# Non-Supersymmetric CS-Matter Theories with Known AdS Duals

Authors: Davide Forcella; Alberto Zaffaroni
Journal: Advances in High Energy Physics
 (2011)

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## Abstract

We consider three-dimensional conformal field theories living on a stack ofN anti-M2 branes at the tip of eight-dimensional supersymmetric cones. The corresponding supergravity solution is obtained by changing sign to the four-form in the Freund-Rubin solution representing M2 branes (“skew-whiffing” transformation) and it is known to be stable. The existence of these non-supersymmetric, stable field theories, at least in the large N limit, is a peculiarity of the AdS4/CFT3 correspondence with respect to the usual AdS5/CFT4, and it is worthwhile to study it. We analyze in detail the KK spectrum of the skew-whiffed solution associated with S7/ℤk and we speculate on the natural field content for a candidate non-supersymmetric dual field theory.


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## Body

## 1. Introduction

There has been some progress in understanding the conformal field theories living on a stack ofN M2 branes at the tip of noncompact eight-dimensional cones. These theories are holographically dual to Freund-Rubin compactifications of M theory of the form AdS4×H7, where H7 is the Einstein manifold at the base of the cone. In the case of large supersymmetry, 𝒩≥3, the conformal field theory has been identified with a Chern-Simons theory in [1–10]. The case where the cone is a Calabi-Yau fourfold corresponds to 𝒩=2 supersymmetry, and a general construction of the dual Chern-Simons theories has been discussed in [11, 12]; a large number of models have been subsequently constructed [13–23]. For the smallest amount of supersymmetry, 𝒩=1, the cone is a Spin(7) manifold and a generic construction of the dual field theories for orbifolds has been given in [24]. In this paper we are interested in the three-dimensional conformal field theories living on a stack of N anti-M2 branes at the tip of eight-dimensional cones with at least Spin(7) holonomy. The existence of these non-supersymmetric, stable field theories, at least in the large N limit, is a peculiarity of the AdS4/CFT3 correspondence with respect to the usual AdS5/CFT4, and it is worthwhile to study it (Previous studies of three-dimensional non-supersymmetric field theories in similar setups can be found in [25, 26].)The supergravity solutions ofN anti-M2 branes at the tip of supersymmetric cones is obtained by changing sign to the four-form in the familiar solutions representing M2 branes. This operation is called “skew-whiffing” in the supergravity literature and it is proven to produce a stable non-supersymmetric background [27]. The KK spectrum of the final theory is obtained from the original spectrum by a reshuffling of states. We will mostly focus on the simple case H7=S7 in this paper. In this particular case the skew-whiffing procedure is equivalent to a triality transformation in the isometry group SO(8) and it leaves the theory invariant. However, following the recent results on AdS4×CFT3, we are really interested in H7=S7/ℤk. For k≥2 the skew-whiffing produces a stable non-supersymmetric background. It is interesting then to find a plausible dual field theory. (In [28] there is a discussion of the effect of the skew-whiffing on the dual field theory for k=1.) In this paper we analyze in detail the KK spectrum of the skew-whiffed theory and we speculate on a candidate for the underlying field theory. Without supersymmetry, it is difficult to make explicit checks of the proposal. We are guided in our search by the attempt of implementing the skew-whiffing procedure to the ABJM theory [6].The paper is organized as follows. In Section2 we discuss the skew-whiffing construction. In Section 3 we discuss a natural field content for the skew-whiffing of the ABJM theory. In Section 4 we make some checks of the proposal and in particular we see that the relevant features of the KK spectrum in supergravity are compatible with the operator content of the field theory. In Section 5 we discuss possible generalizations.


## 2. The Skew-Whiffed Solutions

M-theory has a very natural compactification to four dimensions. (For a comprehensive review see [29].) It comes from the Freud-Rubin ansatz for the 3-form field,
(2.1)Fμνρσ=3mϵμνρσ,Fmnpq=0,
where m is a real constant, the greek letters label the four space-time directions, while the latin letters label the internal seven-dimensional space. As a consequence the metric satisfies the equations
(2.2)Rμν=-12m2gμν,Rmn=6m2gmn
and M theory spontaneously compactifies to AdS4×H7, where H7 is an Einstein space. If the Einstein manifold H7 has at least weak G2 holonomy, then the solution is supersymmetric and hence stable. This solution can indeed be interpreted as the near horizon solution for M2 branes at the tip of the real cone C(H7). There is another very natural solution that can be obtained sending m to -m: the four-form changes sign, while the metric is invariant. This solution can be interpreted as the near horizon solution for anti-M2 branes at the tip of the real cone C(H7) and it is called the “skew-whiffed” solution.It is interesting to observe that the skew-whiffed transformation changes the sign of the Page chargeP=1/π4∫H7*F and can indeed be equivalently interpreted as a change of orientation for H7.The number of preserved supersymmetries of a solution is the number of independent Killing spinorsη solving the equation
(2.3)(∇n-12mΓn)η=0.
This supersymmetric condition explicitly depends on m. Indeed it is possible to prove that, with exception of the round sphere S7, where both orientations give the maximum supersymmetry 𝒩=8, at most one orientation can have 𝒩>0 [29]. Moreover it is possible to prove that the skew-whiffing of a supersymmetric Freud-Rubin solution is perturbatively stable [27]. Hence, given a supersymmetric Freud-Rubin solution, we can find another non-supersymmetric stable solution, obtained by applying the skew-whiffing transformation. (See [30, 31] for some recent applications of the skew-whiffed solutions.)These theories are expected to have a well-defined dual non-supersymmetric three-dimensional conformal field theory. In this paper we will discuss a natural field content for these theories.It is important to observe that the skew-whiffing procedure is somehow peculiar of M theory. Indeed the same transformation could be applied to the five-form in the Freud-Rubin ansatz for type IIB supergravity. However, in this case, the resulting theory would still be supersymmetric.


