \bigotimes_{e \in E} \phi_e \in P_+(V)$ for some graph $G = (V, E)$. In Sect. 2.3, we considered more general background states $\phi_V \in P_-(V)$, where we no longer have a tensor product structure along the edges of some graph, and applying the replica trick does not yield a local spin model for the moments of the tensor network state. This situation is of independent interest, but will also be useful as an intermediate step when applying bounds based on one-shot entropies to link states. In Sect. 3, we studied link states for which the entanglement spectrum of the edge states $\phi_e$ had bounded variation, and we used the replica trick to compute the moments of the spectrum of $\rho_A$ for a boundary subsystem $A$. For general background states, we saw that the replica trick for $k = 2$ extends as in Eq. (2.20). What are the minimal cuts in this setting? Based on Eq. (2.20), a first guess would be that $\Gamma_A \in C(A)$ would be a minimal cut (i.e., correspond to the dominant term in the replica trick) if for all other cuts $\Delta_A \in C(A)$ we would have $H_2(\Gamma_A)_\phi \ll H_2(\Delta_A)_\phi$. If the state is a link state, this corresponds to adding weights to the edges of the graph corresponding to the Rényi-2 entropies along the edges, and computing a weighted minimal cut. Indeed, this would yield an accurate approximation of $\text{tr}[\rho_A^2]$ and hence of $H_2(\rho_A)$. However, if the spectrum of $\rho_A$ is not close to a flat spectrum, this does not imply that $\text{spec}_+(\rho_A)$ is close to $\text{spec}_+(\phi_{\Gamma_A})$. We would like to show that for link states with unbounded spectral variation, and an appropriate minimal cut condition for $\Gamma_A \in C(A)$, it is still true that $\text{spec}_+(\rho_A)$ is close to $\text{spec}_+(\phi_{\Gamma_A})$.

We will adapt the $k = 2$ replica trick for general background states to get a bound on the difference in trace norm between $\text{spec}_+(\rho_A)$ and $\text{spec}_+(\phi_{\Gamma_A})$ in terms of conditional Rényi-2 entropies,<fnref n="4" /> as defined in Eq. (4.2). In Sect. 4.3, we will use this to formulate a condition for cut minimality in terms of smooth entropies for link states.

The main result of this subsection is a tensor network version of one-shot decoupling. Let $\phi_V \in P_-(V)$. We allow $\phi_V$ to be a general state, which need not be pure and also need not be a product state along the edges of some graph. Let $R$ be a purifying system and $\phi_{VR} \in P_-(VR)$ be a purification of $\phi_V$. Then, we can construct the random tensor network state $\rho_{V\partial R}$ where the boundary systems are given by $V_\partial \cup R$, which is a purification of the random tensor network state $\rho_{V\partial}$ as in Eq. (2.18) by

$$ \phi_{V\partial R} = \text{tr}_{V_\partial} [(I_{V\partial R} \otimes \psi)\phi] \quad (4.5) $$

where $\psi$ is a tensor product of random tensors. We briefly recall our notation for boundary subsystems and cuts: For a boundary subsystem $A \subseteq V_\partial$, we denote its boundary complement by $\bar{A} = V_\partial \setminus A$, and for a cut $\Gamma_A \in C(A)$, we

<footnote n="4">⁴Note that while $H(A|B)_\phi = H(AB)_\phi - H(B)_\phi$, in general $H_2(A|B)_{\phi|\phi} \neq H_2(AB)_\phi - H_2(B)_\phi$.</footnote>
let $\Gamma_A^c = V \setminus \Gamma_A$, which is a cut for $\bar{A}$. The purifying system $R$ can be thought of as an additional boundary system in the tensor network construction.

In Theorem 4.4, we will assume that we have a cut $\Gamma_A \in C(A)$ which is such that for all cuts $\Delta_A \in C(A)$ for which $\Delta_A \subsetneq \Gamma_A$ we have $H_2(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi|\phi} \gg 1$, and similarly for all cuts $\Delta_A \in C(\bar{A})$ for which $\Gamma_A \subsetneq \Delta_A$ we have $H_2(\Delta_A \setminus \Gamma_A | \Gamma_A R)_{\phi|\phi} \gg 1$. We show that this condition implies that with high probability there exist isometries $V_A : \mathcal{H}_A \to \mathcal{H}_{\Gamma_A}$ and $V_{\bar{A}} : \mathcal{H}_{\bar{A}} \to \mathcal{H}_{\Gamma_A^c}$ such that

$$ (V_A \otimes V_{\bar{A}} \otimes I_R) |\rho\rangle \approx |\phi\rangle. \qquad (4.6) $$

The approximation accuracy will be measured in trace norm. In particular, this implies that $\text{spec}_+(\rho_A) \approx \text{spec}_+(\phi_{\Gamma_A})$. If the state $\phi$ is a tensor product of link states, $\text{spec}_+(\phi_{\Gamma_A})$ is precisely the entanglement spectrum along the cut $\gamma_A$. The isometries $V_A$ and $V_{\bar{A}}$ are recovery isometries, which allow us to “recover” $\Gamma_A$ from the $A$ system, and similarly we can recover $\Gamma_A^c$ from $\bar{A}$.

The result is closely related to quantum error correction. One way to interpret this is as follows: Consider a subspace $\mathcal{H}_S$ of $\mathcal{H}_V$ and let $R$ be a reference system of dimension $\text{dim}(\mathcal{H}_S)$, and $\phi_{VR}$ a maximally entangled state between $S$ and $R$. Then, Eq. (4.6) can be interpreted as saying that if we encode the subspace $S$ by projecting onto random tensors, the information in $\Gamma_A$ is protected, after encoding, against an erasure error on $\bar{A}$. This idea is also discussed in [61] for perfect tensor network models, and in [40] for random tensor networks with maximally entangled link states. In holography, the notion of local recovery isometries and their error correction interpretation goes under the name of entanglement wedge reconstruction or subregion-subregion duality. See [6,7] for a detailed discussion of entanglement wedge reconstruction in holographic systems with bulk entropy, relating to one-shot entropies. We provide more details in “Appendix B.”

Our approach to showing Eq. (4.6) is that we start by projecting only on the random tensors in $\Gamma_A$, and not on the random tensors in $\Gamma_A^c$. This yields a random tensor network state $\sigma$ on $A\Gamma_A^c R$.

We then show that, by a version of one-shot decoupling, the reduced state on $\sigma_{\Gamma_A^c R}$ has not changed much from $\phi_{\Gamma_A^c R}$. By Uhlmann’s theorem, this implies that there exists an isometry $V_A$ such that $(V_A \otimes I_{\Gamma_A^c R}) |\sigma\rangle \approx |\phi\rangle$. Combining this with a similar result for $\Gamma_A^c$ we obtain Eq. (4.6), as will be made precise in Theorem 4.4.

In our construction of $\sigma$, we can relabel the vertices in the graph, and think of the vertices in $\Gamma_A \setminus A$ as the bulk vertices $V_b$, the boundary subsystem $A$ as the complete boundary $V_\partial$, and relabel all other subsystems as the reference system $R$. Then, we prove the following result, which is closely related to the one-shot decoupling results in [24].

**Proposition 4.1.** Consider a random tensor network state $\rho_{V_\partial R}$ as in Eq. (4.5) with a (purified) background state $\phi_{VR} \in \mathcal{P}_\leq(VR)$. Let $A = V_\partial$ and let $\Gamma_A = V$ and suppose that for any cut $\Delta_A \in C(A)$ other than $\Gamma_A$

$$ H_2(\Gamma_A \setminus \Delta_A | R)_{\phi|\phi} \geq K $$
then

$$ \mathbb{E}\|\rho_R - \phi_R\|_1 \le 2^{\frac{|V_b|}{2}} \sqrt{\text{tr}[\phi]} 2^{-\frac{1}{2}K}. $$

Note that since $\Gamma_A = V_b \cup A$, the sets $\Gamma_A \setminus \Delta_A$ for $\Delta_A \in C(A) \setminus \{\Gamma_A\}$ are exactly the non-empty subsets of $V_b$. The formulation in terms of $\Delta_A \in C(A)$ will be natural when we apply this result in Theorem 4.4.

**Proof.** We closely follow the strategy in [24,26]. We first note a basic fact (Lemma 3.7 in [24]): For any operator $X$ and $\omega$ a subnormalized density matrix, it holds that

$$ \|X\|_1 \le \|\omega^{-\frac{1}{4}} X \omega^{-\frac{1}{4}}\|_2. \quad (4.7) $$

The proof is an application of the Cauchy–Schwarz inequality. We use Eq. (4.7) with $\omega = \phi_R$ and Jensen's inequality to see that

$$ \mathbb{E}\|\rho_R - \phi_R\|_1 \le \sqrt{\mathbb{E}\text{tr}[(\tilde{\rho}_R - \tilde{\phi}_R)^2]} $$

where $\tilde{\rho}_{V_b R} = (I \otimes \phi_R)^{-\frac{1}{4}} \rho_{V_b R} (I \otimes \phi_R)^{-\frac{1}{4}}$ and $\tilde{\phi}_{VR} = (I \otimes \phi_R)^{-\frac{1}{4}} \phi_{VR} (I \otimes \phi_R)^{-\frac{1}{4}}$. Now, $\mathbb{E}\tilde{\rho}_R = \tilde{\phi}_R$ by Eq. (2.21), and the replica trick in Eq. (2.20) yields

$$ \begin{aligned} \mathbb{E}\text{tr}[(\tilde{\rho}_R - \tilde{\phi}_R)^2] &= \mathbb{E}\text{tr}[\tilde{\rho}_R^2] - \text{tr}[\tilde{\phi}_R^2] \\ &= \sum_{\Delta_A \in C(A), \Delta_A \subsetneq \Gamma_A} \text{tr}[\tilde{\phi}_{(\Gamma_A \setminus \Delta_A)R}^2] \\ &= \sum_{\Delta_A \in C(A), \Delta_A \subsetneq \Gamma_A} \text{tr}[\phi] 2^{-H_2(\Gamma_A \setminus \Delta_A | R)_{\phi|\phi}} \end{aligned} $$

using the definition of $\tilde{\phi}$ and Eq. (4.2) and hence

$$ (\mathbb{E}\|\rho_R - \phi_R\|_1)^2 \le 2^{|V_b|} \text{tr}[\phi] 2^{-K}. $$

□

Suppose that in the setup of Proposition 4.1, we would have equality $\rho_R = \phi_R$. Then, by Uhlmann's theorem, their purifications $\rho_{AR}$ and $\phi_{\Gamma_{AR}}$ are related by an isometry $V_A$ from $A$ to $\Gamma_A$. The following lemma is useful to extend to the case where the reduced states are close in trace distance.

**Lemma 4.2.** Suppose $\rho_{AB} \in \mathcal{P}(AB)$ and $\sigma_{AC} \in \mathcal{P}(AC)$ are pure states on Hilbert spaces $\mathcal{H}_A \otimes \mathcal{H}_B$ and $\mathcal{H}_A \otimes \mathcal{H}_C$, respectively. Then,

$$ \min_V \|(I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger) - \sigma_{AC}\|_1 \le 2\sqrt{2\|\rho_A - \sigma_A\|_1 + 2\|\rho_A - \sigma_A\|_1^2}. $$

where the minimum is over all isometries $V: \mathcal{H}_B \to \mathcal{H}_C$.

**Proof.** Uhlmann's theorem states that if $\rho_{AB} \in \mathcal{P}(AB)$ and $\sigma_{AC} \in \mathcal{P}(AC)$ are pure quantum states with $\dim(\mathcal{H}_B) \le \dim(\mathcal{H}_C)$, then there exists an isometry $V: \mathcal{H}_B \to \mathcal{H}_C$ such that

$$ P(\rho_A, \sigma_A) = P((I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger), \sigma_{AC}) $$
and, in particular, the isometry is the solution to an optimization problem:

$$P(\rho_A, \sigma_A) = \min_V P((I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger), \sigma_{AC}).$$

Moreover, if both $\rho$ and $\sigma$ are subnormalized, by Eq. (4.1), we can bound

$$\begin{aligned} \min_V \|(I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger) - \sigma_{AC}\|_1 &\le \min_V 2P((I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger), \sigma_{AC}) \\ &= 2P(\rho_A, \sigma_A) \\ &\le 2\sqrt{2\|\rho_A - \sigma_A\|_1}. \end{aligned}$$

From this, it follows that if $\sigma$ is subnormalized and $\rho$ has $\text{tr}[\rho] > 1$,

$$\min_V \|(I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger) - \sigma_{AC}\|_1 \le 2\sqrt{2\text{tr}[\rho]\|\rho_A - \sigma_A\|_1}.$$

Since $\text{tr}[\rho] \le \text{tr}[\sigma] + \|\rho - \sigma\|_1$ and $\text{tr}[\sigma] \le 1$, we conclude that

$$\min_V \|(I_A \otimes V)\rho_{AB}(I_A \otimes V^\dagger) - \sigma_{AC}\|_1 \le 2\sqrt{2\|\rho_A - \sigma_A\|_1 + 2\|\rho_A - \sigma_A\|_1^2}.$$

for arbitrary $\rho$ and subnormalized $\sigma$. $\square$

<figure><img src="image_11.png" /></figure>

Finally, we will need a basic lemma relating tensor network states with differing background states:

**Lemma 4.3.** Suppose we consider random tensor network states $\rho_{V_R}$ and $\tilde{\rho}_{V_R}$ with (purified) background states $\phi_{VR}, \tilde{\phi}_{VR} \in \mathcal{P}_\le(VR)$ and projecting onto the same random tensors. Then,

$$\mathbb{E}\|\rho_{V_R} - \tilde{\rho}_{V_R}\|_1 \le \|\phi_{VR} - \tilde{\phi}_{VR}\|_1.$$

