SYK/AdS duality with Yang-Baxter deformations

In this paper, based on the notion of SYK/AdS duality we explore the effects of Yang-Baxter (YB) deformations on the SYK spectrum at strong coupling. In the first part of our analysis, we explore the consequences of YB deformations through the Kaluza-Klein (KK) reduction on $ (AdS_2)_{\eta}\times (S^1)/Z_2 $. It turns out that the YB effects (on the SYK spectrum) starts showing off at \textit{quadratic} order in $ 1/J $ expansion. For the rest of the analysis, we provide an interpretation for the YB deformations in terms of bi-local/collective field excitations of the SYK model. Using large $ N $ techniques, we evaluate the effective action upto quadratic order in the fluctuations and estimate $ 1/J^2 $ corrections to the correlation function at strong coupling.

Abstract: In this paper, based on the notion of SYK/AdS duality we explore the effects of Yang-Baxter (YB) deformations on the SYK spectrum at strong coupling. In the first part of our analysis, we explore the consequences of YB deformations through the Kaluza-Klein (KK) reduction on (AdS 2 ) η × (S 1 )/Z 2 . It turns out that the YB effects (on the SYK spectrum) starts showing off at quadratic order in 1/J expansion. For the rest of the analysis, we provide an interpretation for the YB deformations in terms of bi-local/collective field excitations of the SYK model. Using large N techniques, we evaluate the effective action upto quadratic order in the fluctuations and estimate 1/J 2 corrections to the correlation function at strong coupling.

Overview and Motivation
Very recently, the SYK model [1]- [22] has been proposed as one of those handful examples (within the realm of AdS/CFT correspondence) where one might hope to solve the spectrum associated with the quantum mechanical system at strong coupling 1 . Other than its solvability, this (1 + 0)D system of (N 1) fermions possesses two other remarkable features namely,-(I) the Lyapunov exponent associated with the out of time ordered four point correlators saturates the bound [24]- [26] and (II) the emerging scale invariance at low energies. Understanding the dual gravitational counterpart [27]- [33] corresponding to the SYK model had always been challenging until very recently [34]- [36]. In [34], the authors provide a very solid evidence in favour of the dual 3D gravitational counterpart corresponding to the zero temperature version of the model where they explore the Kaluza-Klein (KK) tower associated with the scalar field excitations on AdS 2 × (S 1 )/Z 2 . In the strict IR (|Jt| 1) limit, the metric along the compact third direction becomes constant, whereas on the other hand, away from the fixed point it acquires non trivial dependence on the AdS 2 coordinates through the dilaton profile. In their analysis [34], the authors explore the 1/J corrections to the zero modes of the theory and compute the strong coupling corrections to the propagator that precisely matches to that with the earlier results in [8]. The purpose of the present paper is to explore and understand this duality conjecture in the presence of so called Yang-Baxter (YB) deformations 2 [37]- [39] and also to understand its possible consequences on the corresponding bi-local excitations [13]- [14] associated with the SYK model at strong coupling. The motivation behind our analysis strictly follows from holography where we start with the deformed AdS 2 version of the theory in the bulk [37] and lift it to three dimensions in order to compute the KK spectrum associated with the scalar field excitations in the dual gravitational counterpart. Our analysis reveals that the holographic correspondence between the SYK model and its dual gravitational counterpart brings into a non trivial 1/J 2 corrections to the spectrum of the SYK model which has its origin in the YB deformations associated with the (AdS 2 ) η ×(S 1 )/Z 2 theory in (2+1) D. For the rest of our analysis, we search for an interpretation of such deformations in terms of collective field excitations [41] associated with the SYK model. Looking at the holographic side of the duality, we propose a possible YB scaling of the collective excitations within the SYK model and compute the effective action at quadratic order in the fluctuations (around IR critical point) and thereby the corresponding propagator at strong coupling (|Jt| 1). Our analysis reveals that the effective action receives non trivial 1/J 2 corrections that has remarkable structural similarity to that with the corresponding quadratic action associated with scalar field excitations computed on the dual gravitational counterpart of the theory. The organisation of the paper is as follows: In section 2, we briefly review the YB deformations to the Almheiri-Polchinski (AP) model [37]- [39]. In section 3, we compute the zero modes associated with the spectrum and estimate the 1/J 2 corrections to it. In section 4, we provide a possible interpretation of the YB effects on the collective excitations within the SYK model. Finally, we conclude in section 5.

