# Renormalization of Chiral Nuclear Forces with Multiple Subtractions in Peripheral Channels

Authors: E. F. Batista; S. Szpigel; V. S. Timóteo
Journal: Advances in High Energy Physics
 (2017)

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## Abstract

We analyse the renormalization of the of two-nucleon interaction with multiple subtractions in peripheral waves considering two chiral forces at N3LO. Phase shifts at low energies are then computed with several subtraction points belowμ=10 fm−1. We show that for most peripheral waves the phase shifts have nearly no dependence on the renormalization scale. In two cases the phase shifts converge slowly as the renormalization scale approaches μ=1 fm−1 and in one case the phase shifts presented oscillations with respect to the subtraction point μ.


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## Body

## 1. Introduction

It is widely established in nuclear physics that Quantum Chromodynamics (QCD) is in fact the underlying theory which describes the properties of strong nuclear forces. In this theory, the fundamental degrees of freedom are quarks which interact with each other via exchange of colored gluons. On the other hand, the strong nuclear force is also responsible for the binding of protons and neutrons in atomic nuclei. But according to QCD, nucleons are bound states of quarks and the nuclear force is considered as the residual part of the quark-quark interaction inside of the nucleon with exchange of gluons. Due to the property of asymptotic freedom, the running coupling constant is small enough at high energies to allow QCD to be handled within a perturbative approach. However, at low energies, where mesons and nucleons are the relevant degrees of freedom, the running coupling constant becomes large and QCD is no longer perturbative. The nonperturbative nature of QCD at low energies is implied in several mathematical and computational problems which makes the description of nucleon properties a hard task.Since QCD cannot be treated perturbatively at low energies, a new approach was developed to handle nuclear forces with degrees of freedom appropriate for low-energy systems. The idea was to use quantum field theory but replacing quarks and gluons degrees of freedom by pions and nucleons, keeping the fundamental properties of the underlying theory like chiral symmetry. This effective field theory (EFT) scheme was already used in other systems to describe different types of interactions and Weinberg proposed an EFT approach to nuclear systems based on QCD. This idea generated a new branch in nuclear physics and allowed a deeper understanding of the nuclear force and few-nucleon systems. In particular, the two-nucleon system requires a nonperturbative extension of Chiral Perturbation Theory (ChPT) which works well in the case of pion-nucleon scattering.Basically, an EFT is constructed by isolating the most relevant degrees of freedom and symmetries for the system under consideration and applying standard quantum field theory. In nuclear physics, replacing quarks and gluons by pions and nucleons means moving to a different (lower) energy scale and a connection between the symmetry properties of the underlying fundamental theory and the symmetries of their effective versions must be well-established. Thus, in a nuclear effective theories it is necessary to establish scale parameters which enable us to separate the high energy components of the interaction from the low-energy part. In a series of papers [1–3], Weinberg proposed an effective field theory scheme for nuclear forces based on the chiral symmetry of QCD.This approach was first applied by Ordóñez et al. [4, 5] and allowed the perturbative treatment of the NN interaction. An expansion in powers of (Q/Λχ)ν is performed and Q is a generic low momentum scale and Λ is the chiral symmetry breaking scale which is approximately 1GeV. This expansion is controlled by a power counting scheme, called Weinberg power counting (WPC), which provides an hierarchical organization for the processes in few-nucleon systems. Following the WPC, the NN interaction at leading order (LO) consists of one-pion-exchange (OPE) plus a contact term. At next-to-leading order (NLO), two-pion exchange (TPE) and O(p2) contact interactions are added; at next-to-next-to-leading order (N2LO) there is an additional set of TPE diagrams and, finally, at next-to-next-to-next-to-leading order (N3LO) corrections to both OPE and TPE are included along with O(p4) contact interactions.Regardless of how the chiral expansion is organized, the issue of how to renormalize the two-body interaction is of fundamental importance and has been subject of investigation for decades. Early works by Adhikari et al. started by discussing the renormalization of two-body quantum hamiltonians [6–8]. Later, the problem was focused in the NN interaction using renormalization group analysis and a new power counting was proposed by Kaplan et al. [9–11]. Discussions on the renormalization of singular and one-pion-exchange two-body interactions, power counting, and renormalization of the three-body system are detailed by van Kolck et al. [12–14]. Another renormalization group approach to two-body and nucleon-nucleon scattering was presented by Birse et al. [15–18] and a complete analysis of cutoff renormalization in configuration space was performed by the Granada group [19–22]. Also, a comparison between renormalization in configuration and momentum spaces has been carried out in [23].Another renormalization approach for theNN system consists of a hybrid scheme, where the LO contribution is treated nonperturbatively and the higher orders are handled perturbatively [24]. Results for P-waves and D-waves show that perturbative two-pion exchange reproduces the experimental data up to kcm~300 MeV. Here we treat all terms nonperturbatively since in our renormalization scheme the pieces of the interaction are inserted as the subtractions are performed.Apart from the divergences due to pion loops in the irreducible diagrams, the reducible diagrams also generate divergences in the scattering equation. To overcome this problem the most common employed method is introducing a cutoff regularization scaleΛ which limits the momentum integration, in the scattering equation, above this scale parameter resulting in a finite phase shifts. The cutoff scheme handles the divergences by modifying the potential and keeping the scattering equation intact. The regularized interaction contains only low momentum components and the cutoff scale is fixed at some scale, typically ~2-3 fm−1. A slight discomfort with this method comes from the fact that all physics above a certain momentum scale is excluded. Recently, a N3LO interaction has been optimized by an improved renormalization approach in configuration space which maintains the analytic structure of the scattering amplitude [25].An alternative renormalization procedure referred to as subtractive method or multiple subtractions treats the divergences with a different perspective: instead of modifying the potential, as in cutoff method, and keeping the scattering equation untouched, here the interaction is kept intact and the scattering equation is modified by the introduction of subtractions in its kernel. The dependence of the phase shifts on the cutoff is replaced by a dependence on the subtraction point that can be later eliminated by using the renormalization group flow. With this procedure no components are neglected from the interaction and both low and high momentum components are included. Detailed descriptions of this approach can be found in [26–32].In this work we employ the subtract kernel method to renormalize the Lippmann-Schwinger equation in N3LO and perform a detailed renormalization scale dependence analysis of the phase shifts in peripheral channels. The high angular momentum waves are interesting because the force in their channels contains no contact interactions and consists only of pion exchanges. The N3LO potential has contact contributions up toD-waves so that F and higher waves have contributions purely from pion exchanges and no core given by contact interactions.This paper is organized as follows: Section2 describes the renormalization of N3LO interactions with five subtractions; Section 3 presents the numerical results for both uncoupled and coupled channels up to J=6 and our main conclusions are given in Section 4.


