{'fraction_non_alphanumeric': 0.028541082273482392, 'fraction_numerical': 0.012908848280181922, 'mean_word_length': 4.505247376311844, 'pattern_counts': {'":': 0, '<': 7, '<?xml version=': 0, '>': 4, 'https://': 0, 'lorem ipsum': 0, 'www.': 0, 'xml': 0}, 'pii_count': 0, 'substrings_counts': 0, 'word_list_counts': {'cursed_substrings.json': 2, 'profanity_word_list.json': 0, 'sexual_word_list.json': 0, 'zh_pornsignals.json': 0}}
Giant Gravitons in the Schrodinger holography

We construct and study new giant graviton configurations in the framework of the non-supersymmetric Schrodinger holography. We confirm in the original Schrodinger spacetime, the picture discovered previously in the pp-wave limit of the geometry, namely that it is the giant graviton that becomes the energetically favored stable configuration compared to the point graviton one. Furthermore, there is a critical value of the deformation above which the point graviton disappears from the spectrum. The former fact leads also to the possibility of tunnelling from the point graviton to the giant graviton configuration. We calculate, explicitly, the instanton solution and its corresponding action which gives a measure of the tunnelling probability. Finally, we evaluate holographically the three-point correlation function of two giant gravitons and one dilaton mode as a function of the Schrodinger invariant.


Introduction
An important and efficient tool in exploring a gravity background (especially one that comes as a continuous deformation of the N = 4 SYM) is the inclusion of brane probes and the subsequent study of their dynamics. A prominent example in this class of configurations is a D3-brane that wraps a three-sphere inside the five-sphere of the celebrated AdS 5 × S 5 geometry and it known as the giant graviton [1]. It has the same quantum numbers as the point particle and a nonzero angular momentum along the equator of the internal space. Stability against shrinking is guaranteed by the RR repulsion but also the perturbative stability analysis around the giant graviton solution has been performed in [2]. When the three-sphere that the giant wraps is inside the AdS part of the space the configuration to be realized is the dual giant graviton, with similar properties [3,4].
While in the original AdS 5 ×S 5 geometry (and depending on the value of the conjugate angular momentum) the point graviton is either energetically favored or at most degenerate with respect to the giant graviton, the situation becomes intricate and interesting when the geometry gets deformed. When the deformation is purely on a sphere, as in the marginally deformed backgrounds, there is a variety of behaviors but in none of them the energetically favored solution is the giant graviton. More specifically, there are cases that the degeneracy that is inherited by the parent undeformed background is intact [5,6], cases that the degeneracy is lifted in favor of the point graviton [7,8] and cases where the initially energetically favored point graviton becomes even more pronounced [7]. However, when the deformation involves directions of the anti de Sitter space, as it happens in the cases of the non-commutative or the dipole deformation, there are situations where the energetically favored solution is the giant graviton (see [9] for the non-commutative example and [10] for the pp-wave geometry of certain dipole deformed theories).
There are several interesting examples of gauge/gravity dualities in which the original AdS/CFT scenario [11] is deformed. One such example is the duality between a certain spacetime with Schrödinger symmetry and its dual dipole-deformed non-relativistic conformal field theory [12]. Compared to the original AdS/CFT duality very few observables have been calculated in the Schrödinger/dipole CFT version of the correspondence. In particular, in [13] and [14] two and three, as well as n-point correlation functions of scalar operators were calculated by employing the gravity side of the correspondence. It is important to mention that all the operators involved in these correlators correspond to point-like strings propagating in the Sch 5 × S 5 background. In [15] extended dyonic giant magnon and spike solutions were constructed and their dispersion relations were derived. 1 A complementary study with finite size corrections of those classical solutions was presented in [17]. 2 The existence of the aforementioned solutions is in complete agreement with the fact that the theories involved in the Schrödinger/dipole CFT duality remain integrable despite the presence of the deformation. In the same work [15] an exact, in the 't Hooft coupling λ, expression for the dimensions of certain gauge invariant operators dual to the giant magnons was conjectured. Subsequently, this conjecture was further improved in [20] in such a way that it is in perfect agreement with the string spectrum in the ppwave limit of the Schrödinger spacetime. Furthermore, agreement between this expression and the one-loop anomalous dimension of BMN-like operators was found in the large J limit providing, thus, further evidence in favor of the correspondence. On the field theory side, the one-loop spectrum of operators belonging in a SL(2) closed sub-sector of the null dipole-deformed CFT has been studied in [21]. The authors found agreement between the one-loop anomalous dimensions of certain long operators and the energies of the dual string solutions (see [22], as well).