The deformed AP model
The purpose of this Section is to provide a formal introduction to the Almheiri-Polchinski (AP) model [29] and its Yang-Baxter (YB) form of deformations introduced very recently in [37]. The Yang-Baxter (YB) deformation of the AdS 2 metric is based on the usual notion of coset space formulation of the 2D non-linear sigma model that acts both on the metric as well as the anti-symmetric two form field. For the metric part, the YB deformation was introduced as [37], where, η is the deformation parameter. Here, the left invariant one form J(∈ sl (2)) is defined as usual, where g is an element of SL(2)/U (1). The projection could be defined as follows [37], together with the chain operation of the following form, where the linear operator R satisfies the modified classical YB (mCYBE) equation of the following form, where, c = 0 for mCYBE and c = 0 for homogeneous CYBE [37]. Taking the generators, T I ∈ so (1,2) in the fundamental representation, (where, σ I s are the Pauli matrices) a straightforward calculation of (2.1) reveals [37], where, the function F η (X.P ) could be formally expressed as, Here, α, β and γ are three constant parameters of the theory that satisfy the following constraint, Clearly in the limit, η → 0 one recovers the usual AdS 2 metric as a part of the full background solutions corresponding to the AP model [29]. The major accomplishment of [37] was to embed the above YB deformed AdS 2 metric (2.7) as a solution within 1 + 1 D dilaton gravity system 3 , with a particular type of η modification introduced to the dilaton potential (U (Φ)) that drives the potential from its standard quadratic form to a hyperbolic function. The resulting dilaton profile could be formally expressed as [37],

3D holography
In this section we intend to build up a notion for 3D holography in the presence of YB deformations described above. The first step towards this direction would be to uplift the deformed AP model (2.10) in one higher dimension by introducing an additional compact direction (Θ) and compute the corresponding scalar spectrum associated with Kaluza-Klein (KK) modes [34].

A 3D uplift
We propose the 3D metric of the following form, A straightforward computation reveals, where 4 , and Σ I is the corresponding volume of the compact manifold. As a trivial check of our analysis, we first notice that in the limit, η → 0 and with the following choice of the metric, one correctly reproduces the desired form of the dilaton potential [37], The above scenario generalizes quite non-trivially for non zero deformations, that reproduces the desired form of the dilaton potential [37], Therefore like in the undeformed scenario, the YB deformed (1+1) D dilaton gravity could be uplifted to (2 + 1) D with dilaton being the third direction. The above background (3.1) would serve as the starting point of our subsequent analysis.

Kaluza-Klein modes
The purpose of this Section is to obtain the KK spectrum of a single scalar field (φ) over the η deformed background (3.1) obtained previously. We start with the scalar action of the following form, is the delta function potential as usual [34]. In the subsequent analysis we focus on the case with homogeneous CYBE which amounts of setting [37], and simplifies the background metric (3.1) as, (3.10) In the following we (Fourier) decompose the scalar field as, which finally yields the scalar action of the following form, where, the individual operators could be formally expressed as 5 , Notice that like in the undeformed scenario [34], the zeroth order operator D 0 (and hence the associated Green's function) does not receive any η corrections. However, the operator at next to leading order modifies substantially due to YB deformations, For n = 1 one has the usual contribution as in the undeformed case. Quite interestingly, the η modification appears with, n = 2 which is an effect associated to O(α 2 ). Therefore, strictly at linear order in α(∼ 1/J) [34] one should not expect to find any of the imprints of YB deformations on the SYK spectrum.