*Proof.* Let $\phi - \tilde{\phi} = \Delta_+ - \Delta_-$ where both $\Delta_+$ and $\Delta_-$ are positive semidefinite and are such that $\|\phi - \tilde{\phi}\|_1 = \text{tr}[\Delta_+ + \Delta_-]$. Then, we can also consider the random tensor network states $\sigma_+$ and $\sigma_-$ which take $\Delta_+$ and $\Delta_-$ as background states, and by the linearity of Eq. (4.5) in the background state we have $\rho - \tilde{\rho} = \sigma_+ - \sigma_-$. By Eq. (2.21), $\mathbb{E}\sigma_\pm = \Delta_\pm$. We then estimate

$$\begin{aligned} \mathbb{E}\|\rho - \tilde{\rho}\|_1 &= \mathbb{E}\|\sigma_+ - \sigma_-\|_1 \le \mathbb{E}(\|\sigma_+\|_1 + \|\sigma_-\|_1) = \mathbb{E}\text{tr}[\sigma_+ + \sigma_-] \\ &= \text{tr}[\Delta_+ + \Delta_-] = \|\phi - \tilde{\phi}\|_1. \end{aligned}$$

where we have used that $\sigma_+$ and $\sigma_-$ are positive semidefinite and hence $\|\sigma_\pm\|_1 = \text{tr}[\sigma_\pm]$. $\square$

<figure><img src="image_12.png" /></figure>

With all our tools assembled, we are ready to prove the main result of this subsection. We again let $\phi_{VR} \in \mathcal{P}_\le(VR)$ be a background state with $R$ a purifying system, and we let $\rho_{V_R}$ be the associated random tensor network state as constructed in Eq. (4.5). Let $\Gamma_A$ be an arbitrary cut for the boundary region $A$. In Theorem 4.4, we provide a criterion to determine whether $\Gamma_A$ is a minimal cut in terms of conditional entropies. Informally speaking, the following result shows that if $\Gamma_A$ is a minimal cut in this sense, we can recover the system $\Gamma_A$ from the boundary subsystem $A$, while we can recover $\Gamma_A^c$ from the boundary subsystem $\bar{A}$. For general $\phi$, Theorem 4.4 is closely related to the task of split transfer, see “Appendix B” for a discussion. The following result closely follows Proposition 18 of [26].
**Theorem 4.4** (Recovery isometries). Let $\phi_{VR} \in \mathcal{P}_{\le}(VR)$, and let $\rho_{V_{\partial}R}$ be the associated random tensor network state as in Eq. (4.5). Let $\Gamma_A \in \mathcal{C}(A)$ and suppose that

$$H_2(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi|\phi} \geq K_1 \qquad (4.8)$$

for all cuts $\Delta_A \in \mathcal{C}(A)$ such that $\Delta_A \subsetneq \Gamma_A$ and

$$H_2(\Delta_A \setminus \Gamma_A | \Gamma_A R)_{\phi|\phi} \geq K_2 \qquad (4.9)$$

for all cuts $\Delta_A \in \mathcal{C}(A)$ such that $\Gamma_A \subsetneq \Delta_A$. Then,

$$\begin{aligned} \mathbb{E} \min_{V_A, V_A} & \|(V_A \otimes V_{\bar{A}} \otimes I_R) \rho_{V_{\partial}R} (V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR} \|_1 \\ &= \mathcal{O}(\mathrm{tr}[\phi]^{\frac{1}{4}}(2^{-\frac{1}{4}}K_1 + 2^{-\frac{1}{4}}K_2)). \end{aligned} \qquad (4.10)$$

where the minimum is over isometries $V_A : \mathcal{H}_A \to \mathcal{H}_{\Gamma_A}$ and $V_{\bar{A}} : \mathcal{H}_{\bar{A}} \to \mathcal{H}_{\Gamma_A^c}$.

*Proof.* Let $\sigma_{\Gamma_A^c R}$ be the state where we have contracted along the tensors in $\Gamma_A$ but not along those in $\Gamma_A^c$, and similarly let $\tau_{\bar{A}\Gamma_A R}$ be the state where we have contracted along the tensors in $\Gamma_A^c$ but not along those in $\Gamma_A$. We first use Proposition 4.1 to show that $\sigma_{\Gamma_A^c R} \approx \phi_{\Gamma_A^c R}$ and $\tau_{\Gamma_A R} \approx \phi_{\Gamma_A R}$. Indeed, for $\sigma$ we simply apply Proposition 4.1 with $V_b \cap \Gamma_A$ as the set of bulk vertices, $A$ as the set of boundary vertices and $\Gamma_A^c R$ as the reference system. This gives

$$\mathbb{E}\|\sigma_{\Gamma_A^c R} - \phi_{\Gamma_A^c R}\|_1 = \mathcal{O}(\sqrt{\mathrm{tr}[\phi]})2^{-\frac{1}{2}K_1}.$$

A similar application of Proposition 4.1, with $V_b \cap \Gamma_A^c$ as the set of bulk vertices, $\bar{A}$ as the set of boundary vertices and $\Gamma_A R$ as the reference system, shows

$$\mathbb{E}\|\tau_{\Gamma_A R} - \phi_{\Gamma_A R}\|_1 = \mathcal{O}\left(\sqrt{\mathrm{tr}[\phi]} 2^{-\frac{1}{2}K_2}\right).$$

We note that for any isometries $V_A : \mathcal{H}_A \to \mathcal{H}_{\Gamma_A}$ and $V_{\bar{A}} : \mathcal{H}_{\bar{A}} \to \mathcal{H}_{\Gamma_A^c}$

$$\begin{aligned} & \|(V_A \otimes V_{\bar{A}} \otimes I_R) \rho (V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR} \|_1 \\ & \le \|(I_{\Gamma_A} \otimes V_{\bar{A}} \otimes I_R) \tau (I_{\Gamma_A} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR} \|_1 \\ & \quad + \|\tau - (V_A \otimes I_{\bar{A}R}) \rho (V_A^{\dagger} \otimes I_{\bar{A}R}) \|_1, \end{aligned}$$

where we have applied the triangle inequality after adding and subtracting $(I_{\Gamma_A} \otimes V_{\bar{A}} \otimes I_R)\tau(I_{\Gamma_A} \otimes V_{\bar{A}}^{\dagger} \otimes I_R)$, and then using the invariance of the trace norm under isometries in the second term. We use this to estimate

$$\begin{aligned} \mathbb{E} \min_{V_A, V_{\bar{A}}} & \|(V_A \otimes V_{\bar{A}} \otimes I_R) \rho (V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR} \|_1 \\ & \le \mathbb{E} \left( \min_{V_A} \|(I_{\Gamma_A} \otimes V_{\bar{A}} \otimes I_R) \tau (I_{\Gamma_A} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR} \|_1 \right. \\ & \qquad \left. + \min_{V_A} \|\tau - (V_A \otimes I_{\bar{A}R}) \rho (V_A^{\dagger} \otimes I_{\bar{A}R}) \|_1 \right), \end{aligned} \qquad (4.11)$$
where the minimum is over isometries $V_A : \mathcal{H}_A \to \mathcal{H}_{\Gamma_A}$ and $V_{\bar{A}} : \mathcal{H}_{\bar{A}} \to \mathcal{H}_{\Gamma_{\bar{A}}^c}$.
For the first term of Eq. (4.11), we apply Lemma 4.2 to get

$$ \begin{aligned} \min_{V_{\bar{A}}} & \|(I_{\Gamma_A} \otimes V_{\bar{A}} \otimes I_R)\tau(I_{\Gamma_A} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR}\|_1 \\ & \le 2\sqrt{2}\|\tau_{\Gamma_{AR}} - \phi_{\Gamma_{AR}}\|_1 + 2\|\tau_{\Gamma_{AR}} - \phi_{\Gamma_{AR}}\|_1^2 \\ & \le 2\sqrt{2}\left(\sqrt{\|\tau_{\Gamma_{AR}} - \phi_{\Gamma_{AR}}\|_1} + \|\tau_{\Gamma_{AR}} - \phi_{\Gamma_{AR}}\|_1\right) \end{aligned} $$

and by Jensen's inequality

$$ \begin{aligned} \mathbb{E} \min_{V_{\bar{A}}} & \|(I_{\Gamma_A} \otimes V_{\bar{A}} \otimes I_R)\tau(I_{\Gamma_A} \otimes V_{\bar{A}}^{\dagger} \otimes I_R) - \phi_{VR}\|_1 \\ & \le 2\sqrt{2} \left( \sqrt{\mathbb{E}\|\tau_{\Gamma_{AR}} - \phi_{\Gamma_{AR}}\|_1} + \mathbb{E}\|\tau_{\Gamma_{AR}} - \phi_{\Gamma_{AR}}\|_1 \right) \\ & = \mathcal{O}\left(\text{tr}[\phi]^{\frac{1}{4}} 2^{-\frac{1}{4}K_2}\right) \end{aligned} \quad (4.12) $$

For the second term of Eq. (4.11), we can think of $\tau$ and $(V_A \otimes I_{\bar{A}})\rho(V_A^\dagger \otimes I_{\bar{A}})$ as the random tensor network states with $\phi$ and $(V_A \otimes I_{\Gamma_A^c})\sigma(V_A^\dagger \otimes I_{\Gamma_A^c})$ as the full state on edges, applying random tensors in $\Gamma_A^c$. Then, denoting by $\mathbb{E}_{\Gamma_A^c}$ the expectation value over all random tensors in $\Gamma_A^c$, by Lemma 4.3

$$ \mathbb{E}_{\Gamma_A^c} \| \tau - (V_A \otimes I_{\bar{A}}) \rho(V_A^\dagger \otimes I_{\bar{A}}) \|_1 = \mathcal{O}(\|\phi_{VR} - (V_A \otimes I_{\bar{A}}) \sigma(V_A^\dagger \otimes I_{\bar{A}})\|_1). $$

We thus estimate

$$ \begin{aligned} \mathbb{E} \min_{V_A} \| \tau - (V_A \otimes I_{\bar{A}}) \rho(V_A^\dagger \otimes I_{\bar{A}}) \|_1 \\ = \mathcal{O} \left( \mathbb{E}_{\Gamma_A} \min_{V_A} \| \phi_{VR} - (V_A \otimes I_{\bar{A}}) \sigma(V_A^\dagger \otimes I_{\bar{A}}) \|_1 \right) \end{aligned} $$

for which we may argue exactly as in Eq. (4.12) and using Lemma 4.2 that

$$ \mathbb{E}_{\Gamma_A} \min_{V_A} \| \phi_{VR} - (V_A \otimes I_{\Gamma_A^c}) \sigma(V_A^\dagger \otimes I_{\Gamma_A^c}) \|_1 = \mathcal{O} \left( \text{tr}[\phi]^{\frac{1}{4}} 2^{-\frac{1}{4}K_1} \right). $$

We conclude that

$$ \begin{aligned} \mathbb{E} \min_{V_A, V_{\bar{A}}} & \|(V_A \otimes V_{\bar{A}} \otimes I_R) \rho(V_A^\dagger \otimes V_{\bar{A}}^\dagger \otimes I_R) - \phi_{VR}\|_1 \\ & = \mathcal{O}\left(\text{tr}[\phi]^{\frac{1}{4}}\left(2^{-\frac{1}{4}K_1} + 2^{-\frac{1}{4}K_2}\right)\right). \end{aligned} $$

<figure><img src="image_13.png" /></figure>

We hence find that the closeness of the boundary and background state can be bounded via conditional Rényi-2 entropies of cuts. In particular, for large $K_1, K_2$, the recovery isometries can recover states to good accuracy, and we find that $\mathbb{E}\|\text{spec}_+(\rho_A) - \text{spec}_+(\phi_{\Gamma_A})\|$ is small. However, this result is not yet completely satisfying. The conditional Rényi-2 entropy is not a “robust” quantity, in the sense that a small deformation of $\phi$ can drastically change the values of the conditional Rényi-2 entropies in Eqs. (4.8) and (4.9). For this reason, we would like a condition with smoothed entropies. We first note that one can actually show that for the condition in Eq. (4.8), we can bound

$$ H_2(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi|\phi} \ge H_{\min}(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi} \quad (4.13) $$
and similarly for Eq. (4.9),

$$H_2(\Delta_A \setminus \Gamma_A | \Gamma_A R)_{\phi|\phi} \geq H_{\min}(\Delta_A \setminus \Gamma_A | \Gamma_A R)_{\phi} \quad (4.14)$$

To make the condition “robust,” we would like to replace these by smoothed entropies and express a condition in terms of $H_{\min}^{\epsilon}(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi}$ and $H_{\min}^{\epsilon}(\Delta_A \setminus \Gamma_A | \Gamma_A^c R)_{\phi}$. This will require simultaneous smoothing: finding a state $\phi_{VR}^{\epsilon} \in \mathcal{P}_{\le}(VR)$ which is close to $\phi$, such that $H_{\min}(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi^{\epsilon}} \ge H_{\min}^{\epsilon}(\Gamma_A \setminus \Delta_A | \Gamma_A^c R)_{\phi}$ and $H_{\min}(\Delta_A \setminus \Gamma_A | \Gamma_A^c R)_{\phi^{\epsilon}} \ge H_{\min}^{\epsilon}(\Delta_A \setminus \Gamma_A | \Gamma_A^c R)_{\phi}$ for all relevant cuts $\Delta_A$. If we have a general background state, it is not known how this can be done [25,31]. However, if the background state is actually a tensor product of link states, we can perform the simultaneous smoothing.

### 4.3. One Minimal Cut

The primary result in this subsection is Theorem 4.7, which states that if the background state is actually a tensor product of link states as in Eq. (2.2), then the spectrum of the boundary state is well approximated by the spectrum of the minimal cut link state in expectation, where the approximation accuracy is controlled by smooth one-shot entropies. It is a straightforward application of Theorem 4.4.

For a cut $\Gamma_A \in C(A)$ we define

$$C_1(\Gamma_A) = \{\Delta_A \in C(A) : \Delta_A \subsetneq \Gamma_A\}$$

$$C_2(\Gamma_A) = \{\Delta_A \in C(A) : \Gamma_A \subsetneq \Delta_A\}.$$

The key result we need is the following lemma, which we prove in “Appendix C,” which shows that if we have a link state, we can perform the desired joint smoothing.

