Joint Topics on Exotic Hadron States and Heavy Flavor Hadronic Decay
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Pablo G. Ortega, David R. Entem, Francisco Fernández, "Unquenching the Quark Model in a Nonperturbative Scheme", Advances in High Energy Physics, vol. 2019, Article ID 3465159, 7 pages, 2019. https://doi.org/10.1155/2019/3465159
Unquenching the Quark Model in a Nonperturbative Scheme
Abstract
In recent years, the discovery in quarkonium spectrum of several states not predicted by the naive quark model has awakened a lot of interest. A possible description of such states requires the enlargement of the quark model by introducing quarkantiquark pair creation or continuum coupling effects. The unquenching of the quark models is a way to take these new components into account. In the spirit of the Cornell Model, this is usually done by coupling perturbatively a quarkantiquark state with definite quantum numbers to the mesonmeson channel with the closest threshold. In this work we present a method to coupled quarkantiquark states with mesonmeson channels, taking into account effectively the nonperturbative coupling to all quarkantiquark states with the same quantum numbers. The method will be applied to the study of the X(3872) resonance and a comparison with the perturbative calculation will be performed.
1. Introduction
Constituent quark models (CQM) have been extremely successful in describing the properties of hadrons such as the spectrum and the magnetic moments. However, since the earliest days of the hadron spectroscopy, it was realized [1] that such models neglect the contribution of higher Fock components (virtual pairs, unitary loops, or hadronhadron channels) predicted by QCD. Unquenching the quark model is a way to incorporate these components, in a similar way as unquenched lattice theories included dynamical quarks instead of static quarks (quenched theories). It is worth noticing, though, that the name “unquenched quark model” refers to different approaches to include these higher Fock components. Thus, Tornqvist and collaborators [2, 3] use a “unitarized” quark model to incorporate the effects of two meson channels to and spectrum. Van Beveren and Rupp [4, 5] showed the influence of continuum channels on the properties of hadrons, in a model which describes the meson as a system of one or more closed quarkantiquark states in interaction with several two meson channels. More recently, Bijker and Santopinto [6] developed an unquenched quark model for baryons, in which a constituent quark model is modified to include, as a perturbation, a QCDinspired quarkantiquark creation mechanism. Under this assumption, the baryon wave function consists of a zerothorder threevalence quark configuration plus a sum over baryonmeson loops.
The components beyond the naive constituent quark model became more relevant since 2003, when the and other XYZ states were discovered. At that time hadron spectroscopy begins to measure hadron states near two particle thresholds and in this situation loop corrections are relevant.
The resonance has been studied using different versions of the unquenched quark model in Ref. [7–9]. Eichten et al. [7] considered the influence of mesonmeson channels using the Cornell coupled channels scheme [10], obtaining a perturbative mass shift of the configuration below threshold and an additional decay width for configurations above threshold. Using the Resonance Spectrum expansion [11] Coito et al. showed that the is compatible with a description in terms of a regular charmonium state with a renormalized mass, via opened and closed decay channels. Finally, in Ref. [12], it was shown that one can describe the as a interpreted as a core plus higher Fock components due to perturbative coupling to the mesonmeson continuum.
A different point of view from the references mentioned above is presented in Ref. [13]. The authors of Ref. [13] also study the coupling of the states with mesonmeson channels, but in this case the mesonmeson interaction which originates by the underlying quarkquark interaction is fully taken into account, in contrast to other studies such as Ref. [14]. The approach of Ref. [13] allows to have bound states not only in the channels but, under certain circumstances, in the mesonmeson channels. They start from a coupled channels approach for the channel, to study the influence of the channels in the mesonmeson one. Solving the coupling for the states one arrives to a Schrödingertype equation in which the mesonmeson interaction gets modified by the coupling with the bare states, generating a resonance which can be identified with the . Besides this state, one gets an orthogonal one which can be identified with the . Both are different combinations of and mesonmeson states.
Some models, as our previous work in Ref. [13], choose a particular state which gets modified by the interaction with the two meson channels. Usually, the states “closer” to the threshold of the mesonmeson channel are chosen, but sometimes it is difficult to decide which ones are relevant. Moreover, in some models, this state is modified perturbatively.
In an attempt to improve these caveats, we have developed a new scheme in which the contributions of the complete tower of radial excitations corresponding to a given value of states are automatically taken into account. A similar approach was already done in Ref. [14], in which a model that can be solved analytically was used, but with no mesonmeson interaction included. The rationale of the method is to leave the radial wave function as unknown to be determined dynamically. Afterwards, the contribution of each “quenched” state is determined by expanding the obtained wave function in a bare quarkantiquark base. In this way, one incorporates from scratch all possible states and also allows the deformation of the bare wave function due to interaction with the mesonmeson channels. Although the method is general for baryons and mesons, for the sake of clarity in this paper we will develop it only for mesons.
The paper is organized as follows. In Section 2 we first discuss the coupled channel formalism and the coupling mechanism between the different channels and the basic ingredients of the constituent quark model. Results and comments are presented in Section 3. Finally, we summarize the main achievements of our calculation in Section 4.
2. The Model
2.1. The Constituent Quark Model
The constituent quark model used in this work has been extensively described elsewhere [15, 16] and therefore we will only summarize here its most relevant aspects. The chiral symmetry of the original QCD Lagrangian appears spontaneously broken in nature and, as a consequence, light quarks acquire a dynamical mass. The simplest Lagrangian invariant under chiral rotations must therefore contain chiral fields and can be expressed aswhere is the Goldstone boson fields matrix and is the dynamical (constituent) mass. This Lagrangian has been derived in Ref. [17] as the lowenergy limit in the instanton liquid model. In this model the dynamical mass vanishes at large momenta and it is frozen at low momenta, for a value around 300 MeV. Similar results have also been obtained in lattice calculations [18]. To simulate this behavior we parametrize the dynamical mass as , where , andThe cutoff fixes the chiral symmetry breaking scale.