Subsequently, by utilising the Schrödinger background, the three-point functions involving two heavy and one light operator were calculated holographically in [23]. The heavy states were generalizations either of the giant magnon or spike solutions constructed in [15] while the light operator was chosen to be one of the dilaton modes. These results for the three-point functions are the first in the literature in which the heavy states participating in three-point correlation functions are described by extended string solutions. The aforementioned results are in complete agreement with the form of the correlator dictated by non-relativistic conformal invariance and provide us with the leading term of the correlators in the large λ expansion. Finally, pulsating strings solutions in the Schrödinger background were recently derived in [24,25] while the holographic Fisher information metric in Schrödinger spacetime was studied in [26].
Very recently, giant graviton solutions in the pp-wave limit of the Schrödinger geometry were constructed in [10]. These solutions have the remarkable property that the deformation breaks the degeneracy between the point and giant graviton solutions in favour of the giant graviton which becomes the energetically favoured stable solution. The focus of the current paper is twofold. On one hand, it is to identify the classical configurations describing giant gravitons in the Schrödinger background before taking the pp-wave limit and on 1 Giant magnon solutions in other deformed geometries like the β-deformed theories have been found in [16].
2 Giant magnon-like solutions with a different dispersion relation were found in [18], while giant magnons and spiky strings on Sch5 × T 1,1 and the corresponding dispersion relations were found in [19].
the other to use these solutions in order to probe the holography in Schrödinger spacetimes. This second goal will be accomplished through the calculation of the three-point correlation functions of the dilaton modes and two "heavy" operators. The giant gravitons will serve as the gravity duals of the heavy states and the result of the holographic computation will provide us with the leading term in the large λ expansion of the the three-point correlators. The plan of the paper is as follows: In section 2, we revisit the type IIB supergravity solution of the Schrödinger background and present a consistent giant graviton ansatz. The Hamiltonian of the system is a function of two variables: the deformation parameter and the conjugate momentum with respect to one of the internal angles of the five-sphere. We investigate the behavior of the system either fixing the conjugate momentum and varying the deformation parameter or vice versa and extract a plethora of interesting observations. The importance of the ansatz we introduce is that the zero deformation limit of our Hamiltonian leads smoothly to the Hamiltonian of the undeformed AdS 5 × S 5 that appears in [1,3]. In section 3 we focus the attention to potential tunnelling effects between the two graviton solutions and calculate instanton transitions, in that part of the parametric space where the giant graviton is the energetically favored solution. Emphasis is put on a novel instanton solution that arrises when the deformation parameter and the conjugate momentum are related through a constraint in such a way that, despite the presence of a deformation, the energies of the two gravitons, the point and the giant graviton, are equal. In section 4, we compute holographically the three-point correlation function of the dilaton modes and two "heavy" operators whose gravity duals are the giant gravitons, in the special case where the giant and the point graviton are degenerate. The result is in complete agreement with the constraints put by conformal invariance. In section 5 we conclude the paper and identify potential future directions for endeavors in the framework of Schrödinger holography.