## 3. The Skew-Whiffing of the ABJM Theory

When the seven-dimensional Einstein space is aℤk quotient of the round sphere, S7/ℤk, the dual field theory is the well-known ABJM model [6]. This is an 𝒩=6 three-dimensional U(N)×U(N) Chern-Simons theory with levels k and -k, coupled to four complex bosons XA and four complex fermions ψA transforming in the bifundamental of the gauge group. The global symmetry is SU(4)R×U(1), the non-abelian part being the R symmetry group, while the abelian part being the baryonic symmetry. The bifundamental bosons XA transform in the representation 41 of the global symmetry group and the bifundamental fermions ψA transform in the 4¯-1. All fields have canonical dimension: 1/2 for the bosons and 1 for the fermions.This specific field content can be understood as the decomposition of the degrees of freedom of the𝒩=8 conformal theory dual to S7 under the breaking of the R symmetry group SO(8)→SU(4)×U(1) induced by ℤk. The natural field content of the theory describing S7 consists in a scalar Φa transforming in the 8v vectorial representation of SO(8), and a fermion Yα transforming in the 8s spinorial representation of SO(8) (this is the singleton representation of the superconformal group); the eight supercharges transform in the 8c conjugate spinor representation. These are the degrees of freedom that we expect to live on a supersymmetric M2 brane in flat space. The existing 𝒩=8 Chern-Simons theory describing membranes, the BLG model [1–5], have indeed this field content. The 𝒩=8 multiplet decomposes as 8v→41+4¯-1,8s→41+4¯-1 under SO(8)→SU(4)×U(1) and we recover the ABJM matter content describing S7/ℤk. The ABJM model has enhanced 𝒩=8 supersymmetry for k=1 but this enhancement is not manifest and it is conjectured to be realized through light monopole operators which become relevant for k=1.We would like to identify a candidate for the skew-whiffing solution onS7/ℤk. As we explained in the previous section, the skew-whiffing procedure can be understood as the change of orientation of S7, and hence as a parity transformation on ℝ8. The scalar fields living on the M2 can be seen as the coordinates of the transverse space, and, under parity, an odd number of them change sign, while the associated eight-dimensional spinor changes chirality.The skew-whiffing procedure can be seen as a map,(3.1)SW:(8v,8s)⟶(8v,8c).An explicit realization of this map on an𝒩=8 multiplet is
(3.2)SW:(Φi,Φ8,Ya)⟶(Φi,-Φ8,(Γ8)ȧaYa).Fork=1, this transformation should be an invariance of the dual-field theory, since S7 is skew-whiffing invariant. We can test this transformation in the BLG theory [1–5], which is an explicit 𝒩=8 lagrangian theory invariant under the SO(8)R symmetry and describes a pair of membranes. It is an easy exercise to see that the BLG Lagrangian is indeed invariant under the transformation (3.2), as required by the supergravity skew-whiffing transformation. In the ABJM theory with k=1, this transformation is, on the other hand, nonlocally realized.For generick, the SO(8) symmetry is broken to SU(4)×U(1). Under skew whiffing, the 8s fermions are replaced by 8c and the fields decompose as 8v→41+4¯-1, 8c→12+60+1-2. The original supersymmetry charges would now transform in the 8s→41+4¯-1. None is invariant under the U(1) symmetry and hence the theory naturally breaks all the supersymmetries.It is natural to expect that the dual of the skew-whiffedS7/ℤk is a non-supersymmetric three-dimensional Chern-Simons theory with matter. Let us try to understand what is the natural field content. We still expect a gauge group U(N)×U(N) and a global symmetry SU(4). Comparing with the geometric action of the SW transformation, we introduce complex scalars XA transforming in the bifundamental of the gauge groups and in the fundamental of the global symmetry SU(4); real fermions ΨI transforming in the adjoint of the first gauge group and in the antisymmetric of SU(4); complex fermions ξ transforming in the bifundamental of the SU(N)×SU(N) gauge group, with charge 2 under the difference of the two U(1) gauge factors and as singlets under the global symmetry SU(4). The matter content of such a theory is summarized in Table 1 below.Table 1
Matter content and charges.
FieldsSU(N)1SU(N)2U(1)1-U(1)2U(1)1+U(1)2SU(4)XANN¯104ΨIAdj0006ξNN¯201As we will see in Section4, the supergravity KK spectrum predicts the existence of operators with integer dimensions in the dual-field theory. A peculiarity of the skew-whiffing transformation indeed is the fact that it just reshuffles the KK states without changing their dimensions. To match the KK spectrum with the above field content we need to assume that all the fields have canonical dimensions: 1/2 for the scalars and 1 for the fermions. It is then tempting to write a classically conformal invariant Lagrangian for the fields XA,ΨI,ξ. The most general Lagrangian we can write is
(3.3)L=LCS+Lkin+Vbos+Vfer,
where
(3.4)LCS=k4πTr⁡[ϵμνλ(Aμ∂νAλ+2i3AμAνAλ)-ϵμνλ(Ãμ∂νÃλ+2i3ÃμÃνÃλ)],Skin=Tr⁡(-DμXADμXA†+iΨ¯IγμDμΨI+iξ¯†γμDμξ),Vbos=π212k2Tr⁡(XAXA†XBXB†XCXC†+XA†XAXB†XBXC†XC+4XAXB†XCXA†XBXC†-6XAXB†XBXA†XCXC†),Vfer=iπ2kTr⁡(c1(ΓIJ)ABXAXB†ΨIΨJ+c2(XAXA†ξξ†-XA†XAξ†ξ)),
where the covariant derivatives act according to Table 1. We keep the same bosonic potential of the ABJM theory, and we introduce two real couplings ci to parametrize the fermionic potential. The same potential of the ABJM theory guarantees that a probe see ℝ8/ℤk as a moduli space; in the skew-whiffed supergravity background an anti-M2 brane feels no potential, exactly as a M2 brane in the original background. The Lagrangian is scale invariant at classical level. Obviously, without supersymmetry, there is no guarantee that the theory remains conformal invariant at the quantum level and, in general, we expect that the fields acquire anomalous dimensions. It is tempting to speculate that, in the limit where supergravity is valid (large N limit and strong coupling N/k≫1 in type IIA), the theory becomes conformal with canonical dimensions for the fields.One could try to impose a relation between theci in the fermionic potential by requiring that the scalar BPS operators of the ABJM theory do not acquire anomalous dimensions at weak coupling in the SW ABJM theory. This constraint is suggested by the dimensions of the scalar part of the KK spectrum in supergravity, and the strong assumption that we can extrapolate from strong to weak coupling. The argument goes as follows. Starting from the lagrangian (3.4) it is possible to compute the quantum part of the two loop dilatation operator (mixing matrix) for small values of N/k. The mixing matrix acting on the gauge invariant operators of the field theory gives their anomalous dimensions. The mixing matrix acting on the gauge invariant operators done by contracting only the scalar fields XA and XA† was computed in [32] for the ABJM theory. The computation can be easily repeated for the SW ABJM theory: the only difference is the contribution coming from the fermions running into the loops, and in particular their contribution to the identity and the trace part of the mixing matrix. By imposing that the scalar mixing matrix of the SW ABJM theory is annihilate by the scalar symmetric traceless operators (4.12) we find a constraint on the ci. It would be much harder to perform a similar computation with operators with fermionic insertions to see if some of them remain with canonical dimensions with such a choice of ci.


