Stability analysis of 5D gravitational solutions with bulk scalar fields
We study the stability of 5D gravitational solutions containing an arbitrary number of scalar fields. A closed set of equations is derived which governs the background and perturbations of scalar fields and the metric, for arbitrary bulk and boundary scalar potentials. In particular the effect of the energy-momentum tensor of the scalar fields on the geometry is fully taken into account, together with all the perturbations of the system. The equations are explicitly written as an eigenvalue problem, which can be readily solved to determine the stability of the system and obtain the properties of the fluctuations, such as masses and couplings. As an example, we study a dynamical soft-wall model with two bulk scalar fields used to model the hadron spectrum of QCD and the Higgs sector of electroweak physics. It is shown that there are no tachyonic modes, and that there is a (radion) mode whose mass is suppressed by a large logarithm compared to that of the other Kaluza-Klein modes.
Brane-world models have proved to be very useful for model building, providing a way to not only address the hierarchy problem in the Standard Model ArkaniHamed:1998rs (); Antoniadis:1998ig (); Randall:1999ee (), but also to explain the hierarchy of fermion masses and mixings ArkaniHamed:1999dc (); Grossman:1999ra (); Gherghetta:2000qt (); Huber:2000ie (). A variety of constructions are usually employed with fields, other than gravity, in the bulk and/or on the branes. Furthermore, aided by the AdS/CFT correspondence, a dual description of strongly coupled four-dimensional (4D) gauge theories can be obtained Maldacena:1997re (); ArkaniHamed:2000ds (); Rattazzi:2000hs (). These fields are normally treated as test fields, where the corresponding energy density is sufficiently small not to disturb the background geometry. Therefore, for a given geometry one performs a Kaluza-Klein (KK) decomposition. Solving the field equations in this geometry gives the bulk profile and the eigenmasses of the KK modes. The profile, in turn, determines the couplings of the KK modes.
Eventually, a complete model has to provide the dynamical elements that determine the bulk geometry, and the brane positions (when present). As an example, the Randall-Sundrum model Randall:1999ee (), does not solve the hierarchy problem until the exact location of the TeV brane is fully specified. Most of stabilization mechanisms, starting from Goldberger:1999uk (), typically employ one scalar field, due to its simplicity.
The system of perturbations in the presence of a bulk scalar was studied, for example, in Ref. Csaki:2000zn () (see also Lesgourgues:2003mi ()). This analysis considered the properties of various excitations coupled to SM fields, which were assumed to be localized on the brane. Of particular relevance was the study of the radion, which is the lightest of these scalar perturbations. The analysis of Csaki:2000zn () was limited to a regime of small backreaction of the bulk scalars on the bulk geometry. Later, Kofman:2004tk () generalized this study to a bulk field with arbitrary bulk/brane potential.
However, there are systems in which more than one dynamical scalar field is relevant. For instance, in the soft-wall model of Batell:2008zm (), two bulk scalar fields are used to obtain a solution of the Einstein equations. Furthermore in string theory, multiple scalar fields (such as the dilaton and moduli fields) are quite common. This motivates generalizing the study of Kofman:2004tk () to the case of bulk (real) scalar fields, which will be presented in this paper. The generalization to bulk scalar fields has also been previously considered in Refs. Toharia:2010ex (); Aybat:2010sn (); George:2011tn (). In our analysis we make no assumption on the form of the bulk and boundary potentials.
The perturbations are obtained by studying the linearized problem. It is useful to distinguish them as scalar/vector/tensor modes under Lorentz transformations of the ordinary 4D spacetime: we assume that the noncompact space has a Minkowski metric. As a consequence the scalar/vector/tensor modes are decoupled from each other at the linearized level and therefore can be studied separately. The mode count proceeds as follows. There are 15 perturbations in the five-dimensional (5D) metric, and perturbations from the bulk (real) scalar fields. Of these, are nondynamical and 5 more can be removed by a gauge choice
It is technically challenging to identify the scalar degrees of freedom because they can arise either from the components of the metric perturbations or the actual bulk scalar field perturbations. The number can be reduced to by using constraint equations to derive a manageable set of closed equations for the modes. This must be done for both the bulk and brane equations. The latter equations are boundary conditions and we will consider both cases either with or without branes at the boundaries (in the second case, the boundary condition is typically given by the requirement of normalizability). We derive this system of equations, which for convenience is written as an eigenvalue problem, with the appropriate number of equations needed to obtain a solution. Our goal is to provide an explicit formulation of the eigenvalue problem that can be used to study any 5D model with an arbitrary number of bulk scalar fields. By solving the eigenvalue problem the physical properties of the perturbations (masses and couplings) can be obtained. This can then be used to check the stability of the model, so that if for some scalar modes, the background solution is unstable.