**Lemma 4.5.** Let $\phi \in \mathcal{P}_{=}(V)$ be a link state, $A \subseteq V_{\partial}$ a boundary subsystem and $\Gamma_A \in C(A)$ a cut for A. Then, there exists a pure state $\phi^{\epsilon} \in \mathcal{P}_{\le}(V)$ which is such that

$$P(\phi, \phi^{\epsilon}) \le 2 \left( \sqrt{|C_1(\Gamma_A)|} + \sqrt{|C_2(\Gamma_A)|} \right) \sqrt{\epsilon}$$

and it holds that for any $\Delta_A \in C_1(\Gamma_A)$

$$H_{\min}(\Gamma_A \setminus \Delta_A | \Gamma_A^c)_{\phi^{\epsilon}} \ge H_{\min}^{\epsilon}(\Gamma_A \setminus \Delta_A | \Gamma_A^c)_{\phi}$$

and for any $\Delta_A \in C_2(\Gamma_A)$

$$H_{\min}(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi^{\epsilon}} \ge H_{\min}^{\epsilon}(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi}.$$

We now define the notion of a minimal cut for an arbitrary link state.

**Definition 4.6.** (Generalized minimal cut) A cut $\Gamma_A$ is an $(\epsilon, K)$-minimal cut if for all $\Delta_A \in C_1(\Gamma_A)$

$$H_{\min}^{\epsilon}(\Gamma_A \setminus \Delta_A | \Gamma_A^c)_{\phi} \ge K$$

and for all $\Delta_A \in C_2(\Gamma_A)$

$$H_{\min}^{\epsilon}(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi} \ge K.$$
This definition is consistent with the smooth entropy conditions for minimal surfaces in holography from [6]. The following is now a straightforward consequence of Theorem 4.4 and Lemma 4.5. It justifies our notion of a generalized minimal cut, as it controls the degree to which the spectrum of the corresponding cut link state $\phi_{\Gamma_A}$ is close to the boundary state $\rho_A$.

**Theorem 4.7.** Consider a random tensor network state $\rho$ constructed with $\phi \in P_+(V)$ a tensor product of link states as in Eq. (2.2). Let $A$ be a boundary region of the network, $\rho_A$ the corresponding boundary state, and $\Gamma_A$ an $(\varepsilon, K)$-minimal cut. Then, the spectra of $\rho_A$ and the state $\phi_{\Gamma_A}$ on $A$ are related as:

$$ \mathbb{E}\|\text{spec}_+(\rho_A) - \text{spec}_+(\phi_{\Gamma_A})\|_1 = \mathcal{O}(2^{-\frac{1}{4}K} + \sqrt{\varepsilon}). $$

*Proof.* Let $\phi^\varepsilon$ be a state as constructed in Lemma 4.5, and let $\rho^\varepsilon$ be the random tensor network state using this background state. Then, by Theorem 4.4

$$ \begin{aligned} \mathbb{E}\|\text{spec}_+(\rho_A^\varepsilon) - \text{spec}_+(\phi_{\Gamma_A}^\varepsilon)\|_1 & \le \mathbb{E}\min_{V_A, V_{\bar{A}}} \|(V_A \otimes V_{\bar{A}} \otimes I_R)\rho^\varepsilon(V_A^\dagger \otimes V_{\bar{A}}^\dagger \otimes I_R) - \phi^\varepsilon\|_1 \\ & = \mathcal{O}(\text{tr}[\phi]^{\frac{1}{4}}(2^{-\frac{1}{4}K_1} + 2^{-\frac{1}{4}K_2})) \end{aligned} $$

where $K_1$ is the minimal value over $\Delta_A \in \mathcal{C}_1(\Gamma_A)$ of

$$ \begin{aligned} H_2(\Gamma_A \setminus \Delta_A | \Gamma_A^c)_{\phi^\varepsilon | \phi^\varepsilon} & \ge H_{\min}(\Gamma_A \setminus \Delta_A | \Gamma_A^c)_{\phi^\varepsilon} - \log \text{tr}[\phi^\varepsilon] \\ & \ge H_{\min}^\varepsilon(\Gamma_A \setminus \Delta_A | \Gamma_A^c)_{\phi} - \log \text{tr}[\phi^\varepsilon] \end{aligned} $$

using Eq. (4.4), the defining property of $\phi^\varepsilon$ from Lemma 4.5 and accounting for the normalization. Similarly $K_2$ is the minimal value over $\Delta_A \in \mathcal{C}_2(\Gamma_A)$ of

$$ \begin{aligned} H_2(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi^\varepsilon | \phi^\varepsilon} & \ge H_{\min}(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi^\varepsilon} - \log \text{tr}[\phi^\varepsilon] \\ & \ge H_{\min}^\varepsilon(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi} - \log \text{tr}[\phi^\varepsilon] \end{aligned} $$

and hence $K_1 \ge K$ and $K_2 \ge K$, so

$$ \mathbb{E}\|\text{spec}_+(\rho_A^\varepsilon) - \text{spec}_+(\tilde{\phi}_{\Gamma_A}^\varepsilon)\|_1 = \mathcal{O}(2^{-\frac{1}{4}K}). $$

Moreover, $\|\phi - \phi^\varepsilon\|_1 \le 2T(\phi, \phi^\varepsilon) \le 2P(\phi, \phi^\varepsilon) = \mathcal{O}(\sqrt{\varepsilon})$ by Eq. (4.1) and hence by Lemma 4.3

$$ \mathbb{E}\|\rho - \rho^\varepsilon\|_1 = \mathcal{O}(\sqrt{\varepsilon}). $$

We conclude that

$$ \begin{aligned} \mathbb{E}\|\text{spec}_+(\rho_A) - \text{spec}_+(\phi_{\Gamma_A})\|_1 & \le \mathbb{E}\|\text{spec}_+(\rho_A^\varepsilon) - \text{spec}_+(\phi_{\Gamma_A}^\varepsilon)\|_1 \\ & \quad + \mathbb{E}\|\rho_A - \rho_A^\varepsilon\|_1 + \|\phi_{\Gamma_A} - \phi_{\Gamma_A}^\varepsilon\|_1 \\ & = \mathcal{O}(2^{-\frac{1}{4}K} + \sqrt{\varepsilon}). \end{aligned} $$

□
## 4.4. Two Competing Minimal Cuts

We now consider the case of two minimal cuts for A, where the link states do not have bounded spectral variation as in Sect. 3. We cannot directly apply Theorem 4.7 if there are two competing minimal cuts (note that we will need to define what this means exactly), nor can we assume that the empirical measure, or even a rescaling of it, will converge. Instead, we will see that the spectrum can be approximated in trace distance in a way that allows one to compute entropies, as well as showing convergence of certain measures depending on the spectrum of the reduced state. In particular, under these regularity conditions, we will prove the main result of this subsection: The distribution defined by the boundary state converges to the measure defined by the pushforward along the min-function acting on the distributions of the two competing minimal cuts. The intuition behind this is that the state on the edges can be approximated by a superposition of two states which both do have a unique minimal cut. As a corollary of this result, we will then show how to approximate the von Neumann entropy of the boundary state in such a situation.

We begin by introducing the relevant family of probability distributions for our purposes. Given a probability distribution vector $p \in \mathbb{R}^d$ of $d$ outcomes and $f(d) > 0$ and $g(d) \in \mathbb{R}$, consider the random variable which takes value $f(d)[-\log(p_i) - g(d)]$ with probability $p_i$. It has distribution

$$ \nu_p = \sum_{i=1}^{d} p_i \delta_{f(d)[-\log(p_i) - g(d)]}. \qquad (4.15) $$

Typically, we will have families of probability distributions with increasing $d$, let $f(d) = (\log d)^{-1}$ and choose $g(d)$ such that it corresponds to the entropy of $p$. We will also write $\nu_\rho = \nu_{\text{spec}(\rho)}$ for a quantum state $\rho$. We may also consider Eq. (4.15) for the case where $p \in \mathbb{R}^d$ is positive but normalized, in which case $\nu_p$ is a finite measure. To motivate the study of the distribution in Eq. (4.15), we note that it is closely related to the central limit theorem. Let $d = d_0^n$ and $\rho = \rho_0^{\otimes n}$ for some state $\rho_0$ on $\mathbb{C}^{d_0}$. Then,

$$ \nu_{\rho}^{(n)} = \sum_{\lambda \in \text{spec}(\rho_0^{\otimes n})} \lambda \delta_{\frac{1}{\sqrt{n}}[-\log(\lambda) - nH(\rho_0)]} $$

converges in distribution to a normal distribution by the central limit theorem. We study this particular measure because the empirical measures we investigated in Sect. 3 may not have good convergence properties if, for example, the full state on edges consists of many copies of a single non-maximally entangled link state. Moreover, the measure in Eq. (4.15) clearly captures information about the entropy of the probability distribution, and turns out to capture information about second-order asymptotics of information processing tasks [38, 72]. In fact, the example of many independent copies of a single link state is not the only relevant situation. In [14, 19], it was argued that the entanglement spectrum of conformal field theories with large central charge (which are the motivating example to study random tensor networks) have similar behavior.
Before diving into more technical details, we can build some intuition for how distributions of the form Eq. (4.15) will behave in the two-cut setting. Consider the situation with a single random tensor. Let us take a single bulk vertex $x$ and two boundary vertices $a$ and $b$, with edges $(xa)$ and $(xb)$. There is a single random tensor at $x$, and we take link states $|\phi_1\rangle^{\otimes n}$ along $(xa)$ and $|\phi_2\rangle^{\otimes n}$ along $(xb)$. We denote

$$|\phi_j\rangle = \sum_i \sqrt{\lambda_{i,j}} |ii\rangle$$

for $j = 1, 2$ and we let $h_j := H(\{\lambda_{i,j}\})$ be the entanglement entropies along the two minimal link states. There are two separating cuts for the boundary subsystem $\{a\}$: If $h_1 < h_2$, then $(xa)$ is the minimal cut, and if $h_1 > h_2$, the minimal cut is given by $(xb)$. In these cases, for large $n$, the entanglement spectrum of $\rho_{\{a\}}$ can be approximated by the entanglement spectrum along the minimal cut. What happens at the “phase transition” where $h_1 = h_2 = h$? The intuition is that we can split $|\phi_1\rangle^{\otimes n} \otimes |\phi_2\rangle^{\otimes n}$ into a superposition of the two states, one for which the minimal surface is at $(xa)$ and one for which the minimal surface is at $(xb)$. We find that in this case, if we let $\sigma_j^2 = \sum_i \lambda_{i,j} (\log(\frac{1}{\lambda_{i,j}}) - h)^2$, then for any bounded continuous function $f$, the quantity

$$\sum_{\lambda \in \text{spec}(\rho_{\{a\}})} \lambda f \left( \frac{-\log(\lambda) - nh}{\sqrt{n}} \right)$$

converges to

$$\frac{1}{2\pi\sigma_1\sigma_2} \iint e^{-\frac{(x_1-h)^2}{2\sigma_1^2} - \frac{(x_2-h)^2}{2\sigma_2^2}} f(\min(x_1, x_2))dx_1dx_2$$

in probability as $n$ goes to infinity. Our goal in this section will be to prove a general version of this result for full random tensor networks.

In Sect. 3, we used the method of moments. (If all moments of a distribution converge, and the distribution is uniquely determined by its moments, then we have weak convergence.) However, convergence of moments is a stronger condition than weak convergence, and it requires computation of all moments. In this section, we will use that for distributions of the form Eq. (4.15), convergence in distribution follows from convergence in trace norm:

**Lemma 4.8.** Consider a sequence of increasing integers $\{d_n\}_{n \in \mathbb{N}}$ and for each $n$, positive vectors $p^{(n)}, q^{(n)} \in \mathbb{R}^{d_n}$. Let $\sigma, h: \mathbb{N} \to \mathbb{R}$ be such that $\sigma(d) > 0$ for $d \in \mathbb{N}$ and $\lim_{d \to \infty} \sigma(d)^{-1} = 0$. Let

$$\nu_p^{(n)} := \sum_{i=1}^{d_n} p_i^{(n)} \delta_{\frac{1}{\sigma(d_n)}[-\log(p_i^{(n)}) - h(d_n)]}$$

and similarly let

$$\nu_q^{(n)} = \sum_{i=1}^{d_n} q_i^{(n)} \delta_{\frac{1}{\sigma(d_n)}[-\log(q_i^{(n)}) - h(d_n)]}.$$
1. Suppose $\|p^{(n)} - q^{(n)}\|_1$ goes to zero as $n$ goes to infinity, and $\nu_p^{(n)} \Rightarrow \nu$ for some probability distribution $\nu$. Then, $\nu_q^{(n)} \Rightarrow \nu$.

2. Suppose the vectors $q^{(n)}$ and $p^{(n)}$ are random, $\mathbb{E}\|p^{(n)} - q^{(n)}\|_1$ goes to zero as $n$ goes to infinity, and $\nu_p^{(n)} \Rightarrow \nu$ in probability. Then, $\nu_q^{(n)} \Rightarrow \nu$ in probability.