## 4. The KK Spectrum

In this section, we discuss in details the KK spectrum of the skew-whiffed M theory solution onS7/ℤk and of its reduction to type IIA. The KK states should correspond to the single trace operators of the dual field theory with finite dimensions in the large N and strong coupling limit. It obviously difficult to predict the spectrum of operators with finite dimensions in a non-supersymmetric theory. However, the distinctive features of the KK spectrum put constraints on the dual field content.


### 4.1. The Spectrum onS7

The KK spectrum of the M-theory Freud-Rubin solution onS7 is well known [33, 34] and reported for completeness in Table 2. The states are classified by the dimension and the representation under SO(8) and are organized in superconformal multiplets specified by an integer number m≥2. The lowest state in each multiplet is scalar field of dimension m/2 transforming in the [m,0,0,0] representation of SO(8). The other states are obtained by acting on the lowest state with the 𝒩=8 supersymmetries transforming as 8c=[0,0,0,1] under SO(8). The multiplet is short and has spin range equal to two, compared with the spin range of four of a long multiplet. The multiplets m=2,3 sustain further shortenings; m=2 corresponds to the massless multiplet of the 𝒩=8 gauged supergravity. Partition functions encoding the spectrum of S7 (and of its quotient) in a related context can be found in [35–38].Table 2
The spectrum onS7.
SpinSO(8)Δ2+[m-2,0,0,0]m+4232(1)[m-2,0,0,1]m+3232(2)[m-3,0,1,0]m+521-(1)[m-2,1,0,0]m+221+(2)[m-3,0,1,1]m+421-(2)[m-4,1,0,0]m+6212(1)[m-1,0,1,0]m+1212(2)[m-3,1,1,0]m+3212(3)[m-4,1,0,1]m+5212(4)[m-4,0,0,1]m+720+(1)[m,0,0,0]m20-(1)[m-2,0,2,0]m+220+(2)[m-4,2,0,0]m+420-(2)[m-4,0,0,2]m+620+(3)[m-4,0,0,0]m+82We can understand the structure of the multiplets by considering a very simple theory of eight free bosonsΦi and eight free fermions Ya. These are the expected degrees of freedom living on a membrane in flat space. The lowest state of the m-th KK supermultiplet can be represented by Φm, which is a schematic expression for the product of m fields completely symmetrized in their SO(8) indices and with all the traces removed:
(4.1)Φm≡Φ{i1⋯Φim}-traces.
The other states are obtained by applying the supersymmetry transformations that schematically read
(4.2)[Qαȧ,Φi]=i(Γ̃i)ȧaYαa,{Qαȧ,Yβa}=(γμ)αβDμΦi(Γi)aȧ.
The first spinorial state (1/2)(1) with dimension (m+1)/2 reads
(4.3)YαaΦm-1,
where, again, Φm will represent a fully symmetrized and traceless string of fields Φik. The indices are contracted in such a way that the operator transforms as [m-1,0,1,0]. The states with dimension (m+2)/2 are obtained by applying two supercharges whose Lorentz indices can be antisymmetrized or symmetrized giving a scalar 0-(1) and a vector 1-(1) of schematic form
(4.4)Y[α{aYβ]b}Φm-2,(Y{α[aYβ}b]+γαβμΦ[i1DμΦi2])Φm-2.
The fermionic bilinears transform in the [0,0,2,0] and [0,1,0,0] representation of SO(8), respectively, which can be contracted with [m-2,0,0,0] to give the expected representations [m-2,0,2,0] and [m-2,1,0,0] given in Table 2. The states with dimension (m+3)/2 read schematically
(4.5)(YαaYβbYγc+⋯)Φm-3.
The Lorentz indices can be completely symmetric or with mixed symmetry; we obtain a state (3/2)(1) with three SO(8) indices transforming in the [1,0,0,1] and a state (1/2)(2) with three indices [0,1,1,0], respectively. Combining with the bosonic part we easily recover the representations [m-2,0,0,1] and [m-3,1,1,0] reported in Table 2. The states with dimension (m+4)/2 have four fermions whose Lorentz indices can be contracted in order to give a scalar 0+(2), a vector 1+(2), and a spin two 2+. We can write, for example, the schematic form of the spin two operator in the [m-2,0,0,0] representation of SO(8),
(4.6)DμΦiDνΦiΦm-2+Y{α1[a1⋯Yα4}a4]Φm-4+⋯.
The scalar and vector are obtained with different contraction of the Lorentz indices; it is easy to check that the SO(8) indices then transform as reported in Table 2. The rest of the spectrum can be similarly reconstructed.The KK spectrum onS7 should reproduce the full spectrum of short operators with finite dimensions in the large N limit of the field theory dual to AdS4×S7. It is however difficult to write explicit expressions for these multiplets in terms of local operators. The ABJM theory with k=1 is an explicitly scale invariant local Lagrangian dual to AdS4×S7 and its spectrum of single trace chiral operators should match the KK spectrum on S7. However, the explicit correspondence is somehow obscured by the fact that the 𝒩=8 supersymmetry of ABJM is not manifest and monopole operators are required to match the spectrum. In the particular case N=2, the ABJM theory with group SU(2)×SU(2) has manifest 𝒩=8 supersymmetry and SO(8) global symmetry; in fact it coincides with the BLG theory [1–5]. However, even in this case we can only give an explicit representation for the multiplets with even m. Let us discuss briefly how. We use the formulation as a Chern-Simons theory with gauge group SU(2)×SU(2). The matter content consist of bosonic and fermionic fields Φi and Ya transforming in the bifundamental representation of the gauge group and in the 8v in the 8s representation of SO(8), respectively. The fields can be written as two-by-two matrices satisfying the reality condition
(4.7)ΦAȦi=ϵABϵȦḂ(Φi†)ḂB,(Ya)AȦ=ϵABϵȦḂ(Ya†)ḂB.
The reality conditions ensures that the basic degrees of freedom of an 𝒩=8 multiplet consist in eight real bosons and fermions. Compared with the free theory discussed above, the supersymmetry transformations are modified as
(4.8)[Qαȧ,Φi]=i(Γ̃i)ȧaYαa,{Qαȧ,Yβa}=(γμ)αβDμΦi(Γi)aȧ+ϵαβΦiΦj†Φk(Γijk)aȧ.
The lowest state of the mth KK supermultiplet is given by TrΦm which is schematic expression for a product of m fields Φik or Φik† completely symmetrized in their SO(8) indices and with all the traces removed
(4.9)Φ{i1Φi2†Φi3Φi4†⋯Φim}†-traces.
In order to have a gauge invariant expression m must be even and Φ and Φ† should be alternated. The other states are obtained, similarly to the free case, by applying the supersymmetry transformations. Let us quote, for example, the schematic form of the scalar 0-(1) and the vector 1-(1) with dimension (m+2)/2(4.10)Tr⁡(Y[α{aYβ]b}†+Φ[i1Φi2†Φi3Φi4]†)Φm-2,Tr⁡(Y{α[aYβ}b]†+γαβμΦ[i1DμΦi2]†)Φm-2.