Eigenfunctions of D 0
The eigenfunctions corresponding to the operator D 0 are clearly separable, where the function f K (Θ) satisfies Schrodinger equation of the following form, In our calculations, we stick to the parity even sector [34] of the wave function, with, E = K 2 . Clearly, with the above choice of the wave function (3.18) one ends up with the following boundary conditions 6 , Next, integrating (3.17) within a small interval around Θ ∼ 0 we notice, which upon substitution of (3.19) yields the following transcendental equation, whose solutions could be formally denoted as p a with a(= 0, 1, 2, ..) being an integer and 2a + 1 < p a < 2a + 2 [34].

Eigenfunctions of D (η)
Likewise, we separate the eigenfunctions of the operator D (η) as, where, fK n is the eigenfunction corresponding to the operator F n defined in (3.15), Restricting ourselves to the parity even sector of the wave function (3.18) it is trivial to arrive at the following set of transcendental equations, Notice that the second Eq.(3.25) makes sense only in the presence of YB deformations (η = 0). As we shall see, the eigenfunctions corresponding to F 2 introduce a non trivial shift in the SYK spectrum at strong couplings. We denote the solutions corresponding to the above set of equations (3.24)-(3.25) as 2a + 1 < q (n) a < 2a + 2 where, n = 1, 2 refers to F 1 and F 2 respectively. We focus our attention on the first two roots (1 < q (2) 0 < 2 and 3 < q (2) 1 < 4) corresponding to F 2 and explore their functional dependence with the deformation parameter (η). To see this explicitly 6 For the moment we ignore the overall normalization constant.

Green's functions
Given the desired choices for the parameters (V, L) of the theory, we now compute the Green's function corresponding to the operator, D ≡ D 0 + D (η) . It is naturally expected that the effects of YB deformations on the SYK spectrum would appear through the Green's function corresponding to the operator D (η) .

Zeroth order solution
The solution corresponding to the zeroth order propagator, remains the same as in the undeformed scenario 7 [34]. Setting, Θ = 0 = Θ into (A.13) one finally obtains, where we note, . (3.32) Setting, m 2 = −1/4 the integral I(z, z ) could be expressed as a sum of two terms [34], where, the index ν is real. The above entity (3.33) has discrete poles at ν = p a (on real ν axis) and is clearly valid for ν = 3/2 + 2n (n = 0, 1, 2...) for which ξ ν = 0 [7]. This corresponds to bound energy (eigen)states with eigenvalues precisely as the roots of the transcendental equation (3.21). The second contribution to the integral I(z, z ) comes from the scattering states [7] with ν = ir (0 < r < ∞) that amount of setting 8 , where, the individual entities in the integrand (3.34) could be formally expressed as, A trivial change in the variable, ν → −ν yields, which thereby simplifies (3.34) as, (3.37) We close the contour on the Re(ν) > 0 plane which essentially extends along the positive real axis of the complex ν plane and extends to infinity along the imaginary 7 See Appendix A for details. 8 The resulting wave function is a linear superposition of these two states [7].
axis. Clearly there are two types of poles within this contour-(I) simple pole at ν = p a and (II) the poles (distributed along the real axis) associated with ξ −ν at ν = 3/2 + 2n, Combining (3.33) and (3.38) finally yields,