*Proof.* We need to show that

$$ \left| \int f(x) \mathrm{d}\nu_q^{(n)}(x) - \int f(x) \mathrm{d}\nu(x) \right| \to 0 $$

for any $f \in C_b(\mathbb{R})$. In fact, it suffices to show this for $f$ uniformly continuous (see, for instance, Theorem C.10 in [3]). Let $\varepsilon > 0$, then if we assume $f$ to be uniformly continuous, there exists $\delta > 0$ such that for any $x, y$ for which $|x - y| \le \delta$, it holds that $|f(x) - f(y)| \le \varepsilon$. We use a triangle inequality to bound

$$ \left| \int f(x) \mathrm{d}\nu_q^{(n)}(x) - \int f(x) \mathrm{d}\nu(x) \right| \le \left| \int f(x) \mathrm{d}\nu_q^{(n)}(x) - \int f(x) \mathrm{d}\nu_p^{(n)}(x) \right| + \left| \int f(x) \mathrm{d}\nu_p^{(n)}(x) - \int f(x) \mathrm{d}\nu(x) \right|. \quad (4.16) $$

Since $\nu_p^{(n)} \Rightarrow \nu$, the second term on the right-hand side vanishes as $n$ goes to infinity. If we write $g_n(x) = \frac{1}{\sigma(d_n)}(\log \frac{1}{x} - h(d_n))$, then the first term on the right-hand side of Eq. (4.16) is given by

$$ \left| \sum_{i=1}^{d_n} q_i^{(n)} f(g_n(q_i^{(n)})) - p_i^{(n)} f(g_n(p_i^{(n)})) \right|. $$

This can be bounded by

$$ \sum_{i=1}^{d_n} \left| q_i^{(n)} f(g_n(q_i^{(n)})) - p_i^{(n)} f(g_n(p_i^{(n)})) \right| \le \sum_{i=1}^{d_n} \left| q_i^{(n)} - p_i^{(n)} \right| \left| f(g_n(q_i^{(n)})) \right| + \sum_{i=1}^{d_n} \left| f(g_n(q_i^{(n)})) - f(g_n(p_i^{(n)})) \right| $$

In this expression, the first term is bounded by

$$ \sum_{i=1}^{d_n} \left| q_i^{(n)} - p_i^{(n)} \right| \left| f(g_n(q_i^{(n)})) \right| \le C \|q^{(n)} - p^{(n)}\|_1 \quad (4.17) $$
where $C$ is a uniform upper bound for $f$ (using $f \in C_b(\mathbb{R})$). For the second term, we partition the sum over $[d_n]$ into three sets

$$
\begin{align*}
I_1 &= \left\{ i \in [d_n] \text{ such that } 2^{-\delta\sigma(d_n)} \le \frac{p_i^{(n)}}{q_i^{(n)}} \le 2^{\delta\sigma(d_n)} \right\} \\
I_2 &= \left\{ i \in [d_n] \text{ such that } \frac{p_i^{(n)}}{q_i^{(n)}} > 2^{\delta\sigma(d_n)} \right\} \\
I_3 &= \left\{ i \in [d_n] \text{ such that } \frac{p_i^{(n)}}{q_i^{(n)}} < 2^{-\delta\sigma(d_n)} \right\}.
\end{align*}
$$

The idea is that for $i \in I_1$, $p_i$ and $q_i$ are sufficiently close that we may use the continuity of $f$, whereas $I_2$ and $I_3$ cannot have too much weight (using that $p_i^{(n)}$ and $q_i^{(n)}$ are close in trace distance). Let us now make this precise. For the sum over the elements in $I_1$, we have

$$ \sum_{i \in I_1} p_i^{(n)} \left| f(g_n(q_i^{(n)})) - f(g_n(p_i^{(n)})) \right| \le \sum_{i \in I_1} p_i^{(n)} \varepsilon \le \|p^{(n)}\|_1 \varepsilon, \quad (4.18) $$

using the uniform continuity of $f$ and the fact that for $i \in I_1$, we have $g(q_i^{(n)}) - g(p_i^{(n)}) = \frac{1}{\sigma(d_n)} \log\left(\frac{p_i^{(n)}}{q_i^{(n)}}\right)$, implying $|g(q_i^{(n)}) - g(p_i^{(n)})| \le \delta$ by the definition of $I_1$. Next, we observe that

$$
\begin{align*}
\|p^{(n)} - q^{(n)}\|_1 &\ge \sum_{i \in I_2} |p_i^{(n)} - q_i^{(n)}| = \sum_{i \in I_2} p_i^{(n)} \left(1 - \frac{q_i^{(n)}}{p_i^{(n)}}\right) \\
&\ge \sum_{i \in I_2} p_i^{(n)} \left(1 - 2^{-\delta\sigma(d_n)}\right),
\end{align*}
$$

and hence for $\sigma(d_n) \ge \delta^{-1}$, we have

$$ \sum_{i \in I_2} p_i^{(n)} \le 2 \|p^{(n)} - q^{(n)}\|_1. \quad (4.19) $$

In analogous fashion, we see that

$$
\begin{align*}
\|p^{(n)} - q^{(n)}\|_1 &\ge \sum_{i \in I_3, p_i^{(n)}>0} |p_i^{(n)} - q_i^{(n)}| = \sum_{i \in I_3, p_i^{(n)}>0} p_i^{(n)} \left( \frac{q_i^{(n)}}{p_i^{(n)}} - 1 \right) \\
&\ge \sum_{i \in I_3} p_i^{(n)} \left( 2^{\delta\sigma(d_n)} - 1 \right),
\end{align*}
$$

so for $\sigma(d_n) \ge \delta^{-1}$ we have

$$ \sum_{i \in I_3} p_i^{(n)} \le \|p^{(n)} - q^{(n)}\|_1. \quad (4.20) $$
In conclusion, for $\sigma(d_n) \ge \delta^{-1}$, collecting Eqs. (4.18), (4.19), (4.20) and using that $f$ is uniformly bounded by $C$, we can bound

$$ \sum_{i=1}^{d_n} p_i^{(n)} \left| f(g_n(q_i^{(n)})) - f(g_n(p_i^{(n)})) \right| \le \varepsilon \|p^{(n)}\|_1 + 3C \|p^{(n)} - q^{(n)}\|_1. $$

Together with Eq. (4.17), this implies that for $\sigma(d_n) \ge \delta$, we obtain the bound:

$$ \left| \int f(x) d\nu_q^{(n)}(x) - \int f(x) d\nu_p^{(n)}(x) \right| \le 4C \|q^{(n)} - p^{(n)}\|_1 + \varepsilon \|p^{(n)}\|_1. \quad (4.21) $$

Since $\nu_p^{(n)} \Rightarrow \nu$, $\|p^{(n)}\|_1 \to 1$, and since $\varepsilon > 0$ was arbitrary, we conclude that as $n$ goes to infinity

$$ \left| \int f(x) d\nu_q^{(n)}(x) - \int f(x) d\nu(x) \right| \to 0 $$

proving 1.

To prove 2, we note that by Markov's inequality, it suffices to show that

$$ \mathbb{E} \left| \int f(x) d\nu_q^{(n)}(x) - \int f(x) d\nu(x) \right| \to 0, \quad (4.22) $$

where $f \in C_b(\mathbb{R})$ is a uniformly continuous function. By Eq. (4.16), it suffices to show

$$ \mathbb{E} \left| \int f(x) d\nu_q^{(n)}(x) - \int f(x) d\nu_p^{(n)}(x) \right| \to 0. $$

Let $\varepsilon > 0$, and let $\delta$ such that if $|x - y| \le \delta$, $|f(x) - f(y)| \le \varepsilon$. Then by Eq. (4.21), for $\sigma(d_n) \ge \delta^{-1}$,

$$ \mathbb{E} \left| \int f(x) d\nu_q^{(n)}(x) - \int f(x) d\nu_p^{(n)}(x) \right| \le 4C \mathbb{E} \|q^{(n)} - p^{(n)}\|_1 + \varepsilon \mathbb{E} \|p^{(n)}\|_1. $$

Since $\varepsilon > 0$ was arbitrary, $\mathbb{E}\|q^{(n)} - p^{(n)}\|_1$ goes to zero, and $\mathbb{E}\|p^{(n)}\|_1$ goes to one, we conclude that Eq. (4.22) holds, proving 2. $\square$

The value of this result is clear: So long as we restrict ourselves to measures of the form Eq. (4.15), then we can prove convergence results by proving convergence of trace norms.

We will also need a basic lemma to help estimate overlaps of states.

**Lemma 4.9.** Suppose we have two bipartite pure states $\psi_{AB}, \phi_{AB} \in \mathcal{P}(AB)$. Then,

$$ \|\mathrm{tr}_B[|\psi\rangle\langle\phi|]\|_1 = F(\psi_B, \phi_B). $$

*Proof.* For any operator $M_A$ on $\mathcal{H}_A$ it holds that

$$ \|M_A\|_1 = \sup_{U_A} |\mathrm{tr}[U_A M_A]| $$
where the supremum is over unitary operators $U_A$ on $\mathcal{H}_A$, so

$$ \begin{aligned} \|\mathrm{tr}_B[|\psi\rangle\langle\phi|]\|_1 &= \sup_{U_A} |\mathrm{tr}[U_A \mathrm{tr}_B[|\psi\rangle\langle\phi|]]| \\ &= \sup_{U_A} |\mathrm{tr}[U_A \otimes I_B |\psi\rangle\langle\phi|]| = \sup_{U_A} |\langle\phi|U_A \otimes I_B |\psi\rangle| \end{aligned} $$

which equals $F(\psi_B, \phi_B)$ by Uhlmann's theorem. □

<figure><img src="image_14.png" /></figure>

With these tools in hand, let us now return to the random tensor network setting. Let $\Gamma_{A,1}$ and $\Gamma_{A,2}$ be two cuts with associated sets of edges $\gamma_{A,1}$ and $\gamma_{A,2}$. We will assume these two cuts are non-intersecting: $\gamma_{A,1} \cap \gamma_{A,2} = \emptyset$, and, without loss of generality $\Gamma_{A,1} \subsetneq \Gamma_{A,2}$. We will assume that the full state on edges is a tensor product of link states along the edges, and that the associated central limit measure for the spectrum along the cuts $\gamma_{A,1}$ and $\gamma_{A,2}$ converges to a continuous probability distribution. The most obvious application is where the link states on each edge $\phi_e$ are many copies of some single state $\phi_{e,0}$, so $\phi_e = (\phi_{e,0})^{\otimes n}$, in which case the spectrum is subject to a central limit theorem and the assumptions of Theorem 4.12 are satisfied.

We will now formalize what it means for these two cuts to be competing minimal cuts. We have fixed $\Gamma_{A,1}$ and $\Gamma_{A,2}$ with $\Gamma_{A,1} \subsetneq \Gamma_{A,2}$. Then, we consider three sets of cuts: $C_1(\Gamma_{A,1}, \Gamma_{A,2})$ is the collection of cuts strictly contained in $\Gamma_{A,1}$, $C_2(\Gamma_{A,1}, \Gamma_{A,2})$ is the collection of cuts which strictly contain $\Gamma_{A,2}$, and $C_3(\Gamma_{A,1}, \Gamma_{A,2})$ is the collection of cuts which are “in between” $\Gamma_{A,1}$ and $\Gamma_{A,2}$. That is,

$$ \begin{aligned} C_1(\Gamma_{A,1}, \Gamma_{A,2}) &= \{\Delta_A \in C(A) : \Delta_A \subsetneq \Gamma_{A,1}\} \\ C_2(\Gamma_{A,1}, \Gamma_{A,2}) &= \{\Delta_A \in C(A) : \Gamma_{A,2} \subsetneq \Delta_A\} \\ C_3(\Gamma_{A,1}, \Gamma_{A,2}) &= \{\Delta_A \in C(A) : \Gamma_{A,1} \subsetneq \Delta_A \subsetneq \Gamma_{A,2}\} \end{aligned} $$

and we let $C = C_1(\Gamma_{A,1}, \Gamma_{A,2}) \cup C_2(\Gamma_{A,1}, \Gamma_{A,2}) \cup C_3(\Gamma_{A,1}, \Gamma_{A,2})$. As in the single cut case, we would like to say that the surfaces $\Gamma_{A,1}$ and $\Gamma_{A,2}$ are minimal cuts if an appropriate set of conditional entropies are sufficiently large for all $\Delta_A \in C$. We formalize this as follows:

**Definition 4.10.** A pair of cuts $\Gamma_{A,1}$ and $\Gamma_{A,2}$ for $A$ is a pair of $(\varepsilon, K)$-minimal cuts if

$$ H_{\min}^{\varepsilon}(\Gamma_{A,1} \setminus \Delta_A | \Gamma_{A,1}^c) \geq K $$

for all cuts $\Delta_A \in C_1(\Gamma_{A,1}, \Gamma_{A,2})$

$$ H_{\min}^{\varepsilon}(\Delta_A \setminus \Gamma_{A,2} | \Gamma_{A,2}) \geq K $$

for all cuts $\Delta_A \in C_2(\Gamma_{A,1}, \Gamma_{A,2})$ and

$$ H_{\min}^{\varepsilon}(\Delta_A \setminus \Gamma_{A,1} | \Gamma_{A,1}) \geq K $$

$$ H_{\min}^{\varepsilon}(\Gamma_{A,2} \setminus \Delta_A | \Gamma_{A,2}^c) \geq K $$

for all cuts $\Delta_A \in C_3(\Gamma_{A,1}, \Gamma_{A,2})$.
We will need a joint smoothing result similar to Lemma 4.5 for the particular case where $\Gamma_{A,1} = A$ and $\Gamma_{A,2}^c = \bar{A}$. To this end we consider a graph $G = (V, E)$ with a set of boundary vertices $V_\partial$, and a boundary subsystem $A \subseteq V_\partial$. We denote by $\gamma_{A,1}$ the edges incident to $A$, and $\gamma_{A,2}$ the edges incident to $\bar{A}$, and assume these sets do not intersect. We let $E_b = E \setminus (\gamma_{A,1} \cup \gamma_{A,2})$. For a cut $\Delta_A \in C(A)$ we let $Y^{\Delta_A}$ be the set of half-edges

$$Y^{\Delta_A} = \{(e, x) : e = (xy), x \in \Delta_A^c, y \in A\}.$$

**Lemma 4.11.** Let $\phi \in \mathcal{P}_\le(V)$ be a pure background state which is of the form $\phi = \phi_{\gamma_{A,1}} \otimes \phi_{\gamma_{A,2}} \otimes \phi_{E_b}$, where

$$\phi_{E_b} = \bigotimes_{e \in E_b} \phi_e$$

is a product state and the $\phi_{\gamma_{A,i}}$ have a Schmidt decomposition in the standard basis along the half-edges. Then, there exists a state $\phi^\epsilon$ which is such that

$$P(\phi, \phi^\epsilon) \le 2\sqrt{2^{V_b}\epsilon}$$

and for all cuts $\Delta_A \in C(A)$ it holds that

$$H_{\min}(\Delta_A \setminus A|A)_{\phi^\epsilon} \ge H_{\min}^\epsilon(\Delta_A \setminus A|AY^{\Delta_A})_{\phi}.$$

To state the main result of this section, recall that given a measurable function $f: \mathcal{X} \to \mathcal{Y}$ between measure spaces, the pushforward of the function $f$ on a measure $\mu$ on $\mathcal{X}$ is defined by $(f_*(\mu))(A) = \mu(f^{-1})(A)$ for any measurable set $A \subseteq \mathcal{Y}$. We apply this to the function $\min: \mathbb{R} \times \mathbb{R} \to \mathbb{R}$ in the result:

**Theorem 4.12.** Consider a family of random tensor network states on a graph $G$ with pure state on edges $\phi$, indexed by an increasing sequence of positive integers $n$. We assume that $\Gamma_{A,1}, \Gamma_{A,2} \in C(A)$ are a pair of non-intersecting $(\epsilon(n), K(n))$-minimal cuts for all $n$ where $\epsilon(n) = O(n^{-\gamma})$ for $\gamma > 4$ and $K(n) = \Omega(\log(n)^2)$ as $n$ goes to infinity. We let $H: \mathbb{N} \to \mathbb{R}$, and we assume that

$$\nu_{\phi_{\Gamma_{A,i}}} = \sum_{\lambda \in \text{spec}(\phi_{\Gamma_{A,i}})} \lambda \delta_{\frac{1}{\sqrt{n}}[\log(\frac{1}{\lambda}) - H(n)]}$$

for $i = 1, 2$, is such that $\nu_{\phi_{\Gamma_{A,i}}} \Rightarrow \nu_i$, where $\nu_i$ is a probability distribution with a continuous cumulative distribution function. Then, $\nu_{\rho_A} \Rightarrow \min_*(\nu_1, \nu_2)$ in probability.