Giant Gravitons in a Schrödinger geometry
The starting point for the analysis we will present in this paper is the expressions for the supergravity solution of the 10d Sch 5 × S 5 geometry in global coordinates [21,27] where we have written the metric of the five-sphere as an S 1 -fibration over the CP 2 and the quantities Σ 1 , Σ 2 and Σ 3 are defined as follows The metric is accompanied with a magnetic field and a RR five-form In order to describe Giant Graviton solutions in the Schrödinger background (2.1), we have to consider the action of a probe D3-brane. This action consists of the sum of the Dirac-Born-Infeld (DBI) term and of the Wess-Zumino (WZ) term where P denotes the pullback of the different spacetime fields on the brane worldvolume and T 3 is the tension of the D3-brane. We consider a D3-brane probe that extends along the following directions and the ansatz for the rest of the coordinates is as follows Notice that ρ 0 is the size of the graviton in the internal space. Substituting the ansatz (2.7) in (2.5) and integrating the spatial coordinates of the world volume, we obtain the following expressions for the on-shell action and the Lagrangian where, to simplify notation, we have introduced the following definitions of constants The conjugate momenta to χ and V are given by An important comment is in order. In contradistinction to the giant graviton ansatz in the pp-wave Schrödinger geometry [10], in the current case there are three conserved quantities (namely E, J 1 and J 2 ) instead of two (E and J 1 in the pp-wave case). The need for a generalization of the previous giant graviton ansatz is coming for the following reason. It is known that the ansatz (2.7) satisfies the equations of motion only at the extrema of the on-shell action (see also the discussion in [10]). Following this reasoning, we calculated the equations of motion for the coordinates that are orthogonal to the brane worldvolume directions (namely T, V, X, Z, ρ and χ) and indeed we realized that the equations of motion for Z and ρ are not automatically satisfied. The equation of motion for ρ is satisfied when we impose that the derivative of the Lagrangian with respect to ρ vanishes. However, the equation of motion for Z is not satisfied unless we fix the value of J 2 . Turning on an extra coordinate dependence in the giant graviton ansatz (that for V ) is necessary and gives us the extra freedom that is needed in order for all the equations of motion to be satisfied at the extrema of the Lagrangian. For this to happen the conjugate momentum J 2 should acquire the following value (2.11) The corresponding Hamiltonian H = J 1 ω + J 2 Γ − L D3 for the giant graviton solution in the Schrödinger background becomes (2.12) Taking the limit of zero deformation (i.e. ∆ → 0) the denominator becomes the unit and we recover the Hamiltonian of the N = 4 giant graviton on the sphere [1,3,4]. The quantity inside the square root in the denominator of (2.12) should be always positive, and this sets an upper bound for the value of ∆. The range of values for the deformation parameter is In figure 1 we plot the Hamiltonian (2.12) as a function of the graviton's size ρ 0 , for different values of the deformation ∆ and of the conjugate momentum J 1 . 3 In all expressions and figures below we have chosen units such that the radius of the 5-sphere is L = 1 and we have also set N = 1, that is whereever one sees J 1 it is J 1 /N that should appear. On the left plot, we fix J 1 to a value that is less than one (more specifically J 1 = 0.9) and increase the value of the deformation parameter ∆. For ∆ = 0 we recover the N = 4 result, where the energy of the point and of the giant graviton are the same. Turning on the deformation parameter the initial degeneracy between the three extrema disappears and remarkably, the energetically favored solution (the one having less energy) is the giant graviton. This behavior is in qualitative agreement with the giant graviton calculation in the pp-wave Schrödinger background [10]. Keep increasing the value of ∆, we will continue having three extrema, but the extremum at the position ρ 0 = 0 will change from a minimum to a maximum at the value ∆ = 1/ √ 2. At exactly this value for ∆ the second derivative of the Hamiltonian (2.12) with respect to ρ 0 at ρ 0 = 0 will change sign from positive to negative and if one keeps increasing the deformation parameter there is a value of ∆ = 1 above which the point graviton will cease to exist. Notice that the behavior of the Hamiltonian as a function of the graviton's size ρ 0 will remain qualitatively unaltered if we change the value of J 1 , as long as we stay in the range of J 1 < 1.
On the right plot of figure 1, we fix J 1 to a value that is above one (more specifically J 1 = 1.1) and increase the value of the deformation parameter ∆. For ∆ = 0 we have three extrema and the extremum at ρ 0 = 0 is the energetically favored solution, which is the N = 4 result. Increasing the value of ∆, increases the value of the energy at the ρ 0 = 0 extremum and decreases the values of the other two extrema. As a result of this, there is a critical value of the deformation parameter ∆ for which the three extrema have the same energy. This value depends on the value of J 1 and in figure 6 we depict the relation between the critical ∆ and J 1 . In the next section we will analyze in detail this special class of solutions. In this region of ∆ < ∆ crit the point graviton solution is energetically favored with respect to the giant graviton solution. The behavior of the Hamiltonian for values of the deformation parameter ∆ above the critical value is identical to the behavior we already described for J 1 < 1. More specifically, the giant graviton becomes the energetically favored solution and for values above ∆ = 1/ √ 2 the extremum at the point graviton position turns from a minimum to a maximum and for ∆ > 1 the point graviton is not any more part of the spectrum (see also the discussion in [10]). . . Instead of fixing the conjugate momentum J 1 and varying the deformation parameter ∆, we could have done the inverse. Such an analysis shows that keeping the value of the deformation parameter fixed and below ∆ = 1/ √ 2, that is in the region where the point graviton is still a minimum, and increasing the value of the conjugate momentum beyond J 1 = 1, there is a critical value of J 1 above which the giant graviton solution completely disappears. 4 At this value of J 1 both the first and the second derivative of the Hamiltonian with respect to ρ 0 at the giant graviton position vanish. In figure 2 we have plotted this critical value of J 1 as a function of the deformation parameter ∆. In the undeformed N = 4 case, the critical value of the conjugate momentum is J 1 = 1.125 [3]. Notice that if the value of the deformation parameter is above ∆ = 1/ √ 2 then the extrema corresponding to the giant graviton solution never disappear. This is related to the fact that for values of the deformation parameter above ∆ = 1/ √ 2 the extremum at the point graviton position turns from a minimum to a maximum.