### 4.2. The SW Spectrum

The KK spectrum ofS7/ℤk is also known [39]. ℤk acts by reducing the length of a circle in S7 and, for large k, the orbifold quotient is equivalent to a type IIA reduction of the theory along this circle. As a result, for large k, the KK spectrum of M theory on S7/ℤk is the same as the KK spectrum of type IIA on ℂℙ3. To obtain the type IIA spectrum we just need to decompose the SO(8) representations under the residual SU(4)×U(1) group and project out all the states that are not invariant under the U(1) action. This decomposition was exhaustively studied in [39]: the levels with m odd are completely projected out, while the levels labelled by even values of m organize themselves into 𝒩=6 susy multiplets. The resulting spectrum exactly reproduces the set of chiral multiplets of the ABJM theory [6]. (This is strictly correct in the k→∞ limit. For finite k, some Fourier modes along the M theory circle survive the projection. These states are D0branes in type IIA and are realized in the ABJM model with monopole operators. We will not discuss explicitly such states in the paper.)Consider now the skew-whiffed theory. The skew-whiffing transformation corresponds to a change of chirality for the eight-dimensional fermion:8s→8c. This transformation can be easily implemented on the KK spectrum of S7 given in Table 2. We maintain the dimension Δ invariant while we exchange the spinorial indices in the SO(8) representations: [a,b,c,d]→[a,b,d,c]. After this transformation, we decompose again the SO(8) representations under the residual SU(4)×U(1) group and project out all the states that are not invariant under the U(1) action. For odd m we obtain “multiplets” with only fermionic degrees of freedom: all the bosons are projected out; for even m we obtain “multiplets” with only bosonic degrees of freedom: all the fermions are projected out. The result is reported in Tables 3 and 4.Table 3
Bosonic KK spectrum of the SW theory at levelm=2n, with n≥1. The states with negative Dynkin labels should be excluded. In the case n=1 some of the fields are absent, reflecting the fact that the original S7 multiplet is shorter.
SpinSU(4)Δ2+[n-1,0,n-1]n+21-(1)[n-1,0,n-1]+[n,0,n]+[n,1,n-2]+[n-2,1,n]n+11+[n-1,0,n-1]+[n-1,0,n-1]+[n+1,0,n-3]+[n-3,0,n+1]+[n,1,n-2]+[n-2,1,n]+[n-1,1,n-3]+[n-3,1,n-1]+[n-2,2,n-2]n+21-(2)[n-1,0,n-1]+[n-2,0,n-2]+[n-1,1,n-3]+[n-3,1,n-1]n+30+(1)[n,0,n]n0-(1)[n-1,0,n-1]+[n+1,0,n-3]+[n-3,0,n+1]+[n,1,n-2]+[n-2,1,n]+[n-1,2,n-1]n+10+(2)[n-1,0,n-1]+[n,0,n]+[n-2,0,n-2]+[n,1,n-2]+[n-2,1,n]+[n-1,1,n-3]+[n-3,1,n-1]+[n-2,2,n-2]+[n,2,n-4]+[n-4,2,n]n+20-(2)[n-1,0,n-1]+[n+1,0,n-3]+[n-3,0,n+1]+[n-1,1,n-3]+[n-3,1,n-1]+[n-3,2,n-3]n+30+(3)[n-2,0,n-2]n+4Table 4
Fermionic KK spectrum of the SW theory at levelm=2n+1, with n≥1. The states with negative Dynkin labels should be excluded. In the case n=1 some of the fields are absent, reflecting the fact that the original S7 multiplet is shorter.
SpinSU(4)Δ32(1)[n+1,0,n-1]+[n-1,0,n+1]+[n-1,1,n-1]n+232(2)[n,0,n-2]+[n-2,0,n]+[n-1,1,n-1]n+312(1)[n+1,0,n-1]+[n-1,0,n+1]+[n,1,n]n+112(2)[n+1,0,n-1]+[n-1,0,n+1]+[n,0,n-2]+[n-2,0,n]+[n,1,n]+[n-1,1,n-1]+[n-1,1,n-1]+[n+1,1,n-3]+[n-3,1,n+1]+[n,2,n-2]+[n-2,2,n]n+212(3)[n,0,n-2]+[n-2,0,n]+[n+1,0,n-1]+[n-1,0,n+1]+[n-1,1,n-1]+[n-1,1,n-1]+[n-2,1,n-2]+[n+1,1,n-3]+[n-3,1,n+1]+[n-1,2,n-3]+[n-3,2,n-1]n+312(4)[n,0,n-2]+[n-2,0,n]+[n-2,1,n-2]n+4Let us consider now the non-supersymmetric field theory discussed in the previous section. It obviously difficult to predict the spectrum of operators with finite dimensions in a non-supersymmetric theory. However, we should at least be able to construct a gauge invariant operator with the right quantum numbers for each of KK state. We will see now that the proposed field content is compatible with the distinctive features of the KK spectrum.The dimensionsΔ of the KK states are all integers. This is compatible with our assumption that the elementary fields have classical dimensions (1/2 for the bosons and 1 for the fermions) since, with this assumption, all the gauge invariant operators have integer dimensions. Let us see this in detail. Consider a gauge invariant product of m elementary fields. Consider first the case with m even. The bosonic operators have integer dimensions: the dual field theory operators are obtained with an even number of bosonic fields and an even number of fermionic fields; gauge invariant operators of this type are obtained using XA and ΨI, or ξ fields. The fermionic operators would have half-integer dimensions: in fact they would contain an odd number of bosonic fields and odd number of fermionic fields. However, in the proposed field theory it is not possible to build up a gauge invariant operator with such field content. We conclude that for even m there are only bosons in the KK spectrum. Consider now the case with m odd. The fermionic operators have integer dimensions: the dual field theory operators are obtained with an even number of bosonic fields and an odd number of fermionic fields; gauge invariant operators of this type are obtained using XA and ΨI, or ξ fields. The bosonic operators instead would have half-integer dimensions, in fact they would contain an odd number of bosonic fields and an even number of fermionic fields. Such bosonic operators are still forbidden by gauge invariance. We conclude that for odd m there are only fermions in the spectrum.Let us now check that we can construct at least one field theory operator with the right dimension, Lorentz andSU(4) representation for each KK mode in supergravity. The gauge invariant field theory operators are obtained by contracting the following operators:
(4.11){XA,XA†,ξα,ξα†,ΨαI,Dμ}.
Let us start looking at the generic form of the operators of low dimension for a given n. The first scalar KK modes is 0+(1) and the corresponding field theory operator has the schematic form
(4.12)Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†),
where suitable trace subtractions are understood. The first KK spinor mode is (1/2)(1) and the dual operator is
(4.13)Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†ΨαI).
The first KK vector mode is 1(-1) and the dual operator is
(4.14)Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†Ψ{α[IΨβ}J])+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†ξ{αξβ}†)+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†XAnDμXBn†).
The first pseudoscalar in the KK spectrum is 0(-1) and the dual field operator is schematically
(4.15)Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†Ψ[α{IΨβ]J})+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†ξ[αξβ]†)+Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†X[AX[B†XC]XD]†).
Another interesting operator of lower dimension in the KK towers is (3/2)(1) and its dual field operator has the form
(4.16)Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†Ψ{α[IΨβJΨγ}K])+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†Ψ{αIξβξγ}†)+Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†DμΨαI).It is easy to verify that the above operators can reproduce theSU(4) representations reported in Tables 3 and 4. The first bosonic level has m=2 and the corresponding operators have the schematic form
(4.17)0+(1):Tr⁡(XAXB†),0-(1):Tr⁡(Ψ[α{IΨβ]J})+Tr⁡(ξ[α†ξβ])+Tr⁡(X[AX[B†XC]XD]†),1-(1):Tr⁡(XADμXB†)+Tr⁡(ξ{α†ξβ})+Tr⁡(Ψ{α[IΨβ}J]),2+:Tr⁡(DμXADνXA†)+⋯,
where suitable trace subtractions are understood. In the first bosonic level there are two important operators: the part of the 1-(1) operator in the [1,0,1] representation is the field theory SU(4) global current symmetry Jμ[IJ] dual to the gauge field Aμ[IJ] in the adjoint representation of SU(4) propagating in AdS4, and the singlet 2+ operator is the stress-energy tensor dual to the graviton gμν in AdS4. Of course, since the proposed skew-whiffed theory is not supersymmetric, the supercurrent operator dual to the would be (3/2)(1) gravitino is not present in the operator spectrum.The first fermionic level hasm=3 and the corresponding operators are
(4.18)12(1):Tr⁡(XAXB†ΨαI),12(2):Tr⁡(Ψ{α[IΨ[β}{J]Ψγ]K})+Tr⁡(Ψ{αIξ[β}ξγ]†)+Tr⁡(X[AX[B†XC]XD]†ΨαI),32(1):Tr⁡(Ψ{α[IΨβJΨγ}K])+Tr⁡(Ψ{αIξβξγ}†)+Tr⁡(XAXB†DμΨI),32(2):Tr⁡(ξ[αξβ]†DμΨγI)+⋯.
(The operators corresponding (1/2)(2) have a mixed symmetry in the spin and SU(4) indices which is indicated in a somehow imprecise way in the following formula.)The operators dual to a specific KK modes are, in general, linear combinations of all the gauge invariant operators with the right dimension, Lorentz andSU(4) representation that we can construct. The expectation is that exactly one of these operators will remain with finite dimensions in the large N and strongly coupled regime, while the others will acquire infinite dimension, as standard in the AdS/CFT correspondence.