*Proof.* Proving this result will require several intermediate results. We provide a very high-level, enumerated sketch of our proof here, involving the following steps:

1. Study a reduced problem on a subnetwork; this subnetwork is such that the minimal cuts $\gamma_{A,i}$ are incident to the boundary.

2. Approximate the background state with superpositions of maximally entangled states by binning eigenvalues, and construct approximate tensor network states with the approximate background states.
<figure><img src="image_15.png" /><figcaption>(a) Consider a tensor network with a boundary region A with two competing minimal cuts.</figcaption></figure>

<figure><img src="image_16.png" /><figcaption>(b) We show that the spectrum is almost preserved when removing the boundary regions; that is, the spectrum of $\rho_A$ is approximated by that of $\sigma_B$.</figcaption></figure>

<figure><img src="image_17.png" /><figcaption>(c) The distribution of the logarithms of the eigenvalues has width of order $\sqrt{n}$. We approximate the spectrum of the state along the two minimal cuts by a superposition of maximally entangled states and discard the tails of the spectrum.</figcaption></figure>

<figure><img src="image_18.png" /></figure>

<figure><img src="image_19.png" /><figcaption>(d) We then discard the part of the state where the maximally entangled states along the two cuts are of almost equal dimension to get the approximate state on edges $|\phi\rangle$.</figcaption></figure>

<figure><img src="image_20.png" /><figcaption>(e) We decompose the background state as a superposition over $|\phi^{(J,a)}\rangle$ and $|\phi^{(J,b)}\rangle$. We denote the corresponding tensor network states by $\sigma^{(J,a)}$ and $\sigma^{(J,b)}$.</figcaption></figure>

FIGURE 5. Illustration of the proof of Theorem 4.12

3. Prove that the spectrum of the boundary state converges to the spectrum of the approximate tensor network state, which in turn converges to the spectrum of the approximate background states. We write the background state as a superposition of two states, one of which has $\gamma_{A,1}$
<figure><img src="image_21.png" /></figure>

(f) For the state $|\phi^{(j,a)}\rangle$, the minimal cut is $\gamma_{A,1}$, and along $\gamma_{A,2}$ we have a maximally entangled state, which gives $\sigma_B^{(j,a)} \approx \phi_B^{(j,a)}$. Similarly, for $|\phi^{(j,b)}\rangle$, the minimal cut is $\gamma_{A,2}$ and we get $\sigma_B^{(j,b)} \approx \phi_B^{(j,b)}$.

<figure><img src="image_22.png" /></figure>

(g) All the $\sigma_B^{(j,a)}$ have the same eigenbasis, so we can add the spectra. We can do the same for the $\sigma_B^{(j,b)}$, yielding $\sigma_B^{(a)}$ and $\sigma_B^{(b)}$, which has the same spectrum as $\sigma_B^{(b)}$. Finally we argue that the $\sigma_B^{(a)}$ and $\sigma_B^{(b)}$ are nearly orthogonal, so we can combine the spectra, as in Eq. (4.37). We complete the proof by showing that the resulting spectrum converges to the pushforward measure of the min function applied to the spectra of the two cuts.

<caption>FIGURE 5. (continued)</caption>

as its minimal cut, whereas the other state has $\gamma_{A,2}$ as its minimal cut. We show that the resulting states are approximately orthogonal.

4. Show that the distribution of the approximate background states converges to the min-distribution, and hence conclude that the spectrum of the boundary state converges to the min-distribution.

Figure 5 provides a more detailed visual sketch of the intuition behind our proof strategy. Lemma 4.8 will be a key tool, as it implies that it will suffice to show convergence in trace norm.

We assume without loss of generality that $\Gamma_{A,1} \subset \Gamma_{A,2}$. We now define the subnetwork that we will analyze in our proof. Let $G' = (V', E')$ be the induced graph on $V' = V_b' \cup V_\partial'$, where $V_b' = \Gamma_{A,2} \setminus \Gamma_{A,1}$, and $V_\partial' = B \cup \bar{B}$, with $B$ the set of vertices in $\Gamma_{A,1}$ which are incident to $V_b'$ and $\bar{B}$ the set of vertices in $V \setminus \Gamma_{A,2}$ which are incident to $V_b'$. The subgraph $G'$ is depicted in Fig. 5b.
We also define the random tensor network state $\tau$ as the state obtained by applying random tensors only on bulk vertices in the complement of $V'_b$. Then for this state, by a slight variation on Theorem 4.7, it holds that

$$ \mathbb{E}_{V_A, V_{\bar{A}}} \min \|(V_A \otimes V_{\bar{A}} \otimes I)\tau(V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger} \otimes I) - \phi\|_1 = \mathcal{O}(2^{-K(n)} + \sqrt{\varepsilon(n)}), $$

where the minimum is over isometries $V_A : \mathcal{H}_A \to \mathcal{H}_{\Gamma_{A,1}}$ and $V_{\bar{A}} : \mathcal{H}_{\bar{A}} \to \mathcal{H}_{\Gamma_{A,2}^c}$. Let $\tilde{\tau} = (V_A \otimes V_{\bar{A}} \otimes I)\tau(V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger} \otimes I)$ where the $V_A$ and $V_{\bar{A}}$ are the isometries that realize the minimum.

Now, consider two random tensor network states on $G'$ obtained by applying the same random tensors on $V'_b$ with background states $\tilde{\tau}$ and $\phi$, respectively. The state where we take $\tilde{\tau}$ as the background state yields $(V_A \otimes V_{\bar{A}} \otimes I)\rho(V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger} \otimes I)$. Denote the state where we take $\phi$ as the background state by $\sigma$. Then by Lemma 4.3:

$$ \mathbb{E}\|(V_A \otimes V_{\bar{A}})\rho(V_A^{\dagger} \otimes V_{\bar{A}}^{\dagger}) - \sigma\|_1 = \mathcal{O}(2^{-K(n)} + \sqrt{\varepsilon(n)}). $$

If we let $E_1$ denote the set of edges $(xy)$ for which both $x, y \in \Gamma_{A,1}$, and $E_2$ the set of edges $(xy)$ for which both $x, y \in \Gamma_{A,2}^c$, then $\sigma_{\Gamma_{A,1}} = \phi_{E_1} \otimes \sigma_B$ and $\sigma_{\Gamma_{A,2}} = \phi_{E_2} \otimes \sigma_{\bar{A}}$. This shows that

$$ \mathbb{E}\|\mathrm{spec}_+(\rho_A) - \mathrm{spec}_+(\sigma_B)\|_1 = \mathcal{O}(2^{-K(n)} + \sqrt{\varepsilon(n)}) \quad (4.23) $$

and $\mathrm{spec}_+(\sigma_B) = \mathrm{spec}_+(\sigma_{\bar{A}})$, because $\sigma$ is pure, which follows because its background state $\phi$ is pure. We will continue to study $\sigma$ on the reduced graph $G'$, as in Fig. 5b, and at the end of the proof, we will see that Eq. (4.23) will be sufficient to prove the desired properties of $\mathrm{spec}(\rho_A)$.

We have accomplished Step 1 by reducing the full network to a subnet-work, and we now try to construct an approximation to $\sigma$. We will do so by coarse-graining the spectrum of the background states along the two minimal cuts: slicing the tails of the distribution, binning the remaining eigenvalues, throwing away the smallest bins of the binned distribution, and then approxi-mating the states as a superposition of maximally entangled states defined on the bins. Consider the background states along the two minimal cuts in the Schmidt basis:

$$ |\phi_{\gamma_{A,i}}\rangle = \sum_J \sqrt{\lambda_{i,J}} |JJ\rangle. \quad (4.24) $$

Here, the $|J\rangle$ are a tensor product basis along the half-edges (which we again may take to be the standard basis), so that

$$ |JJ\rangle = \bigotimes_{e=(xy) \in \gamma_{A,i}} |i_{e,x}\rangle \otimes |i_{e,y}\rangle, $$

where the $|i_{e,x}\rangle$ and $|i_{e,y}\rangle$ are a basis for $\mathcal{H}_{e,x}$ and $\mathcal{H}_{e,y}$. First, we truncate the allowed range of eigenvalues by slicing off the tails of the distribution, as in the left side of Fig. 5c. Let

$$ I_n = [2^{-H(n)} - C\sqrt{n \log(n)} , 2^{-H(n)} + C\sqrt{n \log(n)}] $$
for some constant C, and let

$$|\phi_{\gamma_{A,i}}^{(1)}\rangle = \sum_{\lambda_{i,J} \in I_n} \sqrt{\lambda_{i,J}} |JJ\rangle.$$

Note that the entanglement spectrum of $\phi_{\gamma_{A,i}}$ is given by the spectrum of $\phi_{\Gamma_{A,i}}$. This implies that

$$\sum_{\lambda_{i,J} \notin I_n} \lambda_{i,J} = \nu_{\phi_{\Gamma_{A,i}}} ((-\infty, -C \log(n)) \cup (C \log(n), \infty)) \to 0$$

and hence

$$\|\phi_{\gamma_{A,i}} - \phi_{\gamma_{A,1}}^{(1)}\|_1 \to 0.$$

Next, for $\lambda_{i,J} \in I_n$, we define new $\tilde{\lambda}_{i,J}$ according to $\log(\tilde{\lambda}_{i,J}) = \frac{1}{n^\alpha}[n^\alpha \log(\lambda_{i,J})]$, effectively binning the values of $\log(\lambda_{i,J})$ into intervals of size $n^{-\alpha}$, as in the right side of Fig. 5c. We will choose $\alpha > 0$ small (but other choices will be useful for Corollary 4.14); to be precise, we choose $\alpha < \frac{1}{8}(\gamma - 4)$. We can now define the background state

$$|\phi_{\gamma_{A,i}}^{(2)}\rangle = \sum_{\lambda_{i,J} \in I_n} \sqrt{\lambda_{i,J}} |JJ\rangle.$$

Then by Lemma C.4

$$\|\phi_{\gamma_{A,i}}^{(1)} - \phi_{\gamma_{A,i}}^{(2)}\|_1 \le 2\sqrt{\sum_J |\lambda_{i,J} - \tilde{\lambda}_{i,J}|},$$

which we may bound using the fact that $2^{-\frac{1}{n^\alpha}} \le \frac{\tilde{\lambda}_{i,J}}{\lambda_{i,J}} \le 1$, so

$$\sum_J |\lambda_{i,J} - \tilde{\lambda}_{i,J}| = \sum_J \lambda_{i,J} \left(1 - \frac{\tilde{\lambda}_{i,J}}{\lambda_{i,J}}\right) \le \max_J \left(1 - \frac{\tilde{\lambda}_{i,J}}{\lambda_{i,J}}\right) \\ \le 1 - 2^{-\frac{1}{n^\alpha}} = \mathcal{O}\left(\frac{1}{n^\alpha}\right).$$

Thus, $\|\phi_{\gamma_{A,i}}^{(1)} - \phi_{\gamma_{A,i}}^{(2)}\|_1 = \mathcal{O}(n^{-\frac{1}{2}\alpha})$. Since the interval $I_n$ has length $\mathcal{O}(\sqrt{n} \log(n))$ and the distinct values $\tilde{\lambda}_{i,J}$ are $n^{-\alpha}$ apart, the $\tilde{\lambda}_{i,J}$ take $\mathcal{O}(n^{\alpha+\frac{1}{2}} \log(n))$ different values. Denote these values by $p_{i,j}$, and let $d_{i,j}$ be their multiplicities. Setting

$$q_{i,j} = d_{i,j} p_{i,j},$$

we can rewrite the state $|\phi_{\gamma_{A,i}}^{(2)}\rangle$ using the collected eigenvalues:

$$|\phi_{\gamma_{A,i}}^{(2)}\rangle = \sum_j \sqrt{q_{i,j}} |\Phi_{i,j}^{+}\rangle,$$

where the $|\Phi_{i,j}^{+}\rangle$ are maximally entangled states of dimension $d_{i,j}$ which are orthogonal, i.e., $\langle\Phi_{i,j}^{+}|\Phi_{i,k}^{+}\rangle = \delta_{j,k}$. Note that $0 \le q_{i,j} \le 1$ and $\sum_j q_{i,j} \le 1$.
Now, we discard any bins that are too small: Let $\beta > \alpha + \frac{1}{2}$ and consider the state

$$|\phi_{\gamma_{A,i}}^{(3)}\rangle = \sum_{q_{i,j} > n^{-\beta}} \sqrt{q_{i,j}} |\Phi_{i,j}^{+}\rangle \quad (4.25)$$

where we restricted the sum to terms for which $q_{i,j}$ is sufficiently large. (And hence $p_{i,j}$ will be sufficiently close to $d_{i,j}^{-1}$.) Then, since the number of terms is $O(n^{\alpha+\frac{1}{2}} \log(n))$ and using Lemma C.4, we have

$$\|\phi_{\gamma_{A,i}}^{(2)} - \phi_{\gamma_{A,i}}^{(3)}\|_1 = O\left(n^{\frac{1}{2}\alpha + \frac{1}{4} - \frac{1}{2}\beta} \sqrt{\log(n)}\right)$$

To summarize, $\phi_{\gamma_{A,i}}^{(3)}$ is the state obtained from the original background state $\phi_{\gamma_{A,i}}$ by 1) removing the tails of the spectrum, 2) binning the eigenvalues, and finally 3) dropping any of the bins that are too small. The first approximation incurs an error $\|\phi_{\gamma_{A,i}} - \phi_{\gamma_{A,i}}^{(1)}\|_1$, which converges to zero, and the second and third approximations incur errors of order $O(n^{-\frac{1}{2}\alpha})$ and $O(n^{\frac{1}{2}\alpha+\frac{1}{4}-\frac{1}{2}\beta} \sqrt{\log(n)})$, respectively.