While the eigenvalue problem may be solved analytically for the simplest cases, in general a numerical method is needed to obtain a solution. We will employ the shooting method since the boundary equations at one boundary leave freedom for the choice of the mode functions, and of the mass eigenvalue. We show that, for scalars, the boundary conditions at one of the two boundaries leave unspecified quantities. The bulk equations are then used to evolve the solution to the other boundary, where there are precisely constraints that must be satisfied (given by the boundary condition at this boundary). If these constraints are satisfied, then a physical mode has been found.
As an example of the numerical method, we study the perturbation properties, and the stability problem, for the dynamical soft wall model of Ref. Batell:2008zm (). The model is characterized by two scalar fields with a coupled potential term. It is interesting because it leads to a KK mass spectrum with linear Regge-like trajectories, similar to the hadron spectrum in QCD. We conduct a dense scan in parameter space and find approximately 100 modes with positive , and no mode with negative . Moreover, we find an interesting behavior of the radion mass. The mass is suppressed by a large logarithm, that in the dual CFT interpretation corresponds to how scale invariance is broken by quantum corrections. This is the same suppression present in the Goldberger-Wise mechanism Goldberger:1999uk (); Csaki:2000zn ().
The paper is organized as follows. In Section II we introduce the class of models that we are studying; we present the Lagrangian, the background solutions, and the most general set of perturbations. In the following three Sections we study the scalar, vector, and tensor perturbations, respectively. We identify the physical modes, and perform their Kaluza-Klein decomposition. We provide the explicit closed set of equations which can be solved to obtain the mass and the bulk profile of these modes through a boundary value problem. In Section VI we formalize this boundary value problem for the two sectors (scalar and tensor) that contain physical perturbations. In Section VII we study the perturbations of the model in Ref. Batell:2008zm () as an example of how to use our formalism to solve the eigenvalue problem. In Section VIII we briefly summarize our main findings. Some more technical steps are then given in the three Appendices.
Ii 5D Models
The goal of this work is to provide the tools for studying the perturbations, and the stability, of a wide class of models with one extra dimension and bulk scalar fields . Specifically, we consider models characterized by the action
where is the 5D fundamental scale. The first line in (1) contains the bulk terms, which are restricted to lie between two boundary branes, if they are both present, or else either between a boundary brane and infinity, or between . The overall factor of is adopted from Kofman:2004tk (), where the bulk was assumed to be symmetric across each brane, and the symmetry was accounted for by restricting the bulk integral only to one side of each brane. This notation will also be used here, even in the cases where one or both branes are absent; it is trivial to reabsorb this factor away by a rescaling of , , and . We assume that the scalars have a standard kinetic term in the bulk. Notice that the choice of sign for the kinetic term corresponds to . If present, a bulk cosmological constant is included as a constant term in . The second line in (1) is instead the brane action; denotes the induced metric on the brane, and the notation with subscript denotes the jump of the quantity inside the square parenthesis across the brane, which in this case is the extrinsic curvature . denotes the potential of the scalars on the brane (which is a function of the value that the fields have at the brane location), and, if present, a brane tension is included as a constant term in (note that when both boundary terms are present, we do not require them to be equal). In addition we disregard the possibility of brane kinetic terms for the scalar fields.
From the action (1) we obtain the Einstein equations in the bulk
where capital Latin indices run over all the coordinates and the energy momentum tensor is given by
We also obtain the bulk equations for the scalars
When a boundary brane is present, extremizing the action (1) leads to the boundary conditions for the scalar fields
as well as the so-called Israel conditions
where , and denotes the stress energy tensor on the brane
Note that Greek indices run over the usual dimensions only. The explicit definition and computation of the induced metric and the extrinsic curvature are given in Appendix A.