## 4.1. The Spectrum onS7

The KK spectrum of the M-theory Freud-Rubin solution onS7 is well known [33, 34] and reported for completeness in Table 2. The states are classified by the dimension and the representation under SO(8) and are organized in superconformal multiplets specified by an integer number m≥2. The lowest state in each multiplet is scalar field of dimension m/2 transforming in the [m,0,0,0] representation of SO(8). The other states are obtained by acting on the lowest state with the 𝒩=8 supersymmetries transforming as 8c=[0,0,0,1] under SO(8). The multiplet is short and has spin range equal to two, compared with the spin range of four of a long multiplet. The multiplets m=2,3 sustain further shortenings; m=2 corresponds to the massless multiplet of the 𝒩=8 gauged supergravity. Partition functions encoding the spectrum of S7 (and of its quotient) in a related context can be found in [35–38].Table 2
The spectrum onS7.
SpinSO(8)Δ2+[m-2,0,0,0]m+4232(1)[m-2,0,0,1]m+3232(2)[m-3,0,1,0]m+521-(1)[m-2,1,0,0]m+221+(2)[m-3,0,1,1]m+421-(2)[m-4,1,0,0]m+6212(1)[m-1,0,1,0]m+1212(2)[m-3,1,1,0]m+3212(3)[m-4,1,0,1]m+5212(4)[m-4,0,0,1]m+720+(1)[m,0,0,0]m20-(1)[m-2,0,2,0]m+220+(2)[m-4,2,0,0]m+420-(2)[m-4,0,0,2]m+620+(3)[m-4,0,0,0]m+82We can understand the structure of the multiplets by considering a very simple theory of eight free bosonsΦi and eight free fermions Ya. These are the expected degrees of freedom living on a membrane in flat space. The lowest state of the m-th KK supermultiplet can be represented by Φm, which is a schematic expression for the product of m fields completely symmetrized in their SO(8) indices and with all the traces removed:
(4.1)Φm≡Φ{i1⋯Φim}-traces.
The other states are obtained by applying the supersymmetry transformations that schematically read
(4.2)[Qαȧ,Φi]=i(Γ̃i)ȧaYαa,{Qαȧ,Yβa}=(γμ)αβDμΦi(Γi)aȧ.
The first spinorial state (1/2)(1) with dimension (m+1)/2 reads
(4.3)YαaΦm-1,
where, again, Φm will represent a fully symmetrized and traceless string of fields Φik. The indices are contracted in such a way that the operator transforms as [m-1,0,1,0]. The states with dimension (m+2)/2 are obtained by applying two supercharges whose Lorentz indices can be antisymmetrized or symmetrized giving a scalar 0-(1) and a vector 1-(1) of schematic form
(4.4)Y[α{aYβ]b}Φm-2,(Y{α[aYβ}b]+γαβμΦ[i1DμΦi2])Φm-2.
The fermionic bilinears transform in the [0,0,2,0] and [0,1,0,0] representation of SO(8), respectively, which can be contracted with [m-2,0,0,0] to give the expected representations [m-2,0,2,0] and [m-2,1,0,0] given in Table 2. The states with dimension (m+3)/2 read schematically
(4.5)(YαaYβbYγc+⋯)Φm-3.
The Lorentz indices can be completely symmetric or with mixed symmetry; we obtain a state (3/2)(1) with three SO(8) indices transforming in the [1,0,0,1] and a state (1/2)(2) with three indices [0,1,1,0], respectively. Combining with the bosonic part we easily recover the representations [m-2,0,0,1] and [m-3,1,1,0] reported in Table 2. The states with dimension (m+4)/2 have four fermions whose Lorentz indices can be contracted in order to give a scalar 0+(2), a vector 1+(2), and a spin two 2+. We can write, for example, the schematic form of the spin two operator in the [m-2,0,0,0] representation of SO(8),
(4.6)DμΦiDνΦiΦm-2+Y{α1[a1⋯Yα4}a4]Φm-4+⋯.
The scalar and vector are obtained with different contraction of the Lorentz indices; it is easy to check that the SO(8) indices then transform as reported in Table 2. The rest of the spectrum can be similarly reconstructed.The KK spectrum onS7 should reproduce the full spectrum of short operators with finite dimensions in the large N limit of the field theory dual to AdS4×S7. It is however difficult to write explicit expressions for these multiplets in terms of local operators. The ABJM theory with k=1 is an explicitly scale invariant local Lagrangian dual to AdS4×S7 and its spectrum of single trace chiral operators should match the KK spectrum on S7. However, the explicit correspondence is somehow obscured by the fact that the 𝒩=8 supersymmetry of ABJM is not manifest and monopole operators are required to match the spectrum. In the particular case N=2, the ABJM theory with group SU(2)×SU(2) has manifest 𝒩=8 supersymmetry and SO(8) global symmetry; in fact it coincides with the BLG theory [1–5]. However, even in this case we can only give an explicit representation for the multiplets with even m. Let us discuss briefly how. We use the formulation as a Chern-Simons theory with gauge group SU(2)×SU(2). The matter content consist of bosonic and fermionic fields Φi and Ya transforming in the bifundamental representation of the gauge group and in the 8v in the 8s representation of SO(8), respectively. The fields can be written as two-by-two matrices satisfying the reality condition
(4.7)ΦAȦi=ϵABϵȦḂ(Φi†)ḂB,(Ya)AȦ=ϵABϵȦḂ(Ya†)ḂB.
The reality conditions ensures that the basic degrees of freedom of an 𝒩=8 multiplet consist in eight real bosons and fermions. Compared with the free theory discussed above, the supersymmetry transformations are modified as
(4.8)[Qαȧ,Φi]=i(Γ̃i)ȧaYαa,{Qαȧ,Yβa}=(γμ)αβDμΦi(Γi)aȧ+ϵαβΦiΦj†Φk(Γijk)aȧ.
The lowest state of the mth KK supermultiplet is given by TrΦm which is schematic expression for a product of m fields Φik or Φik† completely symmetrized in their SO(8) indices and with all the traces removed
(4.9)Φ{i1Φi2†Φi3Φi4†⋯Φim}†-traces.
In order to have a gauge invariant expression m must be even and Φ and Φ† should be alternated. The other states are obtained, similarly to the free case, by applying the supersymmetry transformations. Let us quote, for example, the schematic form of the scalar 0-(1) and the vector 1-(1) with dimension (m+2)/2(4.10)Tr⁡(Y[α{aYβ]b}†+Φ[i1Φi2†Φi3Φi4]†)Φm-2,Tr⁡(Y{α[aYβ}b]†+γαβμΦ[i1DμΦi2]†)Φm-2.