Now, let $\tilde{\phi}$ be the background state for which we have replaced $\phi_{\gamma_{A,i}}$ by $\phi_{\gamma_{A,i}}^{(3)}$ for $i=1,2$. Recall that $\sigma$ is the state on the random tensor network state constructed with background state $\phi$ on the subgraph $G'$, as in Fig. 5b. We then define the approximation $\tilde{\sigma}$ to be the tensor network state on $G'$ which uses $\tilde{\phi}$ as its background state instead of $\phi$. With these background states, we see

$$\|\phi - \tilde{\phi}\|_1 = O\left(\|\phi_{\gamma_{A,i}} - \phi_{\gamma_{A,i}}^{(1)}\|_1 + n^{-\frac{1}{2}\alpha} + n^{\frac{1}{2}\alpha + \frac{1}{4} - \frac{1}{2}\beta} \sqrt{\log(n)}\right) \to 0. \quad (4.26)$$

We then apply Lemma 4.3 to find:

$$\mathbb{E}\|\sigma - \tilde{\sigma}\|_1 = O\left(\|\phi - \tilde{\phi}\|_1\right) \to 0. \quad (4.27)$$

We now make one final approximation to $\sigma$, in which we discard the parts of the background state where the maximally entangled states along each cut are close in dimension, as in Fig. 5d. Consider the state

$$|\bar{\phi}_{\gamma_{A,1}, \gamma_{A,2}}\rangle = \sum_{2^{n^{1/4}} p_{2,k} \le p_{2,j} \text{ or } 2^{-n^{1/4}} p_{2,k} \ge p_{2,j}} \sqrt{q_{1,k} q_{2,j}} |\Phi_{1,k}\rangle \otimes |\Phi_{2,j}\rangle,$$

where the sum is still only over those $j$ and $k$ for which $q_{1,k} > n^{-\beta}$ and $q_{2,j} > n^{-\beta}$. If we let

$$D_n = \{(x, y) \in \mathbb{R}^2 : x - n^{-\frac{1}{4}} - n^{-\frac{1}{2}} \le y \le x + n^{-\frac{1}{4}} + n^{-\frac{1}{2}}, |x| \le \log(n) + 1\},$$
then as $n$ increases, the measure of $D_n$ converges to zero and since the measures $\nu_{\phi_{\gamma_{A,i}}} \Rightarrow \nu_i$ and $\nu_i$ has continuous cumulative distribution function

$$\sum_{2^{-n^{1/4}} p_{1,j} \le p_{2,k} \le 2^{n^{1/4}} p_{1,j}} q_{1,j} q_{2,k} \le (\nu_{\phi_{\Gamma_{A,1}}} \times \nu_{\phi_{\Gamma_{A,2}}}) (D_n) \to 0. \quad (4.28)$$
Hence, if we let $\bar{\phi}$ denote the background state with $\tilde{\phi}_{\gamma_{A,1}} \otimes \tilde{\phi}_{\gamma_{A,2}}$ replaced by $\tilde{\phi}_{\gamma_{A,1},\gamma_{A,2}}$, we get that $\|\bar{\phi} - \tilde{\phi}\|_1 \to 0$. By Lemma 4.3, if we denote by $\bar{\sigma}$ the state we obtain on $G'$ by using $\bar{\phi}$ rather than $\tilde{\phi}$ as the background state, we get

$$ \mathbb{E}\|\bar{\sigma} - \sigma\|_1 \to 0. \qquad (4.29) $$

We pause here to note that we have accomplished Step 2: We have constructed an approximation $\bar{\sigma}$ to $\sigma$ by approximating the background state along the cuts as superpositions of maximally entangled states. The utility in doing so is that working with this approximated tensor network state allows us to reduce to calculations where we restrict to a maximally entangled state along one of the two surfaces. Our next major step is to then show that the spectrum of $\bar{\sigma}$ can be used to approximate the spectrum of $\rho$, which will then allow us to analyze the convergence of the corresponding distribution. As a first intermediate step, we will show that $\bar{\sigma}$ can be approximated as a superposition of a state with minimal cut $\gamma_{A,1}$ and a state with minimal cut $\gamma_{A,2}$. This will allow us to more easily reason about how the background states are related to the spectrum of $\bar{\sigma}$, in turn, $\sigma$, and in turn, $\rho_A$.

Let us write

$$ |\phi_{\gamma_{A,1}, \gamma_{A,2}}^{(j,a)}\rangle = \sum_{k \text{ s.t. } p_{1,k} \ge p_{2,j} \ge 2^{n^{1/4}}} \sqrt{q_{1,k}q_{2,j}} |\Phi_{1,k}^{+}\rangle \otimes |\Phi_{2,j}^{+}\rangle $$

$$ |\phi_{\gamma_{A,1}, \gamma_{A,2}}^{(j,b)}\rangle = \sum_{k \text{ s.t. } p_{2,k} \ge p_{1,j} \ge 2^{n^{1/4}}} \sqrt{q_{1,j}q_{2,k}} |\Phi_{1,j}^{+}\rangle \otimes |\Phi_{2,k}^{+}\rangle, $$

allowing us to write the background state $\bar{\phi}_{\gamma_{A,1}, \gamma_{A,2}}$ as a different superposition, as depicted in Fig. 5e:

$$ |\bar{\phi}_{\gamma_{A,1}, \gamma_{A,2}}\rangle = \sum_j |\phi_{\gamma_{A,1}, \gamma_{A,2}}^{(j,a)}\rangle + \sum_j |\phi_{\gamma_{A,1}, \gamma_{A,2}}^{(j,b)}\rangle. $$

Let $|\phi^{(j,a)}\rangle$ and $|\phi^{(j,b)}\rangle$ denote the background states on $G'$ where we have replaced $|\bar{\phi}_{\gamma_{A,1}, \gamma_{A,2}}\rangle$ by $|\phi_{\gamma_{A,1}, \gamma_{A,2}}^{(j,a)}\rangle$ and $|\phi_{\gamma_{A,1}, \gamma_{A,2}}^{(j,b)}\rangle$, respectively, and let

$$ |\phi^a\rangle = \sum_j |\phi^{(j,a)}\rangle, \quad |\phi^b\rangle = \sum_j |\phi^{(j,b)}\rangle. $$

Denote by $|\sigma^{(j,a)}\rangle$, $|\sigma^{(j,b)}\rangle$ the random tensor network states on $G'$ with background states $|\phi^{(j,a)}\rangle$ and $|\phi^{(j,b)}\rangle$, respectively. Similarly, denote by $|\sigma^{(a)}\rangle$ and $|\sigma^{(b)}\rangle$ the random tensor network states on $G'$ with background states $|\phi^{(a)}\rangle$ and $|\phi^{(b)}\rangle$, respectively.
We start with the following bound on the rank of $\sigma_B^{(j,a)}$:

$$ 
\begin{aligned}
\mathrm{rank}(\sigma_B^{(j,a)}) &\le \mathrm{rank}(\phi_B^{(j,a)}) \\
&\le \sum_{p_{1,k} \ge p_{2,j} 2^{n^{1/4}}} d_{1,k} \\
&\le \sum_{p_{1,k} \ge p_{2,j} 2^{n^{1/4}}} \frac{q_{1,k}}{p_{1,k}} \\
&\le \sum_k \frac{q_{1,k} 2^{-n^{1/4}}}{p_{2,j}} \\
&\le \frac{2^{-n^{1/4}}}{p_{2,j}}
\end{aligned} 
\quad (4.30) $$

By the same reasoning we may bound the rank of $\sigma_{\bar{B}}^{(j,b)}$ as

$$ \mathrm{rank}(\sigma_{\bar{B}}^{(j,b)}) \le \frac{2^{-n^{1/4}}}{p_{1,j}}. \quad (4.31) $$

Now, we will argue that the state $\sigma^{(j,a)}$ has minimal cut $\gamma_{A,1}$, and $\sigma^{(j,b)}$ has minimal cut $\gamma_{A,2}$, as in Fig. 5f. Intuitively, it is sensible that for $\sigma^{(j,a)}$ the unique minimal cut is along $\gamma_{A,1}$, as for $\phi^{(j,a)}$, we have a fixed maximally entangled state along $\gamma_{A,2}$, and a superposition of maximally entangled states of lower dimension along $\gamma_{A,1}$. Similarly, for $\sigma^{(j,b)}$ the minimal cut is along $\gamma_{A,2}$. To confirm this intuition, we will now show that $\sigma_B^{(j,a)} \approx \phi_B^{(j,a)}$ and $\sigma_{\bar{B}}^{(j,b)} \approx \phi_{\bar{B}}^{(j,b)}$.

We show this for $\sigma_B^{(j,a)}$. In this case, the “minimal” cut is simply $B$. Let $\Delta_B$ be a cut for $B$ unequal to $B$ or to $V'_b \cup B$. We denote by $\Delta_A$ the associated minimal cut for $A$ on the original graph $G$ given by $\Delta_A = \Delta_B \cup \Gamma_{A,1}$. We let

$$ Y^{\Delta_B} = \{(e, x) : e = (xy), x \in \Delta_B^c, y \in B\}. $$

Note that as $\phi$ is a product state we have $H_{\mathrm{min}}^{\varepsilon}(\Delta_B \setminus B | B)_{\phi} = H_{\mathrm{min}}^{\varepsilon}(\Delta_B \setminus B | B Y^{\Delta_B})_{\phi}$. We can obtain $\phi^{(j,a)}$ from $\phi$ by acting with subunital CP maps on $B$ and $\bar{B}$ and therefore (by two applications of data processing)

$$ 
\begin{aligned}
H_{\mathrm{min}}^{\varepsilon}(\Delta_B \setminus B | BY^{\Delta_B})_{\phi^{(j,a)}} &\ge H_{\mathrm{min}}^{\varepsilon}(\Delta_B \setminus B | BY^{\Delta_B})_{\phi} = H_{\mathrm{min}}^{\varepsilon}(\Delta_B \setminus B | B)_{\phi} \\
&\ge H_{\mathrm{min}}^{\varepsilon}(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi}
\end{aligned}
 $$

We now consider $\Delta_B = V'_b \cup B$ (in which case $Y^{\Delta_B}$ is empty, since we assume $\gamma_{A,1} \cap \gamma_{A,2} = \emptyset$). Then,

$$ H_{\mathrm{min}}^{\varepsilon}(\Delta_B \setminus B | B)_{\phi^{(j,a)}} \ge H_{\mathrm{min}}(\Delta_B \setminus B | B)_{\phi^{(j,a)}} = H_{\mathrm{min}}(\bar{B})_{\phi^{(j,a)}} - H_{\mathrm{max}}(B)_{\phi^{(j,a)}} $$

using the product structure of $\phi^{(j,a)}$. Now, we compute

$$ H_{\mathrm{min}}(\bar{B})_{\phi^{(j,a)}} = -\log(\|\phi_{\bar{B}}^{(j,a)}\|_{\infty}) \ge -\log(p_{2,j}), $$
where we recall that $p_{2,j}$ is a binned eigenvalue. By Eq. (4.30), we can bound

$$H_{\max}(B)_{\phi^{(j,a)}} \le \log(\mathrm{rank}(\phi_B^{(j,a)})) \le \log\left(\frac{2^{-n^{1/4}}}{p_{2,j}}\right) = -\log(p_{2,j}) - n^{1/4}.$$

In conclusion,

$$H_{\min}^{\varepsilon}(\Delta_B \setminus B | B)_{\phi^{(j,a)}} \ge n^{1/4}.$$

By Lemma 4.11, we can find $\phi^{(\varepsilon,j,a)}$ such that $P(\phi^{(j,a)}, \phi^{(\varepsilon,j,a)}) = \mathcal{O}(\sqrt{\varepsilon})$ and for all cuts $\Delta_B \ne B$ we have

$$H_{\min}(\Delta_B \setminus B | B)_{\phi^{(\varepsilon,j,a)}} \ge H_{\min}^{\varepsilon}(\Delta_B \setminus B | BY^{\Delta_B})_{\phi^{(j,a)}}$$

and hence for $\Delta_B \ne V'_b \cup B$

$$H_{\min}(\Delta_B \setminus B | B)_{\phi^{(\varepsilon,j,a)}} \ge H_{\min}^{\varepsilon}(\Delta_A \setminus \Gamma_A | \Gamma_A)_{\phi}$$

and for $\Delta_B = V'_b \cup B$

$$H_{\min}(\Delta_B \setminus B | B)_{\phi^{(\varepsilon,j,a)}} \ge n^{1/4}.$$

Therefore, Proposition 4.1 allows us to conclude that if we let $\sigma^{(\varepsilon,j,a)}$ denote the random tensor network state with background state $\phi^{(\varepsilon,j,a)}$, then

$$\mathbb{E}\|\sigma_B^{(\varepsilon,j,a)} - \phi_B^{(\varepsilon,j,a)}\|_1 = \mathcal{O}\left(2^{-\frac{1}{2}K(n)} + 2^{-\frac{1}{2}n^{\frac{1}{4}}}\right),$$

and by Lemma 4.3 and the fact that $T(\phi^{(j,a)}, \phi^{(\varepsilon,j,a)}) \le P(\phi^{(j,a)}, \phi^{(\varepsilon,j,a)})$ this implies

$$\begin{aligned} \mathbb{E}\|\sigma_B^{(j,a)} - \phi_B^{(j,a)}\|_1 &\le \mathbb{E}\|\sigma_B^{(\varepsilon,j,a)} - \phi_B^{(\varepsilon,j,a)}\|_1 \\ &\quad + \mathbb{E}\|\sigma_B^{(\varepsilon,j,a)} - \sigma_B^{(j,a)}\|_1 + \|\phi_B^{(\varepsilon,j,a)} - \phi_B^{(j,a)}\|_1 \\ &= \mathcal{O}\left(2^{-\frac{1}{2}K(n)} + 2^{-\frac{1}{2}n^{\frac{1}{4}}} + \sqrt{\varepsilon(n)}\right). \end{aligned}$$