At the background level, we assume a factorizable geometry with 4D Minkowski slices:
It follows that the background bulk scalars can have a nontrivial dependence on the extra coordinate only:
The only nontrivial equations in (2) then arise from the diagonal , and components. We write here one linear combination of these two equations, and the component:
where prime denotes differentiation with respect to . The scalar equations (4) give instead
where . It is easy to check that the first equation of (10) can be derived by combining (11) and the second equation of (10) (this redundancy is a consequence of a nontrivial component of the Bianchi identity).
From the background expressions of the induced metric and the extrinsic curvature given in Appendix A, the Israel conditions (6) have only a nontrivial part proportional to :
while the boundary conditions (5) can be rewritten as
where . The upper (lower) sign at the right hand side of these two equations refers to a brane at the left (right) of the bulk interval. If one or both branes are absent, equations (12) and (13) can be replaced by different boundary conditions at spatial infinity along the bulk.
In the study of the perturbations, we often make use of the background equations written in this Subsection in order to simplify the linearized equations for the perturbations, without writing this explicitly each time.
It is convenient to characterize the perturbations according to how they transform under 4D Lorentz transformations. Due to the background symmetry, modes that transform differently under these transformations are decoupled at the linearized level, and can be studied separately in our analysis. We therefore have the following decomposition
The modes are scalar (with respect to 4D Lorentz transformations); the modes are vector (we impose that they are transverse, ), and is a tensor (imposed to be symmetric, transverse, and traceless, ). There are also additional scalar modes: the perturbations, of the bulk scalars , and the perturbations, of the brane positions ( runs over the number of branes). All the perturbations are functions of both and , except for which are functions of only. Note that the decomposition (14) becomes ambiguous for massless scalar KK modes, but can be studied using the light cone decomposition of Kiritsis:2006ua (). We assume that there are no massless scalar modes in the cases of interest.
We need to fix the freedom of general coordinate transformations. Under the infinitesimal transformation
(with ) the metric changes as
We can use this relation to see how the various modes in (14) transform. In particular we obtain:
where we have only given the transformations relevant for the present discussion. This allows us to set in (14) and removes the freedom of the transformations in (15) characterized by . Similarly we can also set in (14), which fixes , and choosing then fixes . Therefore we see that one can always choose the gauge ; this completely fixes the freedom of the coordinate transformations (15). This leaves the sets of scalar , vector and tensor modes; these three systems are decoupled from each other at the linearized level, and we will study them separately in the following three sections.
Iii Scalar perturbations
In this Section we write the linearized equations for the scalar perturbations. The main goal is to remove the nondynamical degrees of freedom. As we wrote in the last paragraph of the previous Section, we start from the system of perturbations , where runs over the number of bulk scalars (), while runs over the number of branes.
We can immediately show that the brane displacements are decoupled, and do not introduce any instability. They only enter in the boundary conditions. Specifically, let us assume that a brane is present and consider the linearization of (6) at that location (omitting the index on the displacement ). Using the results in Appendix A, we obtain
(Note that also has a perturbation part). This equation has two tensorial structures that need to vanish independently. In particular, we find that . Using the symmetry at the brane, and the fact that is odd, this equation in turns gives
where denotes the d’Alembertian operator in 4D Minkowski space. As is well known for the single scalar case, the brane bending mode is not sourced by the scalar fields, and is just a decoupled massless mode in the current context. Therefore, in the following we simply disregard this brane mode(s).
We are left with the scalar perturbations . As we discussed in the Introduction, there are only physical perturbations in the scalar sector. In Subsection III.1 we present the linearized bulk equations for the scalars, and show how the two nondynamical modes can be eliminated from two constraint equations. We actually define scalar combinations , that correspond to the canonical variables of the system. In the following three subsections we then compute the boundary conditions for these variables for different relevant cases.
iii.1 Bulk equations
We start by considering the scalar projection of the linearized Einstein equations (2) in the bulk. The components read
The off-diagonal part requires that
From now on, we will enforce this constraint to eliminate . The linearized equations then give
Next, we introduce the combinations
which generalize the canonical variable introduced in Kofman:2004tk () for the case of a single scalar field. These modes are the canonical variables of the system. After the conditions (21) and (22) are used to eliminate the nondynamical modes, one can show (see Appendix B) that the remaining bulk equations are equivalent to the following system of equations for the modes :
This is the explicit set of equations for the dynamical scalar modes of the system.