## 4.2. The SW Spectrum

The KK spectrum ofS7/ℤk is also known [39]. ℤk acts by reducing the length of a circle in S7 and, for large k, the orbifold quotient is equivalent to a type IIA reduction of the theory along this circle. As a result, for large k, the KK spectrum of M theory on S7/ℤk is the same as the KK spectrum of type IIA on ℂℙ3. To obtain the type IIA spectrum we just need to decompose the SO(8) representations under the residual SU(4)×U(1) group and project out all the states that are not invariant under the U(1) action. This decomposition was exhaustively studied in [39]: the levels with m odd are completely projected out, while the levels labelled by even values of m organize themselves into 𝒩=6 susy multiplets. The resulting spectrum exactly reproduces the set of chiral multiplets of the ABJM theory [6]. (This is strictly correct in the k→∞ limit. For finite k, some Fourier modes along the M theory circle survive the projection. These states are D0branes in type IIA and are realized in the ABJM model with monopole operators. We will not discuss explicitly such states in the paper.)Consider now the skew-whiffed theory. The skew-whiffing transformation corresponds to a change of chirality for the eight-dimensional fermion:8s→8c. This transformation can be easily implemented on the KK spectrum of S7 given in Table 2. We maintain the dimension Δ invariant while we exchange the spinorial indices in the SO(8) representations: [a,b,c,d]→[a,b,d,c]. After this transformation, we decompose again the SO(8) representations under the residual SU(4)×U(1) group and project out all the states that are not invariant under the U(1) action. For odd m we obtain “multiplets” with only fermionic degrees of freedom: all the bosons are projected out; for even m we obtain “multiplets” with only bosonic degrees of freedom: all the fermions are projected out. The result is reported in Tables 3 and 4.Table 3
Bosonic KK spectrum of the SW theory at levelm=2n, with n≥1. The states with negative Dynkin labels should be excluded. In the case n=1 some of the fields are absent, reflecting the fact that the original S7 multiplet is shorter.
SpinSU(4)Δ2+[n-1,0,n-1]n+21-(1)[n-1,0,n-1]+[n,0,n]+[n,1,n-2]+[n-2,1,n]n+11+[n-1,0,n-1]+[n-1,0,n-1]+[n+1,0,n-3]+[n-3,0,n+1]+[n,1,n-2]+[n-2,1,n]+[n-1,1,n-3]+[n-3,1,n-1]+[n-2,2,n-2]n+21-(2)[n-1,0,n-1]+[n-2,0,n-2]+[n-1,1,n-3]+[n-3,1,n-1]n+30+(1)[n,0,n]n0-(1)[n-1,0,n-1]+[n+1,0,n-3]+[n-3,0,n+1]+[n,1,n-2]+[n-2,1,n]+[n-1,2,n-1]n+10+(2)[n-1,0,n-1]+[n,0,n]+[n-2,0,n-2]+[n,1,n-2]+[n-2,1,n]+[n-1,1,n-3]+[n-3,1,n-1]+[n-2,2,n-2]+[n,2,n-4]+[n-4,2,n]n+20-(2)[n-1,0,n-1]+[n+1,0,n-3]+[n-3,0,n+1]+[n-1,1,n-3]+[n-3,1,n-1]+[n-3,2,n-3]n+30+(3)[n-2,0,n-2]n+4Table 4
Fermionic KK spectrum of the SW theory at levelm=2n+1, with n≥1. The states with negative Dynkin labels should be excluded. In the case n=1 some of the fields are absent, reflecting the fact that the original S7 multiplet is shorter.
SpinSU(4)Δ32(1)[n+1,0,n-1]+[n-1,0,n+1]+[n-1,1,n-1]n+232(2)[n,0,n-2]+[n-2,0,n]+[n-1,1,n-1]n+312(1)[n+1,0,n-1]+[n-1,0,n+1]+[n,1,n]n+112(2)[n+1,0,n-1]+[n-1,0,n+1]+[n,0,n-2]+[n-2,0,n]+[n,1,n]+[n-1,1,n-1]+[n-1,1,n-1]+[n+1,1,n-3]+[n-3,1,n+1]+[n,2,n-2]+[n-2,2,n]n+212(3)[n,0,n-2]+[n-2,0,n]+[n+1,0,n-1]+[n-1,0,n+1]+[n-1,1,n-1]+[n-1,1,n-1]+[n-2,1,n-2]+[n+1,1,n-3]+[n-3,1,n+1]+[n-1,2,n-3]+[n-3,2,n-1]n+312(4)[n,0,n-2]+[n-2,0,n]+[n-2,1,n-2]n+4Let us consider now the non-supersymmetric field theory discussed in the previous section. It obviously difficult to predict the spectrum of operators with finite dimensions in a non-supersymmetric theory. However, we should at least be able to construct a gauge invariant operator with the right quantum numbers for each of KK state. We will see now that the proposed field content is compatible with the distinctive features of the KK spectrum.The dimensionsΔ of the KK states are all integers. This is compatible with our assumption that the elementary fields have classical dimensions (1/2 for the bosons and 1 for the fermions) since, with this assumption, all the gauge invariant operators have integer dimensions. Let us see this in detail. Consider a gauge invariant product of m elementary fields. Consider first the case with m even. The bosonic operators have integer dimensions: the dual field theory operators are obtained with an even number of bosonic fields and an even