It follows that

$$\begin{aligned} \mathbb{E}\|\sigma_B^{(a)} - \phi_B^{(a)}\|_1 &\le \sum_j \mathbb{E}\|\sigma_B^{(j,a)} - \phi_B^{(j,a)}\|_1 \\ &= \mathcal{O}\left(n^{\alpha+\frac{1}{2}}\log(n)\left(2^{-\frac{1}{2}K(n)} + 2^{-\frac{1}{2}n^{\frac{1}{4}}} + \sqrt{\varepsilon(n)}\right)\right) \to 0 \end{aligned} \quad (4.32)$$

using that the number of terms is $\mathcal{O}(n^{\alpha+\frac{1}{2}}\log(n))$. This expression goes to zero since we assume $K(n) = \Omega(\log(n)^2)$ and $\varepsilon(n) = \mathcal{O}(n^{-\gamma})$. A completely symmetric argument shows that

$$\mathbb{E}\|\sigma_B^{(j,b)} - \phi_B^{(j,b)}\|_1 = \mathcal{O}\left(2^{-\frac{1}{2}K(n)} + 2^{-\frac{1}{2}n^{\frac{1}{4}}} + \sqrt{\varepsilon(n)}\right) \quad (4.33)$$

and hence

$$\mathbb{E}\|\sigma_B^{(b)} - \phi_B^{(b)}\|_1 = \mathcal{O}(n^{\alpha+\frac{1}{2}}\log(n)(2^{-\frac{1}{2}K(n)} + 2^{-\frac{1}{2}n^{\frac{1}{4}}} + \varepsilon(n))) \to 0. \quad (4.34)$$

We have hence shown that $\sigma_B^{(j,a)} \approx \phi_B^{(j,a)}$ and $\sigma_B^{(j,b)} \approx \phi_B^{(j,b)}$ in expectation.
We now show that we can approximate the state $\bar{\sigma}_B$ on $G'$ by the sum of these states. We first claim that we can sum over the $j$ index to obtain the $\sigma_B^{(a)}$ and $\sigma_B^{(b)}$. To see this, we introduce some notation: Given a self-adjoint matrix $X$, let us write $\text{supp}(X)$ for the image, or support, of $X$. In other words, $\text{supp}(X)$ is the space spanned by the eigenvectors of $X$ with nonzero eigenvalue. We let $\mathcal{H}_{B,j}$ be the support of the reduced state of $|\Phi_{1,j}^+\rangle$ on the $B$ system, and we similarly let $\mathcal{H}_{\bar{B},j}$ be the support of the reduced state of $|\Phi_{2,j}^+\rangle$ on the $\bar{B}$ system. Then for $j \neq k$, the subspace $\mathcal{H}_{B,j}$ is orthogonal to $\mathcal{H}_{B,k}$ and similarly $\mathcal{H}_{\bar{B},j}$ is orthogonal to $\mathcal{H}_{\bar{B},k}$. By construction, it is clear that $\text{supp}(\sigma_B^{(j,a)}) \subseteq \mathcal{H}_{\bar{B},j}$ and $\text{supp}(\sigma_B^{(j,b)}) \subseteq \mathcal{H}_{B,j}$. This orthogonality for indices $j \neq k$ then makes it clear that we can sum the reduced states, as in Fig. 5g:

$$ \sigma_B^{(a)} = \sum_j \sigma_B^{(j,a)}, \quad \sigma_B^{(b)} = \sum_j \sigma_B^{(j,b)}, $$

and by the purity of $\sigma^{(b)}$, we have that $\sigma_B^{(b)}$ has the same spectrum as $\sigma_B^{(b)}$, We remind the reader that the (a) and (b) indices indicate that the minimal cut for the state is given by $\gamma_{A,1}$ and $\gamma_{A,2}$, respectively. Naturally, this also holds for the summed states, by orthogonality of the summands.

We now claim that $\bar{\sigma}_B \approx \sigma_B^{(a)} + \sigma_B^{(b)}$, i.e., the spectrum of the approximate state on $G'$, as in Eq. (4.29), is well approximated by the sum of two states with differing minimal cuts. We estimate their difference by

$$ \begin{aligned} \mathbb{E}\|\sigma_B^{(a)} + \sigma_B^{(b)} - \bar{\sigma}_B\|_1 &= \mathbb{E}\left\|\sum_{j,k} \text{tr}_{\bar{B}}\left[|\sigma^{(j,a)}\rangle\langle\sigma^{(k,b)}| + |\sigma^{(k,b)}\rangle\langle\sigma^{(j,a)}|\right]\right\|_1 \\ &\le 2 \sum_{j,k} \mathbb{E}\left\|\text{tr}_{\bar{B}}\left[|\sigma^{(j,a)}\rangle\langle\sigma^{(k,b)}|\right]\right\|_1 \\ &= 2 \sum_{j,k} \mathbb{E}F(\bar{\sigma}_{\bar{B}}^{(j,a)}, \bar{\sigma}_{\bar{B}}^{(k,b)}) \end{aligned} $$

by Lemma 4.9. Now, if $\rho$, $\sigma_1$ and $\sigma_2$ are positive operators, then by Lemma B.9 in [34], we have

$$ |F(\rho, \sigma_1) - F(\rho, \sigma_2)| \le \sqrt{\|\sigma_1 - \sigma_2\|_1 \text{tr}[\rho]}. $$

So, we find that

$$ \begin{aligned} \mathbb{E}F(\sigma_{\bar{B}}^{(j,a)}, \sigma_{\bar{B}}^{(k,b)}) &\le \mathbb{E}\left|F(\sigma_{\bar{B}}^{(j,a)}, \sigma_{\bar{B}}^{(k,b)}) - F(\sigma_{\bar{B}}^{(j,a)}, \phi_{\bar{B}}^{(k,b)})\right| + \mathbb{E}F(\sigma_{\bar{B}}^{(j,a)}, \phi_{\bar{B}}^{(k,b)}) \\ &\le \mathbb{E}\sqrt{\text{tr}[\sigma_{\bar{B}}^{(j,a)}]\|\sigma_{\bar{B}}^{(k,b)} - \phi_{\bar{B}}^{(k,b)}\|_1} + \mathbb{E}F(\sigma_{\bar{B}}^{(j,a)}, \phi_{\bar{B}}^{(k,b)}) \\ &\le \sqrt{\mathbb{E}\text{tr}[\sigma_{\bar{B}}^{(j,a)}]} \sqrt{\mathbb{E}\|\sigma_{\bar{B}}^{(k,b)} - \phi_{\bar{B}}^{(k,b)}\|_1} + \mathbb{E}F(\sigma_{\bar{B}}^{(j,a)}, \phi_{\bar{B}}^{(k,b)}), \end{aligned} $$

where we used Cauchy–Schwarz in the last step. For the first term, we may use Eq. (4.33) and $\mathbb{E}\text{tr}[\bar{\sigma}_{\bar{B}}^{(j,a)}] \le 1$ to see

$$ \sqrt{\mathbb{E}\text{tr}[\sigma_{\bar{B}}^{(j,a)}]} \sqrt{\mathbb{E}\|\sigma_{\bar{B}}^{(k,b)} - \phi_{\bar{B}}^{(k,b)}\|_1} = \mathcal{O}(2^{-\frac{1}{4}K(n)} + 2^{-\frac{1}{4}n^{\frac{1}{4}}} + (\varepsilon(n))^{\frac{1}{4}}). $$
For the second term we use a basic estimate on the fidelity: If $\rho$ and $\sigma$ are positive operators, then

$$ F(\rho, \sigma) = \|\sqrt{\rho}\sqrt{\sigma}\|_1 \le \|\sqrt{\rho}\|_1 \|\sqrt{\sigma}\|_{\infty} \\ \le \sqrt{\mathrm{rank}(\rho)} \|\sqrt{\rho}\|_2 \|\sqrt{\sigma}\|_{\infty} = \sqrt{\mathrm{rank}(\rho) \mathrm{tr}[\rho]} \|\sigma\|_{\infty}, $$

which follows by Hölder's inequality and the standard relation between Schatten 1 and 2-norms. Then, the second term can be estimated as follows: Write $P_{\tilde{B},j}$ for the projection onto $\mathcal{H}_{\tilde{B},j}$, then

$$ \begin{aligned} F(\sigma_{\tilde{B}}^{(j,a)}, \phi_{\tilde{B}}^{(k,b)}) &= F(\sigma_{\tilde{B}}^{(j,a)}, P_{\tilde{B},j} \phi_{\tilde{B}}^{(k,b)} P_{\tilde{B},j}) \\ &\le \sqrt{\mathrm{tr}[\sigma_{\tilde{B}}^{(j,a)}] \mathrm{rank}(\sigma_{\tilde{B}}^{(j,a)})} \|P_{\tilde{B},j} \phi_{\tilde{B}}^{(k,b)} P_{\tilde{B},j}\|_{\infty} \\ &\le \sqrt{\mathrm{tr}[\sigma_{\tilde{B}}^{(j,a)}] \frac{2^{-n^{1/4}}}{p_{2,j}} p_{2,j}} \\ &\le \sqrt{\mathrm{tr}[\sigma_{\tilde{B}}^{(j,a)}] 2^{-n^{1/4}}} \end{aligned} $$

using Eq. (4.30) and $\|P_{\tilde{B},j} \phi_{\tilde{B}}^{(k,b)} P_{\tilde{B},j}\|_{\infty} \le p_{2,j}$. Thus

$$ \mathbb{E}F(\sigma_{\tilde{B}}^{(j,a)}, \phi_{\tilde{B}}^{(k,b)}) \le \sqrt{\mathbb{E} \mathrm{tr}[\sigma_{\tilde{B}}^{(j,a)}] 2^{-n^{1/4}}} \le 2^{-\frac{1}{2}n^{1/4}} $$

and we may estimate

$$ \mathbb{E}F(\sigma_{\tilde{B}}^{(j,a)}, \sigma_{\tilde{B}}^{(k,b)}) = \mathcal{O}(2^{-\frac{1}{4}K(n)} + 2^{-\frac{1}{4}n^{\frac{1}{4}}} + (\varepsilon(n))^{\frac{1}{4}}). $$

and therefore

$$ \begin{aligned} \mathbb{E}\|\sigma_B^{(a)} + \sigma_B^{(b)} - \bar{\sigma}_B\|_1 &\le 2 \sum_{j,k} \mathbb{E}F(\bar{\sigma}_B^{(j,a)}, \bar{\sigma}_B^{(k,b)}) \\ &= \mathcal{O}(n^{2\alpha+1} \log(n)^2 (2^{-\frac{1}{4}K(n)} + 2^{-\frac{1}{4}n^{\frac{1}{4}}} + (\varepsilon(n))^{\frac{1}{4}})) \to 0 \end{aligned} \quad (4.35) $$

using that the number of terms is $\mathcal{O}(n^{2\alpha+1} \log(n)^2)$, $K(n) = \Omega(\log(n)^2)$ and $\varepsilon(n) = \mathcal{O}(n^{-\gamma})$, and our choice of $\alpha$ is such that $\mathcal{O}(n^{2\alpha+1} \log(n)^2 n^{-\frac{1}{4}\gamma})$ goes to zero.

To summarize, we have shown that we can approximate the random tensor network state $\bar{\sigma}_B$ on $G'$ by $\sigma_B^{(a)} + \sigma_B^{(b)}$, and we can approximate $\sigma_B^{(a)}$ by $\phi_B^{(a)}$. Moreover, we can approximate $\sigma_B^{(b)}$ by $\phi_B^{(b)}$, so the spectrum of $\sigma_B^{(b)}$ can be approximated by the spectrum of $\phi_B^{(b)}$. Recall that $\sigma_B^{(a)}$ and $\sigma_B^{(b)}$ are the random tensor network states on $G'$ which take $\phi_B^{(a)}$ and $\phi_B^{(b)}$ as background states, respectively. Furthermore, recall that our larger goal is to show that the spectra of the reduced background states $\phi_B^{(a)}$ and $\phi_B^{(b)}$ are, in some sense, close to the spectrum of the approximate random tensor network state $\sigma_B$ on the subgraph $G'$. This is a two-step process:

1. Show that $\phi_B^{(a)}$ and $\sigma_B^{(a)}$ can be slightly deformed to $\phi_B^{(a,\perp)}$ and $\sigma_B^{(a,\perp)}$, states with support orthogonal to $\mathrm{supp}(\sigma_B^{(j,b)})$ for all $j$.
2. Use the slightly deformed states to show that $\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(b)})$ is close to $\text{spec}_+(\sigma_B^{(a)} + \sigma_B^{(b)})$, and follow the chain of approximations: $\sigma_B^{(a)} + \sigma_B^{(b)} \approx \bar{\sigma}_B \approx \sigma_B$ along with $\text{spec}_+(\sigma_B) \approx \text{spec}_+(\rho_A)$ to conclude that $\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(b)}) \approx \text{spec}_+(\rho_A)$