iii.2 Boundary conditions for finite brane potential
where the left hand side is evaluated in the bulk immediately next to the brane, and the upper (lower) sign at the right hand side refers to a brane at the left (right) of the bulk interval. This equation does not provide any additional information with respect to the bulk equations. We can indeed rewrite the right hand side in terms of bulk quantities using eq.(13); the resulting equation is simply the constraint equation (22) at the brane location. The linearization of (5) is instead nontrivial:
where again the left hand side is evaluated in the bulk immediately next to the brane.
The role of the boundary conditions is to complement the bulk equations (24) and form an eigenvalue problem that can be immediately solved to obtain the physical scalar excitations of the system. By looking at eqs. (24), we see that the most useful form in which these equations can be written is , where the coefficients depend on background quantities. Considerable algebra is required to obtain this equation starting from (26). The final result is
which are indeed equivalent to (26) (we show this in Appendix C). We stress that these equations are valid at the brane location; brane quantities are evaluated immediately next to the brane, and whenever an upper/lower sign appears on the right hand side, it refers to a brane at the left/right of the bulk interval, respectively. Finally, let us clarify the role of the operator on the right hand side. The bulk equations (24) allow for a factorizable solution
Eq. (28) is the decomposition in Kaluza-Klein modes; each mode is characterized by a wave function in the bulk, as well as a 4D (quantum) field . Equations (24) and (27), with the substitution and , provide the complete eigenvalue problem to determine the eigenmasses and the bulk profiles of the scalar modes of the system. It is clear from the form of the equations that this problem is well posed, and can be uniquely solved. We discuss this in detail in Section VI, and provide an explicit example in Section VII.
iii.3 Boundary conditions for (infinitely) stiff brane potential
One can obtain a simpler set of boundary conditions than (27) in the limit of infinitely stiff brane potentials. Let us Taylor expand the brane potential for small fluctuations around the background values :
where the potential and its derivatives on the right hand side are evaluated at the background solution . As can be seen from (12) and (13), only the expectation values of the brane potential and its first derivatives are relevant at the background level. The brane “masses” only enter in the boundary conditions for the linear perturbations; higher-order terms in (30) are instead relevant only beyond the linearized level, and can be disregarded in our study. The stiff potential limit is the limit for which the “masses” are much greater than any other mass scale in the problem. In the original Goldberger-Wise Goldberger:1999uk () stabilization mechanism, this is the limit of large ; it is also explicitly noted there, that the equations considerably simplify in this limit. This limit can always be imposed by simply adding a quadratic potential term centered on the background solution, and then taking the limit of large . Adding this term does not modify the background solution.
The simplification occurs because in this limit at the brane location; this can be seen from eqs. (26). More precisely the fluctuations on the brane “adjust themselves” to the level required to satisfy (26). We actually do not need the explicit solutions for the scalar fluctuations. If we consider the equations in the original set of variables we see that the boundary conditions (26) are the only terms in which the second derivatives are present. These equations can be solved for sufficiently small , but then, once they are satisfied, the only role that these equations play in the stiff limit is to impose that at the boundary can be set to zero in all the other equations of the system. The situation is completely analogous to the scattering of light massive objects against an infinitely heavy object. An object of large mass acquires an infinitesimally small, , velocity in the scattering. For we simply disregard the motion of the heavy object, and the value of drops from the problem; the role of the heavy object is to ensure that the momentum conservation equation is satisfied, but then this momentum conservation equation plays no role in the dynamics of the light mass(es) participating in the scattering. Eqs. (26) are analogous to the momentum conservation equations, is the analog of the mass , and are analogous to the velocity acquired by the heavy object.
In this limit, eq. (23) then imposes the condition
where the proportionality constant is the same for all modes. Eq. (31) provides a system of independent boundary conditions in the eigenvalue problem. The reason why the number is (rather than ) is because the overall normalization of a mode - which is proportional to - cannot be specified by the linearized problem we are solving (if one multiplies the solutions of a linear system by a common factor, one still has a solution). Fortunately, we do not need to know if we are only interested in solving the linearized problem for the eigenmasses of the modes, and therefore we can simply set to any convenient nonvanishing value
(see Section VI).