YB shift in the spectrum
The purpose of this Section is to compute the first order shift in the energy spectrum corresponding to D (η) and explore the effects of YB deformations at next to leading order in the SYK coupling (α ∼ 1/J). A straightforward calculation reveals, where, we have introduced, (3.41) In order to simplify (3.46), we further notice that, which by means of the following two identities, could be further simplified as 9 , Substituting (3.44) into (3.46) we find, (3.45) 9 One has to replace, ν → −ν in the second of the identities in (3.43).
which finally yields the matrix element of the following form, where the individual matrix elements could be formally expressed as, In order to evaluate the above integrals (3.46) we focus on the bound states with discrete energy eigenvalues corresponding to ν = 3/2 + 2n [7]. This yields the following 10 , (3.49) The second term on the R.H.S. of (3.49) could be repackaged as, is precisely the YB contribution to the SYK spectrum that appears as a next to leading order effect in the SYK coupling (∼ 1/J). Notice that, here ∆k Y B (≥ 0) is manifestly positive definite (as a leading order effect in YB deformations) that shifts the pole of the propagator corresponding to the zero mode by an amount, which could be further expanded as a perturbation in the SYK coupling, Here, we have introduced new variables as, (3.53) 10 We have set, m 2 = −1/4 which corresponds to setting the mass of the KK scalar at its BF bound. Also we have set, ν = ν = 3/2. This corresponds to the zero modes of the spectrum.
Notice that the shift ∆ν (2) is purely a next to leading order (∼ 1/J 2 ) contribution to the spectrum that comes into play in the presence of YB deformations which forces us to consider effects beyond linear order in the perturbation expansion. This finally yields the zero mode contribution to the propagator (3.39) as, ∆ν (2) ∆ν (1) .
Clearly, if one switches off the YB deformation and restricts upto leading order (∼ 1/J) in the perturbation series then, Ω = 1 which reproduces the known results of [8].

Bi-local holography and YB deformations
From the analysis in the previous section, it is indeed quite evident that there are precise holographic confirmations of the perturbative energy shift in the SYK model due to the presence of YB deformations in the bulk counterpart. The purpose of this section is therefore to understand this deformation and in particular its consequences on the (1 + 0)D SYK model in terms of bi-local excitations [13] of the theory.

Brief review of SYK
The SYK model consists of N ( 1) Majorana fermions with all-to-all interactions. This is a quantum mechanical model where the interactions between the fermions are completely random, described by a random coupling constant J ijkl which exhibits a Gaussian distribution with zero mean ( J ijkl = 0) and a non zero variance J ijkl J ijkl = 6J 2 N 3 [7]. After performing the disorder averaging, there is only one coupling constant left in the theory [7], that appears in the effective action. The Hamiltonian of the system could be formally expressed as 11 [7], which leads to the Lagrangian of the following form, The generalization of this model for q point vertex is quite straightforward [8].
Here, χ i s (i = 1, 2, · · · , N ) are the so called Majorana fermions which satisfy the following anti-commutation relation, together with the fact that they are equal to their own antiparticles namely, χ † i = χ i . One can usually calculate the free energy of the system by using the so called replica trick 12 , where, the partition function could be formally expressed as, The action corresponding to the replica SYK is given by 13 [13], where, the index a stands for the so called replica index. In the large N limit, one introduces the bi-local (collective) fields as [13], where, we have suppressed the replica indices for later convenience. This yields the following path integral, with the SYK replica action expressed in terms of collective field excitations (4.8), Notice that since the collective field Ψ ∼ O(N 0 ), therefore the collective action in (4.10) is of ∼ O(N ). The trace term in the action (4.10) takes care of the Jacobian 12 Notice that the replica trick is usually used in systems with quenched disorder in order to overcome the averaging over logarithms. Moreover, there is an amount of ambiguity in taking the limit n → 0 since we start from an integer n. Nevertheless, the results with replica method matches well with other methods. 13 The effective replica action in (4.7) could be obtained after integrating over the random coupling, J ijkl in the path integral [13]. The integral that one evaluates is Gaussian and is of the form, ∼ Dχ i (..) that appears due to the change in the path integral measure from χ i (t) → Ψ(t 1 , t 2 ). In the so called IR (|Jt| 1) limit one could ignore the kinematics of collective field excitations and therefore the collective action (4.10) is approximately reduced to, which clearly has the re-parametrization invariance of the following form, characterizing the IR critical point at strong coupling.