Instanton Transitions
The analysis of the previous section has uncovered two brane configurations that in the framework of a Schrödinger background describe a graviton state with angular momentum J 1 : from one side it is the point-like graviton and from the other side the giant graviton, a configuration that consists of a spherical D3-brane extending into the five-sphere. Interestingly, even though the five-sphere is not deformed in the Schrödinger deformation of the parent AdS 5 × S 5 background we consider, due to the presence of the magnetic field, the Hamiltonian of the giant graviton depends on the deformation parameter in a non-trivial way. The interplay between the conjugate momentum J 1 and the deformation parameter ∆ creates a rich space of parameters that we analytically examined in the previous section.
Quantum mechanically we expect the two graviton states to mix and motivated from this expectation we are looking for instanton solutions that tunnel from one graviton state to the other. In the current section we will derive explicit expressions for the instanton solutions that evolve between the expanded three-brane state and the zero-size state. In particular, we will be mostly interested in the tunnelling from the point graviton to the giant graviton configuration since, as was discussed in the previous section, the effect of the deformation µ or equivalently ∆ is to make the giant graviton the energetically favorable state.
To begin the analysis we extend the ansatz that we introduced in (2.7) to allow for a time-dependent ρ 0 coordinate, that is to allow for a time-dependent size of the graviton. The Lagrangian is now extended to the following expression where we have analytically continued to euclidean time τ → iτ . This results in an inversion with respect to the ρ 0 -axis of the potential energy of figure 1.
As a next step we perform a Legendre transformation to eliminate ω and Γ in favor of the conserved angular momenta J 1 and J 2 and produce the Routhian Instead of working with the second order equations of motion coming from the Euclidean action (3.1) (or the Routhian (3.2)), we determine the instanton solution by the evaluation of the corresponding conserved energy Following the same reasoning we have already discussed in detail in section 2, we calculate from the full DBI plus WZW Lagrangian the equations of motion for the coordinates that are orthogonal to the brane worldvolume directions. Using the expression for the derivative of ρ 0 with respect to τ (i.e.ρ 0 ) that is obtained from (3.3), all the equations of motion are satisfied except from the equation of motion for Z. That equation provides a constraint between the conjugate momentum J 2 and the conserved energy p, namely In the last equation V (ρ 0 ) is the same function defined in (2.11). One should, however, keep in mind that in (3.4) ρ 0 is a function of the world-volume time τ while in (2.11) ρ 0 is a constant. Substituting (3.4) in (3.2) we obtain the expression for the Routhian while substituting (3.4

) in (3.3) we obtain the expression for the Hamiltonian
Notice that setting to zero the value of the deformation parameter ∆ the expressions (3.5) and (3.6), for the Routhian and the Hamiltonian respectively, flow to the undeformed counterparts in [3].
For the remainder of the current section we will focus on cases where the giant graviton is the energetically favored solution and we will construct instantons that describe tunnelling from the point to the giant graviton configuration. In terms of the discussion we detailed in the previous section around figure 1, there are two cases of interest: • J 1 < 1 and 0 < ∆ < 1/ √ 2 (left plot of figure 1). We remind the reader that for ∆ > 1/ √ 2 the point graviton is not any more part of the spectrum.