To obtain the desired expression for , we then differentiate with respect to the second of the bulk equations (LABEL:bulk-sca-i55).
iii.4 Boundary conditions without a boundary brane
Next we comment on the possibility that one or both boundary branes are absent. Assume that the bulk coordinate extends to infinity in that particular direction(s). In this case, the boundary conditions for the perturbations can be dictated by the specific problem under consideration. A typical requirement is the one of normalizability. The set of differential equations (24) has solutions. In the example that we study in Section VII, one finds that half of these solutions exponentially grow at , while the remaining half exponentially decrease. Therefore, eliminating the exponentially growing solutions provides precisely boundary conditions, as it was the case for the boundary conditions enforced by a boundary brane. Other models are characterized by a horizon at some bulk position, and one then typically requires that the solutions should be purely infalling modes at the horizon. Also this requirement corresponds to boundary conditions.
iii.5 Quadratic scalar action, and normalization of the scalar modes
To properly normalize the scalar modes, we compute the kinetic term of their quadratic action, obtained by expanding the starting action (1) at second order in these perturbations. We find
If we replace in the first line of this expression through the constraint equation (21), , we can immediately see that the kinetic term is manifestly positive (recall that ), which ensures that the scalar system has no ghosts. The second line of (LABEL:kin2) has been obtained following the steps outlined before eq. (19) of Kofman:2004tk (), where an analogous computation was performed for the case of a single scalar field. By decomposing as in (28), and, analogously, , we arrive at
In evaluating the boundary term, one can make use of eq. (A-7) to express in terms of and .
We note that the result (37) is the most immediate generalization to fields of the expression (26) obtained in Kofman:2004tk () for the single field case (we note that the sign of the boundary term in the intermediate expression in eq. (26) of Kofman:2004tk () is incorrect). Hermiticity of ensures that eigenmodes with different mass are orthogonal, so . Imposing , we then recover a diagonal and canonically normalized kinetic term
If the linearized equations can be solved analytically, one can leave the normalization of the modes (specifically, the quantity , in the case of a stiff boundary potential), and then fix it through . If the equations can be only integrated numerically, one needs to set a provisory value for the normalization by (arbitrarily) fixing the value of one of the wave functions at one boundary (for instance, in the example that we study in Section VII we set at the UV boundary); after performing the numerical integration, one can then insert the solutions in (37) and obtain the provisory result . The rescaling provides the correctly normalized modes.
Iv Vector perturbations
For the vector modes, the and components of the linearized Einstein equations (2) in the bulk give, respectively,
while the component trivially vanishes. Moreover, the linearization of equations (4) has no contributions from the vector modes. The bulk equations therefore enforce , with . This immediately implies that there are no Kaluza-Klein modes in the vector sector, except for a zero mode.
If branes are present, it is also immediate to see that the linearization of the boundary conditions for the scalar fields, eqs. (5) have no contributions from the vector perturbations. The linearization of the Israel junction conditions, eqs. (6), is instead nontrivial. We see from (7) and (A-2) that the brane stress-energy tensor is independent. Using (A-3), we therefore have
Under the assumption of a symmetry, needs to be odd across the brane,
V Tensor perturbations
The components of the linearized Einstein equations (2) in the bulk give
while the other components trivially vanish. Moreover, the linearization of equations (4) has no contributions from the tensor modes.
If branes are present, we again find that the linearization of the boundary conditions for the scalar fields, eqs. (5) have no contributions from the tensor perturbations. The linearization of the Israel junction conditions, eqs. (6) instead gives
We note that the tensor modes only “respond” to the background geometry, and not to the details of the sources. Therefore, these results are similar to those already derived for the case of a single scalar in the bulk (see, for example, Frolov:2002qm ()). In Ref. Frolov:2002qm () the Kaluza-Klein eigenmasses were shown to be nonegative, so that there is no instability in the tensor sector. For completeness, we summarize this computation here:
One starts by decomposing the 5D tensor field as
where satisfies the Schroedinger-like equation
One can further define the operators
so that the bulk and brane equations become, respectively,
where in the last step we have used the symmetry across the brane.