Now, consider the state $\sigma_B^{(j,b)}$. It has support contained in $\mathcal{H}_{B,j}$ and by Eq. (4.31), it has rank($\sigma_B^{(j,b)}$) $\le 2^{-n^{1/4}} p_{1,j}^{-1}$. Let $Q_j$ be the projection onto $\text{supp}(\sigma_B^{(j,b)})$, so $\text{supp}(Q_j) \subseteq \mathcal{H}_{B,j}$ and $\text{rank}(Q_j) \le 2^{-n^{1/4}} p_{1,j}^{-1}$. We find that

$$ \|Q_j \phi_B^{(a)}\|_1 \le \text{rank}(Q_j) \|P_{B,j} \phi_B^{(a)} P_{B,j}\|_{\infty} \le \frac{2^{-n^{1/4}}}{p_{1,j}} p_{1,j} = 2^{-n^{1/4}}. $$

If we let $Q = \sum_j Q_j$, then we see that $(I-Q)\phi^{(a)}(I-Q)$ is a small deformation of $\phi_B^{(a)}$:

$$ \begin{aligned} \|\phi_B^{(a)} - (I-Q)\phi^{(a)}(I-Q)\|_1 &\le 2\|Q\phi^{(a)}\|_1 \le 2 \sum_j \|Q_j \phi_B^{(a)}\|_1 \\ &= \mathcal{O}(n^{9/2} \log(n) 2^{-n^{1/4}}) \to 0. \end{aligned} \quad (4.36) $$

With this property in hand, we can show that $\sigma_B^{(a)}$ can similarly be deformed. Let $\sigma_B^{(a,\perp)} = (I-Q)\sigma^{(a)}(I-Q)$. By construction, $\sigma_B^{(a,\perp)}$ has support orthogonal to that of $\sigma_B^{(b)}$, and hence, $\text{spec}_+(\sigma_B^{(a,\perp)} + \sigma_B^{(b)}) = \text{spec}_+(\sigma_B^{(a,\perp)} \oplus \sigma_B^{(b)})$. We observe that $\sigma_B^{(a,\perp)}$ is a small deformation of $\sigma_B^{(a)}$:

$$ \begin{aligned} \mathbb{E}\|\sigma_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 &\le \mathbb{E}\|\sigma_B^{(a)} - \phi_B^{(a)}\|_1 \\ &\quad + \mathbb{E}\|(I-Q)\sigma_B^{(a)}(I-Q) - (I-Q)\phi_B^{(a)}(I-Q)\|_1 \\ &\quad + \|\phi_B^{(a)} - (I-Q)\phi^{(a)}(I-Q)\|_1 \\ &\le 2\mathbb{E}\|\sigma_B^{(a)} - \phi_B^{(a)}\|_1 + \|\phi_B^{(a)} - (I-Q)\phi^{(a)}(I-Q)\|_1 \end{aligned} \quad (4.37) $$

which goes to zero, using Eq. (4.32) for the first term, and Eq. (4.36) for the second term. By construction, $(I-Q)\phi^{(a)}(I-Q)$ has support orthogonal to $\text{supp}(\sigma_B^{(b)})$. This allows us to bound

$$ \begin{aligned} \mathbb{E}\|\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(b)}) - \text{spec}_+(\sigma_B^{(a)} + \sigma_B^{(b)})\|_1 &\le \mathbb{E}\|\sigma_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 + \mathbb{E}\|\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(a)}) - \text{spec}_+(\sigma_B^{(a,\perp)} \oplus \sigma_B^{(b)})\|_1 \\ &= \mathbb{E}\|\sigma_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 + \mathbb{E}\|\text{spec}_+(\phi_B^{(a)}) \\ &\quad - \text{spec}_+(\sigma_B^{(a,\perp)}) + \text{spec}_+(\phi_B^{(a)}) - \text{spec}_+(\sigma_B^{(b)})\|_1 \\ &\le \mathbb{E}\|\sigma_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 + \mathbb{E}\|\phi_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 + \mathbb{E}\|\text{spec}_+(\phi_B^{(a)}) - \text{spec}_+(\sigma_B^{(b)})\|_1, \end{aligned} $$

where we have used the bound on the difference of spectra by the trace distance of the corresponding states Eq. (1.5). Each term on the RHS can be shown
to converge to zero. The first term goes to zero by Eq. (4.37). Similarly, the second term can be bounded by

$$ \mathbb{E}\|\phi_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 \le \mathbb{E}\|\phi_B^{(a)} - \sigma_B^{(a)}\|_1 + \mathbb{E}\|\sigma_B^{(a)} - \sigma_B^{(a,\perp)}\|_1 $$

which goes to zero by Eq. (4.37) and Eq. (4.32). The third term can be estimated by observing that $\text{spec}_+(\sigma_B^{(b)}) = \text{spec}_+(\sigma_B^{(b)})$ and

$$ \mathbb{E}\|\text{spec}_+(\phi_B^{(a)}) - \text{spec}_+(\sigma_B^{(b)})\|_1 \le \mathbb{E}\|\phi_B^{(a)} - \sigma_B^{(b)}\|_1 $$

which goes to zero by Eq. (4.34). We conclude that $\mathbb{E}\|\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(a)}) - \text{spec}_+(\sigma_B^{(a)} + \sigma_B^{(b)})\|_1 \to 0$.

We now follow a chain of approximations to get the desired closeness between $\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(a)})$ and $\text{spec}_+(\rho_A)$. Using Eqs. (4.29) and (4.35), we can see that

$$ \mathbb{E}\|\sigma_B - (\sigma_B^{(a)} + \sigma_B^{(b)})\|_1 \le \mathbb{E}\|\sigma_B - \bar{\sigma}_B\|_1 + \mathbb{E}\|\sigma_B^{(a)} + \sigma_B^{(b)} - \bar{\sigma}_B\|_1 \to 0, $$

so $\mathbb{E}\|\sigma_B - (\sigma_B^{(a)} + \sigma_B^{(b)})\|_1$ will converge to 0. This then implies

$$ \begin{aligned} \mathbb{E}\|\text{spec}_+(\sigma_B) - \text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(a)})\|_1 & \\ & \le \mathbb{E}\|\sigma_B - (\sigma_B^{(a)} + \sigma_B^{(b)})\|_1 \\ & \quad + \mathbb{E}\|\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(a)}) - \text{spec}_+(\sigma_B^{(a)} + \sigma_B^{(b)})\|_1, \end{aligned} $$

and as we have just shown, both terms on the RHS converge to zero. Together with Eq. (4.23), this yields the desired relationship to the spectrum of $\rho$:

$$ \begin{aligned} \mathbb{E}\|\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(b)}) - \text{spec}_+(\rho_A)\|_1 & \\ & \le \mathbb{E}\|\text{spec}_+(\phi_B^{(a)} \oplus \phi_B^{(b)}) - \text{spec}_+(\sigma_B)\|_1 \\ & \quad + \mathbb{E}\|\text{spec}_+(\rho_A) - \text{spec}_+(\sigma_B)\|_1 \to 0. \end{aligned} \quad (4.38) $$

We pause here again to note that we have accomplished Step 3: approximating the spectrum of $\rho_A$ by the spectra of the (approximate) background states. The final step will then be to consider the convergence properties of the distributions on the background states, which will then translate to convergence for the distribution on $\rho_A$.

Explicitly, we want to relate the above result to $\min_*(\nu_1, \nu_2)$. First, we observe that by Lemma 4.8 and Eq. (4.26), $\nu_{\tilde{\phi}_B} \Rightarrow \nu_1$ and $\nu_{\tilde{\phi}_{\bar{B}}} \Rightarrow \nu_2$, and since $\min$ is a continuous function, convergence holds for the pushforward measure:

$$ \min_*(\nu_{\tilde{\phi}_B}, \nu_{\tilde{\phi}_{\bar{B}}}) \Rightarrow \min_*(\nu_1, \nu_2). \quad (4.39) $$
We compute

$$
\begin{align*}
\min_{*}(\nu_{\tilde{\phi}_B}, \nu_{\tilde{\phi}_B}) &= \sum_{j,k} q_{1,k} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\min(\log(\frac{1}{p_{1,k}}), \log(\frac{1}{p_{2,j}}))-H(n)]} \\
&= \sum_{j} \left( \sum_{p_{1,k} \ge 2^{n^{1/4}}} q_{1,k} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\log(\frac{1}{p_{1,k}})-H(n)]} \right. \\
&\qquad \left. + \sum_{p_{1,k} \le 2^{-n^{1/4}}} q_{1,k} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\log(\frac{1}{p_{2,j}})-H(n)]} \right) \\
&\quad + \sum_{2^{-n^{1/4}} \le p_{2,j} \le p_{1,k} \le 2^{n^{1/4}}} q_{1,k} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\min(\log(\frac{1}{p_{1,k}}), \log(\frac{1}{p_{2,j}}))-H(n)]} \\
&= \sum_{k} q_{1,k} q_{2,k} \delta^{\frac{1}{\sqrt{n}} [\log(\frac{1}{p_{1,k}})-H(n)]} \\
&\quad + \sum_{j} q_{1,j} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\log(\frac{1}{p_{2,j}})-H(n)]} + \nu_0 \tag{4.40}
\end{align*}
$$

where we have written

$$
q_{1, > j} = \sum_{p_{1,k} \ge 2^{n^{1/4}}} q_{1,k}
$$

$$
q_{2, > k} = \sum_{p_{1,k} \le 2^{-n^{1/4}}} q_{2,j}
$$

and

$$
\nu_0 = \sum_{2^{-n^{1/4}} p_{2,j} \le p_{1,k} \le 2^{n^{1/4}} p_{2,j}} q_{1,k} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\min(\log(\frac{1}{p_{1,k}}), \log(\frac{1}{p_{2,j}}))-H(n)]}.
$$

Then by Eq. (4.28), we see that $\nu_0 \Rightarrow 0$. Using Eq. (4.39), we conclude

$$
\min_{*}(\nu_{\tilde{\phi}_{B}}, \nu_{\tilde{\phi}_{B}}) - \nu_{0} \Rightarrow \min_{*}(\nu_{1}, \nu_{2}). \quad (4.41)
$$

On the other hand, by construction, we have

$$
\nu_{\text{spec}}(\phi_B^{(a)} \oplus \phi_B^{(b)}) = \nu_{\phi_B^{(a)}} + \nu_{\phi_B^{(b)}}.
$$

We can explicitly write down

$$
\nu_{\phi_B^{(a)}} + \nu_{\phi_B^{(b)}} = \sum_k q_{1,k} q_{2,k} \delta^{\frac{1}{\sqrt{n}} [\log(\frac{1}{p_{1,k}q_{2,k}}) - H(n)]} \\
+ \sum_j q_{1,j} q_{2,j} \delta^{\frac{1}{\sqrt{n}} [\log(\frac{1}{p_{2,j}q_{1,j}}) - H(n)]}.
$$

Since the $q_{1,k}$ and $q_{2,j}$ are at least $n^{-\beta}$ (if the corresponding term is nonzero),
$|\log(q_{1,>j})| \le \beta \log(n)$ and $|\log(q_{2,>k})| \le \beta \log(n)$. With these bounds in mind,
we can compare to the last line of Eq. (4.40). More precisely, if we let $\nu_{\phi} = \min_{*}(\nu_{\phi_B}, \nu_{\phi_B}) - \nu_0$, then for uniformly continuous $f \in C_b(\mathbb{R})$, we have

$$ \lim_{n \to \infty} \left| \int f(x) d\nu_{\phi}(x) - \int f(x) d\nu_{\phi_B^{(a)}}(x) - \int f(x) d\nu_{\phi_B^{(b)}}(x) \right| = 0 $$

We conclude that

$$ \nu_{\phi_B^{(a)}} + \nu_{\phi_B^{(b)}} \Rightarrow \min_{*}(\nu_1, \nu_2). \quad (4.42) $$

Now, we can finally put all of our ingredients together. Recall the statement of convergence in probability implied by the convergence of spectra, in expectation, as in the second part of Lemma 4.8. Then using Eq. (4.38) as the vectors $p^{(n)}$ and $q^{(n)}$ in the statement of Lemma 4.8 and the convergence of distributions in Eq. (4.42), we conclude

$$ \nu_{\rho_A} \Rightarrow \min_{*}(\nu_1, \nu_2) \quad (4.43) $$

<figure><img src="image_23.png" /></figure>

### 4.5. Computing Entropies with Two Minimal Cuts

Ideally, we would like to use Theorem 4.12 to compute von Neumann entropies of random tensor network states. However, Theorem 4.12 alone is too weak to allow us to directly compute entropies up to $o(\sqrt{n})$ corrections, as weak convergence of the spectrum does not directly imply convergence of the mean. However, we kept track of various approximation errors in the proof of Theorem 4.12, and we will use these to show that with slightly stronger assumptions, these errors allow to compute the entropy up to $O(\log(n))$ corrections.

To begin, we first bound the difference in the entropy of a sum of density matrices and the sum of the entropies of the individual density matrices:

**Lemma 4.13.** Suppose $\{p_i\}_{i=1}^m$ is a subnormalized distribution and $\{\rho_i \in \mathcal{P}(\mathcal{H})\}_{i=1}^m$ is a collection of (unnormalized) density matrices and let $\rho = \sum_i p_i \rho_i \in \mathcal{P}(\mathcal{H})$. Suppose that $C^{-1} \le \text{tr}[\rho_i] \le C$, and $C^{-1} \le \text{tr}[\rho] \le C$, then

$$ \left| H(\rho) - \sum_{i=1}^{m} p_i H(\rho_i) \right| \le C(\log(m) + 2 \log(C)). $$

*Proof.* If the $\rho_i$ are normalized and $\sum_i p_i = 1$, then by the Holevo bound we have

$$ \sum_i p_i H(\rho_i) \le H\left(\sum_i p_i \rho_i\right) \le \sum_i p_i H(\rho_i) + H(\{p_i\}) \le \sum_i p_i H(\rho_i) + \log(m). $$

Now let $q_i = \text{tr}[\rho_i]$, $P = \sum_i q_i p_i$ and let $\sigma_i = \frac{\rho_i}{q_i}$, $r_i = \frac{p_i q_i}{P}$. Then, $H(\sum_i p_i \rho_i) = H(P \sum_i r_i \sigma_i) = P H(\sum_i r_i \sigma_i) - P \log(P)$. On the other hand

$$ P \sum_i r_i H(\sigma_i) = \sum_i p_i H(\rho_i) + \sum_i p_i \log(q_i) $$