To proceed the analysis we set L = N = 1 and since the point graviton at ρ 0 = 0 will be the instanton starting and ending point, the conserved energy obtains the following value (3.7) Solving the differential equation that arises from (3.6) with the boundary condition (3.7), we arrive at the following instanton solution where the auxiliary quantity W is defined as follows The constant τ 0 that appears in (3.8) is an integration constant that gives the position of the instanton in euclidean time, it is in fact the zero mode that determines the instanton position. In the rest of the analysis and for all the plots we fix this constant to zero. i.e. τ 0 = 0. In figure 3 we plot the instanton solution for two values of the conjugate momentum J 1 , one less than one and one larger than one, and three different values of the deformation parameter ∆. The next step is the calculation of the euclidean action. Since the Routhian R E (3.5) evaluated around the point graviton position remains finite the evaluation of the integral dτ R E diverges. To regularize the integral we subtract the Routhian at the point graviton extremum and the relevant quantity to calculate is the following S = where τ turn is the time that corresponds to the maximum of the curve that is depicted in figure 3. Notice that the upper limit of integration is the turning point τ turn since if the graviton manages to tunnel up to this point then it will immediately roll to the global minimum of the potential which is the giant graviton state. In figures 4 and 5 we have plotted the total action (only numerical evaluation of the integral in (3.10) is possible) as a function of the conjugate momentum J 1 and the deformation parameter ∆. Calculation of the total action provides a measure for the degree of tunnelling. More precisely, the transition probability from the point graviton to the stable giant graviton is proportional to the exponential of minus the action of (3.10). Two comments are in order. Firstly, notice that the transition probability is exponentially small since if we reinstate the number of colours N , which has been set to unity in the numerical calculation above, one gets P ∼ e −N s , where s > 0. Secondly, note that figure 4 implies that as the deformation parameter increases the transition probability increases since S becomes smaller. This is fully consistent with the shape of the potential depicted in figure 1. It is evident from that figure that as the deformation parameter increases the height of the barrier which the brane has to tunnel through becomes smaller making the tunnelling more probable.

Special Instanton solution
In this subsection, we will examine a special class of instanton solutions among those that are described by the analytic expression that is presented in (3.8). Setting to zero the value of the auxiliary parameter W that is defined in (3.9) introduces a constraint between the conjugate momentum J 1 and the deformation parameter ∆. Solving the constraint with respect to ∆ means that by choosing the value of J 1 we automatically fix the value of the deformation parameter ∆ as follows In figure 6 we plot this relation between ∆ and J 1 . Implementing the constraint (3.11) on the general instanton solution of (3.8) and calculating the limits at τ → − ∞ and τ → + ∞ we obtain the following results (3.12) The last two relations fully determines the range of values for both J 1 and ∆. More specifically, we have that ∆ ∈ [0, 1/ √ 2) and J 1 ∈ [1, 2). On the left plot of figure 7 the special instanton solution for W = 0 is presented. It corresponds to an instanton transition from the zero-size point graviton solution at τ → − ∞ to the expanded giant graviton solution at τ → + ∞. Notice that another instanton solution, symmetric with respect to the vertical axis at τ = 0, exists that would correspond to a transition from the expanded giant graviton solution at τ → − ∞ to the zero size point graviton solution at τ → + ∞. From the moment that eventually, when increasing the deformation parameter, the energetically favored solution is the giant graviton, we are not interested in transitions from the giant to the point graviton solution.
On the right plot of figure 7 we plot the Hamiltonian of the special instanton solution. In that way a remarkable feature of the special solution is uncovered. When the constraint (3.11) is satisfied, the energies of the point graviton and of the giant graviton are equal. This situation is analogous to the instanton calculation in the undeformed case of N = 4 [3], where the energies of the point and the giant graviton were also equal. Here, tuning the relation between ∆ and J 1 , we are able to identify similar situations where the two solutions have the same energy. The important difference is that increasing the deformation parameter will eventually lead to an energetically favored giant graviton.
The next important step is to calculate the total action of the special solution. Regularizing the Routhian as before in (3.10) but now integrating from −∞ to +∞ we are able to obtain an analytic result for the total action In figure 8 we plot the total action as a function of the angular momentum J 1 , from where it is evident that it monotonically decreases. Thus, as J 1 ( or J 1 /N , if we reinstate the number of colours) increases, the action decreases and the probability of tunnelling is increasing. This qualitative picture is also supported by the plot of the Hamiltonian (see the right plot of figure 7), where one can see that when J 1 increases, the difference between the extremum (minimum) of the point graviton and the nearby extremum (maximum), gets smaller. The potential becomes more shallow and as a result the probability of tunnelling becomes larger.