If the first equation of (46) is multiplied by from the left and integrated over the bulk coordinate , the left hand side can be then integrated by parts. The resulting boundary term then vanishes because of the second equation of (46) and leads to the condition Frolov:2002qm ()
Using Eqs. (46) we can also immediately determine the existence of a tensor massless mode, characterized by the bulk profile
From (43) and the metric decomposition (14), we recover the well-known fact that the massless tensor mode has an identical bulk profile as the background geometry. Incidentally there is no issue with using the decomposition (14) for the massless tensor mode because the tensor equation of motion does not change Kiritsis:2006ua ().
Vi Eigenvalue problem
In the three previous Sections we have obtained the canonical modes in both the scalar and tensor sector, while we have shown that there are no physical vector modes. We have decomposed the canonical perturbations in a Kaluza-Klein sum, and obtained the equations satisfied by the wavefunction of the modes. In the two following Subsections we outline the eigenvalue problem that can be solved to obtain the properties of the physical modes.
vi.1 Scalar sector
When bulk scalars are present, the scalar sector of the perturbations is characterized by the physical 5D perturbations , defined in (23). The wave functions of the corresponding Kaluza-Klein modes satisfy the second order differential equations (24). Each KK mode is therefore characterized by parameters (the mass , and the values required to specify the Cauchy problem), so that the bulk differential equations need to be supplemented by conditions. Each boundary brane enforces conditions, given by eq. (27) in the case of finite brane potentials, and by eqs. (31) and (34) in the case of infinitely stiff brane potentials. We discussed in Subsection III.4 the typical boundary conditions that can be imposed in the case that one or both branes are absent (in general, we expect conditions per boundary). One additional condition is obtained by fixing the overall normalization of the modes. One can typically start by fixing a provisory (and, generally, incorrect) normalization; for instance, one can require that one of the wave functions evaluates to at one boundary. This, together with the conditions coming from the two boundaries, allows the system of linearized equations to be completely solved. In this way, one obtains the masses of the physical modes, and the wavefunctions, up to an overall, yet to be specified, normalization. We stress that the overall normalization of the solutions is an irrelevant quantity in a linearized system of equations (if we rescale all the modes of a solution by a common factor, we still have a solution). Therefore, the system of equations can be solved, and gives the correct values of the eigenmasses, for any arbitrary overall normalization. Still, the overall normalization is crucial to determine the couplings of the perturbations, (since the couplings are determined by the values of the wavefunctions); Subsection III.5 explains how to rescale the solutions, so as to obtain the correct normalization, once the linearized system has been solved.
In many cases, the bulk equations cannot be solved analytically; we expect this to be the norm in the scalar sector, where the perturbations are coupled in the equations (this happens even if the bulk potential is a sum of separate terms, due to the mixing of the scalar field perturbations with the metric perturbations). In this case, the eigenvalue problem needs to be solved with a shooting method; one fixes half of the parameters that are necessary to determine the bulk evolution, by enforcing the conditions at one of the two boundaries. Next one guesses the remaining parameters, and solves the bulk equations which enable the wave functions to be evaluated on the other boundary. If the resulting solutions happen to satisfy the boundary conditions also there, then one has obtained a physical mode of the system. Typically, the initial guess is not correct, and one needs to employ some numerical scheme to obtain the solutions. For example, one can compute by how much the wavefunctions evaluated at the second brane differ from the expected boundary conditions, as a function of the initial guesses. An -dimensional Newton’s method can then be implemented to find the zeros of this function. We perform this algorithm in the example studied in the next Section.
vi.2 Tensor sector
The tensor sector is significantly simpler than the scalar sector. The wave functions , defined in equation (43), satisfy the second order differential equation (44) in the bulk. Each solution is in principle characterized by three parameters: the mass of the eigenmode, and two integration constants . However, as for the scalar case, only the ratio of these two constants, and not the overall normalization of the solution, can be determined from the linearized problem. Therefore to just obtain the eigenmasses and bulk profiles we can simply fix an arbitrary normalization by requiring that acquires a nonzero (but arbitrary) value at a given position (typically, at one boundary brane). This gives one condition. The other two conditions are enforced by the boundary branes (each brane enforces one condition, given by the last expression in (46)), or if a brane is absent, by the requirement that the wavefunction is normalizable. These three conditions then allow and to be determined with the bulk profiles known up to an overall normalization. The correct normalization can be then obtained from the quadratic action of the tensor modes, analogously to what we dicussed for the scalar sector.