The effective action
The classical saddle point equation has a solution [13], Next, we turn on fluctuations around this IR fixed point and propose the following YB modification to the bi-local excitations, where the YB fluctuations associated to collective excitations 14 , would precisely be identified with the corresponding scalar field d.o.f. living in the YB deformed AdS 2 spacetime. The collective action could be expanded around the IR critical point as, Clearly, the first term on the R.H.S. of (4.16) is of O (N ). Whereas, on the other hand, the second term is of O(N 0 ) which could be formally expressed as, where, the kernel could be formally expressed as [13], (4.18) In the following we evaluate the first term in 15 (4.17), where, in the second line of (4.19) we have used the antisymmetry properties associated with the collective fields namely, This finally yields the effective quadratic action as, (4.21) In order to match our results to that with the (AdS 2 ) η calculations in the preceeding section, we define the following coordinate transformations [13], and expand the fluctuations a complete basis, that is defined as follows [13], where, Z ν (|x|) is a linear combination of Bessel functions defined in (A.9). Following the original prescription of [13], one could further re-express (4.23) as 16 , Using (4.26), one could evaluate the quadratic action (4.21) as 17 , where, we have introduced, . (4.28) The above Eq.(4.27) is one of the key findings of our paper. It turns out that the YB scaling associated with the bi-local fields in the SYK model produces a non trivial shift in the effective action (associated with quadratic fluctuations) at next to leading order (∼ 1/J 2 ) in the coupling which is thereby highly suppressed compared to that with the leading order (∼ 1/J) effects. This observation is clearly compatible with our earlier findings in the previous section. This finally leads to the correlation function, where, we have defined, . (4.30)

The (AdS 2 ) η spectrum
Consider an effective action for scalar fields on AdS 2 [13], where, the metric could be formally expressed as, (4.32) A straightforward calculation reveals, On the other hand, it is trivial to notice that 18 [34], where, we have rescaled the scalar field as 19 ,φ m = ϕm Fη(z) . Notice that here we have introduced a new function,F that precisely goes to unity in the limit of the vanishing YB deoformations and thereby one recovers the original results of [34]. Based on the above analysis, we propose the following non local field redefinition, Substituting (4.36) into (4.31) we obtain, where, the pole has been rescaled due to YB deformations as, Implementing the definition [13], one could further express (4.37) as, Notice that the above equation (4.40) clearly resemblance our previous finding in (4.27). It is also worthwhile to mention that in the limit of the vanishing YB deformations, the quadratic action (4.40) precisely reproduces the previous findings of [13]. It is indeed interesting to notice that, as observed in the previous section, the YB deformations shifts the pole (4.38) by an amount that goes with the quadratic order (∼ 1/J 2 ) in the inverse of the SYK coupling.

Concluding remarks
In this paper, based on the notion of SYK/AdS correspondence, we explore the effects of Yang-Baxter (YB) deformations on the collective field excitations within the SYK model. The motivation behind our analysis solely comes from the underlying holographic principle which strongly suggests a possible modification of the SYK spectrum at quadratic (1/J 2 ) order in the SYK coupling. Based on the notion of holography (namely, looking at the scalar fluctuations and their YB scaling in (AdS 2 ) η ) we propose a possible YB scaling of the bi-local fields in the SYK model and compute the effective action upto quadratic order in the fluctuations. It would be really nice to understand this YB scaling in terms of 1/N diagrammatics and thereby the associated Feynman rules in terms of these newly defined collective excitations. We hope to address some of these issues in the near future.
A Evaluation of the Green's function G The zero-th order Green's function G (0) w,w is defined through the following equation, Expressing the Green's function in a basis of orthonormal wave functions, and substituting back into (A.1) we find, where we have introduced,L and used the orthonormality conditions for the wave functions, it is in fact quite straightforward to show, which finally yields the real space zeroth order Green's function, (A. 13) B Evaluation of the quadratic action S (2) We divide the quadratic action (4.21) into following two parts,