Three-point function of two giant gravitons and a dilaton mode
In this section, we will focus on the holographic calculation of the three-point correlation function involving two operators dual to the giant graviton and one operator dual to one of the dilaton modes. 5 The result will provide the strong coupling prediction for the aforementioned three-point correlator. Similar holographic calculations involving giant magnons or spiky strings of the Schrodinger background have been performed recently in [23]. In addition, the holographic computation of heavy-heavy-light correlation functions with the heavy operators being the giant gravitons and the light operators being BPS states of the undeformed AdS 5 × S 5 background have been presented in [34].
In order to proceed with the holographic calculation we need a giant graviton solution that tunnels from one point of the boundary (this is one of the points where the dual field theory operator is situated) to another. To this end we construct a slight generalization of the giant graviton solution presented in section 2. This reads where the constants appearing in (4.1) are given by Notice that we have turned on two additional coordinates of the Schrodinger part of the spacetime, namely X. As can be seen from (4.1) this induces a modification of the V coordinate, too. 6 The next step is to use the following coordinate transformation in order to pass from the global to the Poincare coordinates [35] x + = tan T , and subsequently to perform an analytic continuation to the world-sheet time τ → i τ after which the solution takes the form This is the appropriate giant graviton solution travelling from one point of the boundary at τ = −∞ to another point at τ = +∞. In what follows, we will also need the on-shell value of the D3 brane Lagrangian which can be evaluated from (2.5). It reads One may now define the the following kinematic Schrodinger invariant v 12 = − 1 2 where t ij = t i − t j and similarly x ij = ( x i − x j ). In (4.6), ( x 1 , t 1 ) and ( x 2 , t 2 ) denote the positions of the heavy operator on the boundary while ( x 3 , t 3 ) the position of the dilaton mode. In what follows and in order to keep the expressions for the three-point correlator as simple as possible we take the time ordering of the operators to be as follows As a result the invariant cross ratio simplifies to v 12 = − 1 2 x 2 12 t 12 = 1 2 X 2 T . One may use this last relation to rewrite, by taking into account that the expression for Z 0 becomes the analytically continued giant graviton solution (4.4) in terms of the invariant v 12 , X and T = t 2 − t 1 . It reads The last piece of information needed is the bulk-to-boundary propagator of the light field, that is of the dilaton mode. In the limit (4.7) it takes the form [23] K(z, x, t; where M 3 denotes the mass eigenvalue of the dilaton mode participating in the three-point correlator. Now, we have all the ingredients in order to calculate the three-point correlator. As discussed, in some detail, in a similar calculation [23] the ratio of the three-point to the two-point correlation functions is given by Notice that the result for the three-point function takes the form of a vertex operator that corresponds to the light state integrated over the classical world-volume of the D3-brane which represents the giant graviton at the strong coupling regime. 7 Plugging (4.5) and (4.10) and using the expressions for the solution (4.9) in (4.11) one may perform the integration over the three-sphere along which the D3-brane extends to obtain (4.12) The remaining τ integral can be approximated by The approximation is done in the exponential e i M 3 x − (τ,σ) of (4.11) and consists of replacing the tanh (τ /L) ≈ τ /L appearing in x − . This is a legitimate approximation since the bulkto-boundary propagator in (4.11) has a peak around τ = 0 and falls off exponentially away from this value. As a result the integral can be evaluated to give (4.14) As discussed in [23] (see eq. (3.9)) the ratio of the three to the two-point correlator takes in the limit (4.7) the following form whereF (v 12 ) is an undetermined function of the Schrödinger invariant v 12 that can not be determined by conformal invariance. It reads Our calculation provides the strong coupling prediction for the three-point correlation function and is fully consistent with the three-dimensional conformal symmetry of the Schrödinger group of the theory.

Conclusions
The center of attention of the current paper is the construction and further study of a giant graviton configuration in the framework of the Schrödinger holography. On the gravity side the giant gravitons are described by a D3-branes that extend along the time direction of the Sch 5 part of the geometry and wrap a three-sphere inside the internal space of the undeformed five-sphere. The main result of this paper is to confirm, in the original Schrödinger spacetime, the picture discovered previously in [10] for the case of the pp-wave limit of the Schrödinger geometry , namely that the giant graviton configuration becomes the energetically favored stable configuration compared to the point graviton one. This fact is remarkable by itself since in most of the literature the tendency is exactly the opposite, the point graviton is the ground state of the D3-brane. The aforementioned fact leads also to the possibility of tunnelling from the point to the giant graviton configuration. We calculate, explicitly, the instanton solution and its corresponding action which gives a measure of the tunnelling probability. Finally, we evaluate holographically the 3-point correlation function of two giant gravitons and one dilaton mode.