## 2. Renormalization of N3LO Interactions

At any given order, the modern two-nucleon interactions can always be separated in two components: the pion exchange interactions and the contact terms, which parametrize the short range core of the interaction and are determined by fitting scattering data. TheNN potential is then written as(1)VNN=Vpions+Vcont,where the first term contains one-pion-exchange and two-pion exchanges(2)Vpions=Vπ+V2π.The power counting scheme organizes which set of Feynman diagrams must be included in each order in the chiral expansion:(3)Vpions=Vpions0+Vpions2+Vpions3+Vpions4+⋯,Vcont=Vcont0+Vcont2+Vcont4+⋯,where the superscript numbers in parentheses indicates the order in the chiral expansion. Note that in (3) for the contact contribution, all the odd powers are cancelled due to symmetry requirements. Hence, in the Weinberg power counting scheme, there is no contact interaction Vcont(3) at the third order in the chiral expansion (N2LO). This actually breaks the order-by-order improvement of the chiral expansion when going from NLO to N2LO as shown very clearly in [32]. Nogga et al. [14] looked at the interaction at leading order (LO) and found that additional counterterms that are not predicted by the Weinberg power counting are required in order to improve the description. Later, Valderrama showed that there are also problems in higher orders and they could be treated perturbatively [24].For finite cutoff, however, Epelbaum et al. [33, 34] showed that a better description of the phase shifts is obtained when N2LO instead of NLO interactions are used (with the same contact terms). The same conclusion can be found by studying χ2/datum in Marji et al. [35].Now let us turn to the renormalization of N3LO interactions with five subtractions. This approach introduces a renormalization scaleμ (subtraction point), which denotes the momentum at which the subtractions are performed. For a given energy E the Lippmann-Schwinger (LS) equation for the T-matrix in operator form is written as(4)TE=V+VG0+ETE,where V is the NN potential at a given order in the chiral expansion and G0+ is the free Green’s function which, in terms of the free Hamiltonian H0, is given by(5)G0+E=1E-H0+iϵ.When bare potentials are introduced in the equation above, an ultraviolet divergence arises due to the implicit integral in the second term of the right-hand side of (4), which diverges when the momentum goes to infinity. In the standard cutoff procedure, the NN potential V is multiplied by a regularizing function,(6)Vp,p′⟶VΛp,p′≡exp⁡-pΛ2rVp,p′exp⁡-p′Λ2r,where Λ is the cutoff scale and r≥1. This function suppresses contributions from larger momenta, eliminating the ultraviolet divergences in the momentum integral. Nonrelativistic nucleon-nucleon potentials based on chiral effective field theory with cutoff regularization provide a very accurate description of NN scattering data below pion production threshold Elab~350 MeV.The renormalization with multiple subtractions handles this problem in a different way since theNN potential is not modified in favour of changing Green’s function instead. The N3LO interactions require five subtractions to be renormalized with no cutoff and in this case the subtracted scattering equation is given by(7)Tμ5E=Vμ5E+Vμ5EG5+E;-μ2Tμ5E,where μ is the subtraction scale, Vμ(n)(E) is the driving term(8)VμnE=Vμn-1E+Vμn-1E-μ2-En-1E-q2nVμnE,which has to be calculated recursively, G5+(E;-μ2) is the 5-times subtracted Green’s function, and q is the relative intermediate two-nucleon momentum.(9)G5+E=F5E;-μ2G0+E,where (10)F5E;-μ2=μ2+Eμ2+H05is a term that arises from the recursive nature of the renormalization process and works as a form factor, being responsible for providing a regular T-matrix. Detailed expressions for the integral equations in the recursive calculation with partial wave basis are given in [32] for the case of N2LO interactions with four subtractions.The LS equation with five subtractions (7) has the same operator structure as the original equation (4), with the effective NN potential V replaced by the driving term Vμ(5)(E) and the free Green’s function G0+(E) replaced by Green’s function with five subtractions G5+(E;-μ2). The recursive driving term encodes the physical information apparently lost due to the removal of the propagation through intermediate states at the subtraction point μ. Then, once the driving term is determined for a particular subtraction point, the subtracted Lippmann-Schwinger equation provides a renormalized solution for the T-matrix at any given energy E.The driving termsVμ(n) are built recursively with the components of the nucleon-nucleon interaction. Here we use nonregulated N3LO interactions from Entem and Machleidt (EM) [36, 37] and from Epelbaum et al. (EGM) [38–40]. The main difference between the two chiral forces is the two-pion exchange part. The EGM potential uses Spectral Function Regularization (SFR) for the pion loop integrals resulting in a softer TPE component. Differences in the pionic part will then be compensated by changes in the low-energy constants so that in the end the two forces give similar descriptions for the NN system. Note that in the case of the EGM potential the SFR is still present for the loop integrals, but there is no smooth regulator function to suppress large momentum contributions. The smooth cutoff is also removed from the EM potential so that the interactions we are using are the original EM and EGM interactions with their cutoffs removed. Once the contact interactions are determined for both potentials, even with different off-shell behavior, the resulting on-shell scattering amplitudes are similar. Thus, we expect comparable results for cutoff regularization and subtractive renormalization at low energies. At high energies, Elab>200 MeV the cutoff scheme is more efficient than the renormalization with multiple subtractions as far as describing the phase shifts is concerned.


