Holographic oddballs

The spectrum of the glueball with JP C = 0−− is computed using different bottom-up holographic models of QCD. The results indicate a lowest-lying state lighter than in the determination by other methods, with mass m ≃ 2.8 GeV. The in-medium properties of this gluonium are investigated, and stability against thermal and density effects is compared to other hadronic systems. Production and decay modes are identified, useful for searching the JP C = 0−− glueball.


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tions needed to describe confinement. In QCD, composite gauge-invariant local operators with quantum numbers J PC = 0 −− , involving only gluon fields, can be written in terms of the gluon field strength G a µν (x) and the dual G a µν (x) = 1 2 µνρσ G a ρσ (x): with a, b, c color indices, d abc the symmetric SU(3) c structure constants, and g s the strong coupling constant. The transverse η t αβ metric is defined as η t αβ = η αβ − ∂α∂ β ∂ 2 , with α, β (as well as µ, ν) 4D Lorentz indices, and η αβ the Minkowski metric tensor [7].
We focus on only one operator in (2.1), generically denoted as J 0 (x), which has conformal dimension ∆ = 8, and associate to J 0 (x) a dual field in AdS 5 , O 0 (x, z), with mass obtained by the relation M 2 5 R 2 = ∆(∆ − 4) [10,11]. R is the AdS 5 radius; we set R = 1. We choose Poincarè coordinates x M = (x µ , z) = (x 0 , x, z) for the AdS 5 space, with line element (0 < z), and define an action for the field O 0 (x, z). To account for confinement in QCD, in the definition of the action the breaking of conformal invariance must be implemented: this can be done in different ways, some of which are used in the following.

Hard-wall model (HW)
A simple way of modeling confinement in the holographic setup is by considering a slice of the AdS 5 space, with a sharp cutoff at a finite distance z m along the extra dimension [21,22]. The 5D action for O 0 (x, z) can then be written as with ≤ z ≤ z m and g = |det(g M N )|. The constant k makes the action dimensionless, and its derivation is presented in the next section. The value of 1/z m sets the hadronic scale in the model, so that the dimensionful quantities are given in terms of this parameter. The equation of motion for the Fourier together with the Dirichlet boundary condition for O 0 (p, z) at the ultraviolet z = brane, O 0 (p, ) = 0 (with → 0 + ), and the Neumann boundary condition at the infrared z = z m brane, ∂ z O 0 (p, z m ) = 0, allows to compute the spectrum. The resulting lightest masses, in phenomenological analyses [21]. A linear dependence is obtained for m n vs the radial (in the extra dimension) quantum number n, a feature shared by other hadrons described by this model.
can be computed using the AdS/CFT dictionary identifying J 0 (x) as the source of O 0 (x, z). We define the (4D Fourier transformed) bulk-to-boundary propagator K(p, z) of the glueball field using the equation: with O 0 (p, z) and J 0 (p) the 4D Fourier transformed bulk field and source, respectively, and differentiate twice the on-shell action (2.5) with respect to J 0 . The two-point correlation function, obtained for J 0 → 0, can be written as with the residues R n = − 4 15 (n + 6)! 6! n! c 14 k . (2.12) Comparing the p 2 → −∞ asymptotic behaviour of Π(p 2 ) in QCD [7] Π QCD (p 2 ) = 487α 3 with the expression (2.10) in the same limit, we fix k (for N c = 3): (2.14) The same expression holds in the HW model.

Einstein-dilaton model (ED)
In both the HW and SW models the implementation of the confinement mechanism, with an AdS 5 background geometry, is an input assumption defining each model. More elaborated approaches include dynamical fields. A dynamical holographic model of QCD has been formulated in [31,32], with a scalar dilaton field Φ(z) in the bulk and the 5D gravitationdilaton coupled action analysed. The resulting geometry takes the form:

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The function A s (z) introduces a quadratic correction in the warp factor distorting the AdS 5 metric, and is chosen with the expression A s (z) =ck 2 z 2 . The profile of the dilaton is obtained solving the Einstein equations for the metric-dilaton system, and with the chosen ansatz for A s (z), Φ(z) reads in terms of the generalized hypergeometric function 2 F 2 . In the model, the dimensionful parameterk is set tok = 0.43 GeV.c isc = ±1, and both cases reproduce, at finite temperature, QCD bulk thermodynamical properties such as the energy density and the speed of sound. On the other hand, the analysis of the thermodynamical properties of loop operators favours the positive sign; hence, we setc = +1. The equation of motion for the oddball field O 0 (x, z) with the metric (2.15)-(2.16) provides for the two lightest states the mass m 0 = 2.82 GeV and m 1 = 4.07 GeV, respectively, close to the result of the HW model.
The outcome of the analyses in the three models is that the mass of the lowest-lying 0 −− state is sensibly lighter than obtained in [6,7], with results spanning the range 1.55 − 2.82 GeV. The upper value, obtained in the HW and ED models, is close to the prediction of the flux-tube model. For the first excited state, the predicted mass is in the range 1.74 − 4.07 GeV, with again the lighter value given by the SW model. The indication in favour of a light oddball is a surprising result with interesting phenomenological implications. Indeed, one can look for this state in the same class of processes investigated for searching the 0 ++ gluonium, namely radiative quarkonium decays including charmonium. The second consequence is that there is enough phase-space for 0 −− decays with a quite clear experimental signature. We discuss both the issues in section 4.