The giant graviton solution depends on the deformation parameter of the spacetime ∆ and on the angular momentum J 1 along the sphere equator. We vary the value of the deformation parameter keeping the angular momentum fixed, either below or above the constant value J 1 = 1. In the former case and for non-zero values of the deformation parameter the degeneracy between the point and the giant graviton, that was present in the undeformed N = 4 case [3], is lifted in favor of the giant graviton. Moreover, there is a maximum value of the deformation parameter (e.g. ∆ = 1/ √ 2) above which the point graviton solution ceases to be at a minimum of the potential and evetually disappears from the spectrum. Notice that both aforementioned features were present also in the analysis of the giant graviton solution in the pp-wave limit of the Schrödinger background [10]. Fixing the conjugate momentum above the constant value J 1 = 1 discloses the presence of a critical deformation parameter, where the energies of the point and the giant graviton solutions are equal. This in turn creates a whole class of solutions (for every value of J 1 between 1 and 2 there is a critical value of ∆ between 0 and 1/ √ 2) and the precise relation between ∆ crit and J 1 is given in equation (3.11). Below this critical value ∆ < ∆ crit the point graviton has less energy than the giant graviton while above, that is when ∆ > ∆ crit it is the giant graviton that is energetically favored. Notice that until now in the literature (see e.g. [8]) the mere presence of a deformation parameter in the geometry lifts a degeneracy between the point and the giant graviton solution. The fact that with a Schrödinger deformation such a degeneracy returns for a finite deformation is an interesting new feature and is related to the drastic changes of the dipole-deformation on the geometry, as well as on the field theory side.
Besides identifying the two graviton solutions (and motivated by the quantum mechanical expectation of state mixing) we focus on cases where the giant graviton is energetically favored with respect to the point graviton and construct the instanton solutions tunnelling from the giant to the point graviton. Plotting the total action as a function of the deformation parameter (see e.g. figure 4) we identify a monotonically decreasing behavior as the deformation parameter increases. This, in turn, means that the transition probability increases, something that is totally expected if one carefully examines the shape of the potential in figure 1. Indeed, as the deformation parameter increases the potential around the point graviton solution gets flattened and as result the probability of tunnelling from the point to the giant graviton increases. We give special attention to the case of the critical deformation parameter. In this case the two configurations have the same energy and the form of the potential resembles that of the N = 4 case of [3], but in the presence of a deformation. The calculation of the total action is analytic and reveals an increased tunnelling probability as the deformation parameter increases (or equivalently, due the the relation that appears in equation (3.11), as the conjugate momentum increases).
Finally we focus our attention of the holographic calculation of the three-point correlation functions of the dilaton modes and two "heavy" operators, following the analysis that is detailed in [23]. In the case at hand, the "heavy" operator is the giant graviton solution and in particular the class of solutions where the deformation parameter acquires the critical value of equation (3.11). Moreover and in order for the classical solution to have the interpretation of a brane tunnelling between two boundary points (where the field theory operators will be located), the giant graviton solution in slightly generalized. The result of the computation is twofold: From one side we confirm the form of the correlator that is dictated by conformal invariance and from the other we specify the scaling function at strong coupling. This is a quantity that is not possible to fix using conformal symmetry.
There is a number of interesting directions which have not be explored in the context of Schrödinger holography. One of these is related to instanton calculations in the Schrödinger/null-dipole CFT duality. The analogous calculations for the marginal deformation of N = 4 called β-deformations and for the three parameter deformation of N = 4 [36] have been performed in [37] and [38], respectively. A second direction would be to focus on the field theory side of the duality and study the gauge invariant operators dual to the giant graviton configurations presented in this work. These should be obtained from the undeformed ones by introducing the appropriate star product among the N = 4 fields which will generate the dipole shift along one of the light-cone directions. Finally. it would be interesting to investigate which are the general features that a background should have so that the giant graviton solution is energetically favored compared to the point graviton. Our analysis points towards the direction that deforming the AdS part of the geometry is essential regarding this aspect.