## 3. Numerical Results

Here we work in a partial wave relative momentum space basis and compute the phase shifts in each peripheral channel. However, a three-dimensional approach without any partial wave decomposition has also been employed [41–43].For numerical reasons, when implementing the renormalization procedure, we solve the subtracted LS equation for theK-matrix using the principal value prescription. We then compute the neutron-proton phase shifts for channels with angular momentum in the range 3≤J≤6 with the N3LO potentials EM and EGM. Expressions for the phases shits as functions of the on-shell K-matrix in coupled and uncoupled channels are given in [44–46].For each wave, we consider several renormalization scales up toμ=10 fm−1, limiting the momentum integrations at Λ=30 fm−1. In practice this means we have an infinite cutoff and the renormalization is completely imposed by the five subtractions, unlike in [47–49] where the cutoff still plays a role since only one subtraction was performed for the N2LO potential which requires four subtractions to allow an infinite cutoff.In the case of the EGM potential, we have used an SFR cutoff ofΛ~=4mπ (550 MeV), the most common choice. The only parameter of the EGM potential we changed was the cutoff Λ→∞. The EGM interaction depends on the SFR cutoff and the results are different if the SFR cutoff is modified, but this dependence is not related to the subtractions. We also believe that it is the SFR that drives the difference between the EM and EGM potentials as far as the renormalization scale dependence is concerned. Nevertheless, here we treated the SFR cutoff as an internal parameter of the EGM potential and looked only at the dependence of the phases on μ.The results for the N3LO-EM potential are displayed in Figures1–4 for the uncoupled channels and in Figures 5 and 6 for the coupled channels. For the N3LO-EGM potential, the results are displayed in Figures 7–10 for the uncoupled channels and in Figures 11 and 12 for the coupled channels. The phase shifts are compared to the Nijmegen partial wave analysis [50]. For an updated high quality partial wave and error analysis, see the works from the Granada group [51–55].Figure 1
(Color on-line) phase shifts inF13 and F33 uncoupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 2
(Color on-line) phase shifts inG14 and G34 uncoupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 3
(Color on-line) phase shifts inH15 and H35 uncoupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 4
(Color on-line) phase shifts inI16 and I36 uncoupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 5
(Color on-line) phase shifts inF34-H34 coupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 6
(Color on-line) phase shifts inG35-I35 coupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 7
(Color on-line) phase shifts inF13 and F33 channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EGM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 8
(Color on-line) phase shifts inG14 and G34 channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EGM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 9
(Color on-line) phase shifts inH15 and H35 channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EGM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 10
(Color on-line) phase shifts inI16 and I36 channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EGM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 11
(Color on-line) phase shifts inF34-H34 coupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EGM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Figure 12
(Color on-line) phase shifts inG35-I35 coupled channels calculated from the solution of the subtracted LS equation for the K-matrix with five subtractions for the N3LO-EGM potential for several values of the renormalization scale compared to the Nijmegen partial wave analysis.Note that in the end we used different ranges of renormalization scales for EM and EGM and the reason is that the results for EGM converges faster as far asμ is concerned and there is no need to go above 2 fm−1. In the case of EM, since there are still some variations in few waves for μ>2 fm−1 we extended the range of the subtraction point to 10 fm−1. We believe this is related to the differences between EM and EGM that makes EGM softer than EM.With few exceptions, in most of the channels we observe very small variation of the phases as we change the subtraction point, indicating that peripheral waves are nearly renormalization group invariant or fixed-points of the subtractive renormalization group. The exceptions areH34 and I35 waves, which show slower convergence and G35 channel where the agreement with the partial wave analysis is only up to ~50 MeV. Also, in the case of the EM potential, the phases for the F33 wave present some oscillations when the renormalization scale approaches μ~10 fm−1.In this case of the coupled channels, the renormalization scheme is not failing but just requiring a slightly largerμ in the coupled channels, where we have the very singular tensor force. And this is what is different in the these channels compared to other F waves. The case of the uncoupled triplet 3F3 is somewhat different; the oscillation observed when going from μ=6 to 9 fm−1 is related to the TPE without SFR of the EM potential. This oscillation is not seen in the 3F3 wave when the EGM potential is used. An additional subtraction does not modify the results and the μ dependence in the these channels, so only the minimum number of subtractions needs to be performed (five at N3LO).It is important to mention that theμ-dependence of the phase shifts is encoded in the recursive driving terms Vμ(n) since they all depend on the renormalization scale. In the case of cutoff regularization in configuration space [56], the cutoff radius RS dependence has been traced to the most singular part of the interaction which can be attraction or repulsion, depending on the channel. Here we observe more dependence on the coupled channels due to the very singular tensor force and the F-wave issue is due to the differences between the TPE components of the EM and EGM potentials.


## 4. Conclusions and Outlook

So far we have renormalized the N3LO interactions with multiple subtractions in peripheral channels considering an infinite cutoffΛ=30 fm−1. Only pions contribute to the nuclear force in these waves and the results are parameter-free.The five subtractions performed in the kernel of the LS equation provide finiteK-matrix in peripheral waves and the resulting phase shifts are rather independent of the subtraction point with the exception of H34 and I35 waves where the fixed point is reached at approximately μ~1 fm−1 after the slow convergence shown in Figures 5, 6, 11, and 12.The oscillation in theF33 channel suggests a closer look at this wave with the renormalization group flow equation that governs the driving terms (interactions) as the subtraction point is changed with the constraint of an invariant scattering amplitude.The advances given by our approach when compared to cutoff regularization are as follows: theNN force does not have to be modified prior to its insertion in the scattering equation; only the scattering equation is modified; the method is renormalization group invariant by construction and provides a nonrelativistic flow equation for the driving terms that tell us how they change when the renormalization scale is modified in order to keep the amplitude invariant. Finally, we would like to point out that the cutoff loses any physical significance since our results were obtained with an extremely large value Λ=30 fm−1.



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