number of fermionic fields; gauge invariant operators of this type are obtained using XA and ΨI, or ξ fields. The fermionic operators would have half-integer dimensions: in fact they would contain an odd number of bosonic fields and odd number of fermionic fields. However, in the proposed field theory it is not possible to build up a gauge invariant operator with such field content. We conclude that for even m there are only bosons in the KK spectrum. Consider now the case with m odd. The fermionic operators have integer dimensions: the dual field theory operators are obtained with an even number of bosonic fields and an odd number of fermionic fields; gauge invariant operators of this type are obtained using XA and ΨI, or ξ fields. The bosonic operators instead would have half-integer dimensions, in fact they would contain an odd number of bosonic fields and an even number of fermionic fields. Such bosonic operators are still forbidden by gauge invariance. We conclude that for odd m there are only fermions in the spectrum.Let us now check that we can construct at least one field theory operator with the right dimension, Lorentz andSU(4) representation for each KK mode in supergravity. The gauge invariant field theory operators are obtained by contracting the following operators:
(4.11){XA,XA†,ξα,ξα†,ΨαI,Dμ}.
Let us start looking at the generic form of the operators of low dimension for a given n. The first scalar KK modes is 0+(1) and the corresponding field theory operator has the schematic form
(4.12)Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†),
where suitable trace subtractions are understood. The first KK spinor mode is (1/2)(1) and the dual operator is
(4.13)Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†ΨαI).
The first KK vector mode is 1(-1) and the dual operator is
(4.14)Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†Ψ{α[IΨβ}J])+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†ξ{αξβ}†)+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†XAnDμXBn†).
The first pseudoscalar in the KK spectrum is 0(-1) and the dual field operator is schematically
(4.15)Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†Ψ[α{IΨβ]J})+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†ξ[αξβ]†)+Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†X[AX[B†XC]XD]†).
Another interesting operator of lower dimension in the KK towers is (3/2)(1) and its dual field operator has the form
(4.16)Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†Ψ{α[IΨβJΨγ}K])+Tr⁡(X{A1X{B1†⋯⋯XAn-1}XBn-1}†Ψ{αIξβξγ}†)+Tr⁡(X{A1X{B1†⋯⋯XAn}XBn}†DμΨαI).It is easy to verify that the above operators can reproduce theSU(4) representations reported in Tables 3 and 4. The first bosonic level has m=2 and the corresponding operators have the schematic form
(4.17)0+(1):Tr⁡(XAXB†),0-(1):Tr⁡(Ψ[α{IΨβ]J})+Tr⁡(ξ[α†ξβ])+Tr⁡(X[AX[B†XC]XD]†),1-(1):Tr⁡(XADμXB†)+Tr⁡(ξ{α†ξβ})+Tr⁡(Ψ{α[IΨβ}J]),2+:Tr⁡(DμXADνXA†)+⋯,
where suitable trace subtractions are understood. In the first bosonic level there are two important operators: the part of the 1-(1) operator in the [1,0,1] representation is the field theory SU(4) global current symmetry Jμ[IJ] dual to the gauge field Aμ[IJ] in the adjoint representation of SU(4) propagating in AdS4, and the singlet 2+ operator is the stress-energy tensor dual to the graviton gμν in AdS4. Of course, since the proposed skew-whiffed theory is not supersymmetric, the supercurrent operator dual to the would be (3/2)(1) gravitino is not present in the operator spectrum.The first fermionic level hasm=3 and the corresponding operators are
(4.18)12(1):Tr⁡(XAXB†ΨαI),12(2):Tr⁡(Ψ{α[IΨ[β}{J]Ψγ]K})+Tr⁡(Ψ{αIξ[β}ξγ]†)+Tr⁡(X[AX[B†XC]XD]†ΨαI),32(1):Tr⁡(Ψ{α[IΨβJΨγ}K])+Tr⁡(Ψ{αIξβξγ}†)+Tr⁡(XAXB†DμΨI),32(2):Tr⁡(ξ[αξβ]†DμΨγI)+⋯.
(The operators corresponding (1/2)(2) have a mixed symmetry in the spin and SU(4) indices which is indicated in a somehow imprecise way in the following formula.)The operators dual to a specific KK modes are, in general, linear combinations of all the gauge invariant operators with the right dimension, Lorentz andSU(4) representation that we can construct. The expectation is that exactly one of these operators will remain with finite dimensions in the large N and strongly coupled regime, while the others will acquire infinite dimension, as standard in the AdS/CFT correspondence.