Oddballs in medium
Before addressing the phenomenology of the lightest oddball, it is interesting to use the same holographic machinery to investigate other aspects of this gluonic state, namely its features in a thermalized and dense hadronic medium. The aim is to make a comparison with the conventional light vector meson and with the scalar glueball, inferring information on the stability properties of the oddball against thermal and density fluctuations. In the holographic approach, the inclusion of matter effects is affordable using appropriate bulk geometries [12]. For definiteness, we consider the SW model for which many results concerning other hadrons are available for the comparison [33,34].
To investigate in-medium effects on the oddball spectrum, we use the 5D Reissner-Nordström AdS metric (AdS/RN). The issue of which phase of QCD is described by this bulk geometry is deferred to the end of this section; for the time being, we consider the possibility of describing a stable or a metastable phase [35].
The AdS/RN geometry is defined by the line element

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with the function f (z) given by At q = 0 the geometry (3.1), (3.2) reduces to the AdS/black-hole metric. z h is the position of the outer horizon of the black-hole, the lowest value of the coordinate z satisfying the condition f (z h ) = 0. Defining Q = qz 3 h and imposing the condition 0 Q √ 2, the black-hole temperature is In (3.2) q is the charge of the black-hole, which can be holographically related to the quark chemical potential µ. In the QCD generating functional, µ multiplies the quark number operator O q (x) = q † (x)q(x). Invoking the gauge/gravity correspondence, the coefficient µ can be considered as the source of the bulk field associated to O q (x), the time component of a U(1) gauge field A M (x, z). The AdS/RN metric results from the gravitational interaction of this U(1) field. Within the SW model, we make use of the AdS/RN geometry together with the background dilaton characterizing the model. To fulfil rotational invariance, the U(1) field A M has components A i = 0 for i = 1, 2, 3, z , while the component A 0 has the expansion, for z → 0, The condition that A 0 vanishes at the horizon, A 0 (z h ) = 0, provides a linear relation between µ and q (or µ and Q), in terms of a dimensionless parameter κ that can be determined from various observables [36]. In the following we set κ = 1, giving the quark chemical potential up to a numerical factor. We also set the dilaton parameter c = 1 and the dimensionful quantities in units of such a scale. The equation for the bulk-to-boundary propagator K(p, z), obtained from the action (2.5) with AdS/RN background geometry, reads: In the frame with p = 0, defining ω 2 = p 2 0 and using the variable u = z/z h , we compute the solution of (3.6) with the boundary conditions JHEP10(2015)137 The latter condition selects the in-falling solution near the horizon. Hence, the retarded Green's function is worked out [37][38][39], and the spectral function ρ(ω 2 ) = Π R (ω 2 ) is determined in ranges of temperature and chemical potential.
At µ = 0, the result in the range of ω 2 corresponding to the lightest resonance is depicted in figure 2, where we plot ρ(ω 2 )/(ω 2 ) 6 (factorizing the constant 10 −8 k/(2z 8 h )) to account for the ρ large-ω 2 dependence. At small T the spectral function displays a narrow resonance, with vanishing width for T → 0. As T increases changing the bulk geometry, the peak moves towards smaller values of ω 2 , accompanied by a broadening of the line shape: the thermal effects on the gluonium reduce the mass and make the state unstable. At some value of T the peak disappears from the spectral function, indicating the in-medium melting of the state.
Also at finite µ the peaks of the spectral function broaden and move towards smaller values of ω 2 as T increases, up to a point where no peak can be distinguished. The same behavior is observed at fixed temperature, increasing the chemical potential. The broadening is a signal that, as the temperature or the quark chemical potential increases, the states become unstable, getting a finite width (a quantum-mechanical argument for such a behavior is in [34]). The results are collected in figure 3 for two values of µ and T .
To quantitatively extract the temperature and chemical potential dependence of the lightest oddball mass, we fit the peak in the spectral function ρ(ω 2 ) using a Breit-Wignerlike expression [33,40]:   to the point where the line-shape starts broadening. The results for two values of T and µ are shown in figure 4, and a synopsis of the T − µ dependence is presented in figure 5.
One can now make a comparison with other hadrons. Considering light vector and scalarqq mesons, the lightest scalar glueball and hybrid mesons, the values of T and µ where the peak of the lowest lying oddball disappears from the spectral function are by far smaller [26,34]. This can be interpreted as an indication of a higher sensitivity of this hadron to thermal and matter effects at T = 0 and µ = 0, and that the state is less stable than other conventional hadrons.
In the above discussion, we have assumed the AdS/RN geometry as suitable to formulate a QCD dual regardless of the values of T and µ. However, with this geometry it is known that duality holds above a line in the T − µ plane, where the deconfined phase is realized; at small T and µ AdS/RN represents a metastable phase, the confining phase being described, e.g. at µ = 0, by thermal-AdS. The transition between the two phases is holo-JHEP10(2015)137 graphically represented by a Hawking-Page transition [35]. This can be seen considering in greater detail the limit T → 0 with finite chemical potential µ.
In the AdS/Reissner-Nordström model the limit T → 0 , µ = 0 corresponds to Q 2 → 2 (while z h → ∞ corresponds to T = 0 and µ = 0). This is the case of an extremal black hole with coinciding outer and inner horizon. The black hole function has a double zero in z = z h : (3.10) Moreover, at T = 0 the geometry has a horizon and a non-vanishing entropy, a known feature of models based on the RN metric and used in the framework of the emergent quantum criticality. Other consequences are in the determination of the spectral functions, where the behavior of the solution of the equation of motion near the horizon is needed. For Q 2 = 2 the asymptotic solution contains divergent terms proportional to p 2 0 , which hinder the selection of the in-falling condition. In studies of, e.g., transport coefficients at T = 0 and µ = 0, the condition p = 0 together with the limit p 0 → 0 avoids divergences in the correlation functions [41].
It has been proposed to study the points at T = 0 , µ = 0 considering a model having the function f (z) in the geometry given by [36] f (z) = 1 + q 2 z 6 (3.11) and the time-component A 0 (z) in (3.4). The metric (3.1), (3.11) is solution of the Einstein equations, with the condition f (z h ) = 0 replaced by putting to zero the coefficient of z 4 . While in the HW model the vanishing A 0 (z 0 ) = 0 at the IR brane provides a relation between µ and q, in the SW model, a linear relation between µ and q can be assumed, with the coefficient fixed computing the boundary action [42]; the dilaton term in the action allows to cure the divergence of f and A 0 at large z (naked singularity). As in the thermal AdS model, the temperature can also be implemented using a periodic Euclidean time coordinate. The obtained geometry (thermal charged AdS -tcAdS) is proposed as JHEP10(2015)137 a dual of the confined phase of QCD at small temperature and chemical potential, while the AdS/Reissner-Nordström model describes the deconfined phase, with a Hawking-Page transition between the two phases [36]. Using the geometry (3.1), (3.11) at T = 0, the two lightest gluonium states have mass as depicted in figure 6, and at small T the results remain unaffected. The difference with respect to the AdS/RN model is the increasing behaviour vs µ, a confirmation that the two models describe different phases of QCD.
The conclusion of the analysis is that, using AdS/RN, the 0 −− oddball is more sensitive to matter effects than all other hadrons studied in the same framework, including the 0 ++ glueball and the 1 +− hybrid [26,34]. On the other hand, with the tcAdS geometry a peculiar µ-dependence of the hadron mass is found.