Vii An explicit example: the dynamical soft wall
As an explicit example of the general method that we have outlined above, we will consider the dynamical soft-wall solution found in Ref. Batell:2008zm (). In addition to the metric, this solution involves two bulk scalar fields. It provides a dynamical realization of the holographic soft-wall model for QCD Karch:2006pv (); Karch:2010eg (), as well as applications to the electroweak sector of the Standard Model Batell:2008me ().
vii.1 The 5D model
We review the soft wall background solution Batell:2008zm () (with the only difference that we use our convention for , that corresponds to in Batell:2008zm ()). The model is characterized by the two fields and , with the bulk potential
One obtains the background solution
The parameter is a dimensionless constant, while is the soft-wall mass scale. As the bulk volume diverges at , a UV brane is placed at . The potential on this brane is chosen so that the solutions (50) satisfy the boundary conditions there: specifically, the background values of and are determined from (12) and (13). We then assume that the brane potential contains large quadratic terms (30), so that the boundary conditions for the perturbations can be given in the infinitely stiff limit of Subsection III.3.
The scalar field configuration provides a finite bulk geometry in the limit , so that there is no need to include a boundary IR brane at large (in fact this is the reason for why it is a “soft wall”, as opposed to a sharp brane or hard-wall cut-off). As we will see in the next two Subsections, the requirement that the perturbations are normalizable there provides sufficient boundary conditions to fully determine them. We focus our study of the perturbations of this model to the choice , as this gives rise to a linear Regge-like mass spectrum, , for the KK modes, which is similar to that encountered in the hadron spectrum of QCD.
vii.2 Tensor modes
The tensor modes for the model were already studied in Batell:2008me (). We summarize these results here for completeness, and to provide an example of an eigenvalue problem that can be solved analytically (and that is technically simpler than the problem for the scalar modes studied in the next Subsection).
It is convenient to use the variable (where TT denotes the transverse-traceless component) for the eigenvalue problem. The Kaluza-Klein decomposition is analogous to (43), and we denote by the wave function of the th mode (, where is introduced in (43)). In the background (50), the bulk equation eq. (41) becomes
where we have introduced the dimensionless quantities and . The boundary condition at the UV brane then has the form
(where corresponds to the location of the UV brane) while the normalizability requirement at translates into the requirement that the solution decreases sufficiently fast at large . More precisely, since the wave function of the canonically normalized mode is , we require that .
The normalizable solution of Eq. (51) is (up to a normalization constant) the Kummer’s confluent hypergeometric function
Eq. (52) is approximately satisfied at the poles of the gamma function, namely for
(we verified numerically that there is indeed no physical mode corresponding to ). We note that in agreement with the general result (47).
vii.3 Scalar modes
where prime () denotes differentiation with respect to , and where the subscript () corresponds to the field (). As we discussed in Section III, to fully determine a mode we must specify the five quantities (, with )
where we recall that is the position of the UV brane in the rescaled variable .
We assume a stiff brane potential on the UV brane, which enforces the Dirichlet boundary conditions (see Subsection III.3). This in turn results in the two boundary conditions (31) and (34). Moreover, we fix the arbitrariness of the overall normalization by fixing the value of at the UV brane. This, together with Eq. (31) gives
We are left with the three parameters subject to the constraint (34):
We used this constraint to determine as a function of and .
The bulk coordinate extends to . To understand the role of the associated boundary conditions, we studied the bulk equations in the limit of large :
We obtained the approximate solutions to these equations under the assumption that one mode is significantly larger than the other one in this limit; the subdominant mode can then be disregarded in the equation of the dominant mode; this equation can be solved analytically, and we can then insert this solution in the remaining equation to obtain the subdominant mode. We then studied the large limit of the solutions, and verified that the starting assumption (the subdominant mode can be neglected in the equation of motion of the dominant one) holds. In this way, we obtained four solutions, that form a complete basis for the solutions of the bulk equations. At , the four solutions read