## 5. Conclusions

In this paper we discussed general properties of the field theory living on a stack ofN anti-M2 branes at the tip of an eight-dimensional real cone with at least one Killing spinor. In particular we focus on the skew-whiffed AdS4×S7/ℤk supergravity solution in M theory (and its reduction to type IIA), which is not supersymmetric but stable. The AdS/CFT correspondence predicts the existence of a dual non-supersymmetric three-dimensional theory, which should be a unitary conformal field theory at least at large N and strong coupling. Based on an analysis of the KK spectrum of the supergravity theory and on the geometrical action of the skew-whiffing transformation, we speculate on the field content of the dual theory, a skew-whiffed version of the ABJM theory. Due to the fact that the theory is non-supersymmetric, direct checks of any proposal are nontrivial. We identified a field content which is at least compatible with the KK spectrum found in the dual supergravity solution. It is interesting to observe that there is some ambiguity in writing a candidate theory. In particular the SW map and the compatibility with the KK spectrum do not fix unambiguously the representation of the fields under the gauge group; for example, the complex spinor ξ could be either in the bifundamental representation, as we considered in this paper, or in the adjoint representation of one of the gauge group. It would be interesting to see if these various theories are somehow duals. Another observation is that the proposed theory is not really a quiver gauge theory, because the fermions transform in the bifundamental of just the SU(N) part of the full U(N) gauge group. This seems to imply that the theory is a good candidate only in the large N limit, that is exactly, the regime for which the dual supergravity solution is demonstrated to be stable. Further investigations are needed.We mainly concentrated on theS7/ℤk supergravity solution. However, as explained at the very beginning of the paper, there is a SW supergravity solution for any Freud-Rubin solution with at least one Killing spinor and we should be able to find a dual non-supersymmetric Chern-Simons matter theory. There is an infinite set of AdS4/CFT3 pairs in the literature and it would be interesting to have a systematic procedure to obtain the SW field theory once the supersymmetric field theory is known. One way to proceed would be to start with orbifolds of the SW ABJM theory. By giving vevs to scalar fields we can flow to other non-supersymmetric Chern-Simons matter field theories. A more efficient way to proceed would be to find the field theory operation dual to the change of orientation of H7. We leave this topic for future research.



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*Source: 393645-2011-09-22.xml*