J PC = 0 −− glueball phenomenology
In our calculations the lowest gluonium state with J PC = 0 −− is quite light. On the basis of this result, we select suitable processes for the production and the identification of this state. 2 Our guidelines are the quantum number selection rules, since the relevant hadronic couplings cannot be computed in the models we are using here. For definiteness, we consider the lightest oddball with mass m 0 −− = 2.8 GeV.
corresponding bottomonium transitions), are only possible for very heavycc (bb) decaying states. We remark the P-wave two-body h b (nP ) decays in J PC = 0 ++ scalar glueball and J PC = 0 −− oddball, which are very peculiar modes for the exclusive gluonium production.
Decay modes of the J PC = 0 −− glueball are listed in table 3. In addition to the modes involving the axial I = 0 f 1 (1285) meson, it is worth mentioning the full set of P −wave decays, among which there is ρπ(I = 0). The couplings governing the various modes cannot be computed in the framework discussed here, and require specific calculations deferred to a dedicated study.

Conclusions
Our main result is that the lowest-lying J PC = 0 −− glueball, examined in different bottomup holographic models of QCD, is lighter than envisaged by other approaches. This opens interesting possibilities for the experimental search of this unconventional hadron. We have also investigated the in-medium effects, obtaining that using AdS/RN the 0 −− oddball is more sensitive to matter effects than all other hadrons studied in the same framework. On the other hand, with the tcAdS geometry a peculiar µ-dependence of the hadron mass is found. Several production and decay modes can be exploited for the search of this elusive gluonium resonance.
As a final remark, we find inspiring that the lowest mass we have obtained using the SW model is close to the D 0 mass, in view of the dominance observed in D 0 → π + π − π 0 of an exotic J PC = 0 −− isoscalar state. It is worth reconsidering this issue in a dedicated study.