The Goldstone boson field matrix can be expanded in terms of boson fields,The first term of the expansion generates the constituent quark mass while the second gives rise to a oneboson exchange interaction between quarks. The main contribution of the third term comes from the twopion exchange which has been simulated by means of a scalar exchange potential.
In the heavy quark sector chiral symmetry is explicitly broken and this type of interaction does not act. However it constrains the model parameters through the light meson phenomenology and provides a natural way to incorporate the pion exchange interaction in the open charm dynamics.
Below the chiral symmetry breaking scale quarks still interact through gluon exchanges described by the Lagrangianwhere are the SU color generators and is the gluon field. The other QCD nonperturbative effect corresponds to confinement, which prevents from having colored hadrons. Such a term can be physically interpreted in a picture in which the quark and the antiquark are linked by a onedimensional color fluxtube.
Lattice calculations have shown that, as far as the quarks get separated, virtual quark antiquark pairs tend to modify the confinement potential, giving rise at some scale to a breakup of the color fluxtube [19]. Coupled channels and screening potential represent similar physics [20]. However, our approach is to couple those channels whose thresholds are near to the states we are studying in detail; therefore it should not be treated perturbatively, and, furthermore, averaging the effects of the rest of the thresholds through the following screened confinement potential,Explicit expressions for these interactions and the value of the parameters are given in Ref. [15, 16].
2.2. The Unquenched Meson Spectrum
Although over the time the procedure to incorporate new Fock components to the wave function has received several names (unitarized quark model [2], resonance spectrum expansion [11], and coupled channel formalism [1]) the basic idea behind the unquenched meson model is to assume that a hadron wave function with fixed quantum numbers combines a zerothorder configuration plus a sum over the possible higher Fock components due to the creation of pairs:where stands for the operator which couples the different components, usually the quarkantiquark pair creator, and is an eigenstate of the bare Hamiltonian .
In practice what is done is to assume that the first Fock component, namely, the structure, is renormalized via the influence of nearby mesonmeson channels and, thus, coupled channels calculation is performed including the bare state and the mesonmeson channels. Solving the coupling with the mesonmeson channels one obtains for the mass shift of the meson where is the kinetic energy of the mesonmeson pair.
As stated in the introduction, this method has two important shortcomings. First of all, it focuses the study on the modification of the channel, avoiding the study of the mesonmeson channel where interesting structures may appear. Second, it is chosen from the beginning one channel to be modified, neglecting those channels which may be generated in the interaction with the mesonmeson channel.
For these reasons, we have developed a new scheme in which the contributions of all states are initially taken into account, being the dynamics the responsible of selecting the contribution of each bound state.
The Hamiltonian we consideris the sum of an “unperturbed” part and a second part which couples a system to a continuum made of mesonmeson states.
Instead of expanding the wave function of the system in eigenstates of the Hamiltonian and then solving the coupled channels equation with the mesonmeson channels, we use a general wave function for the system to solve the coupled channels problem and then develop the solution of the system in the base of the bare states. In this way, the dynamics of the system is the element which determines the contribution of each bare state to the eigenstate, obtained from the twobody Schrödinger equation which includes the effect of the dynamics of the nearby mesonmeson channels.
The meson wave functions to be used all along this work will be expressed using the Gaussian Expansion Method [21] (GEM), expanding the radial wave function in terms of basis functionswhere refers to the channel quantum numbers and are Gaussian trial functions with ranges in geometrical progression. This choice is useful for optimizing the ranges with a small number of free parameters [21]. In addition, the density of the distribution of the Gaussian ranges in geometrical progression at small ranges is suitable for making the wave function correlate with short range potentials.
To introduce higher Fock components in the wave function we assume that the hadronic state iswhere is the wave function, are eigenstates describing the and mesons, is the twomeson state with quantum numbers coupled to total quantum numbers, and is the relative wave function between the two mesons in the molecule. The mesonmeson interaction will be derived from the interaction using the Resonating Group Method (RGM) [22].
We must notice that, although the Gaussian Expansion Method of the wave functions can be also used for the mesons constituting the molecular states, we will assume that the wave functions of these mesons are simple solutions of the Schrödinger twobody equation.
In order to couple both sectors, we use the QCDinspired model [23], which gives a clear picture of the physical mechanism of the coupling. In this model, a quark pair is created from the vacuum with the vacuum quantum numbers. After the pair creation, a recombination of the quarkantiquark of the initial meson with the pair follows to give the two final mesons. The quarkantiquark paircreation operator can be written as [24]where () are the quark (antiquark) quantum numbers and with is a dimensionless constant which gives the strength of the pair creation from the vacuum.
Finally, in the context of the model, the transition operator can be defined from the operator aswhere is the relative momentum of the twomeson state.
Now, we use Eq. (9) to decompose as
Then, the coefficients of the meson wave function and the eigenenergy are determined from the coupledchannel equationswhere is the normalization matrix of the GEM trial Gaussian functions, is the interquark Hamiltonian that defines the bare meson spectrum, and is the RGM Hamiltonian for the two meson states, obtained from the interaction. In the previous equations we have defined the perturbative mass shift as which codifies the coupling with molecular states. Apparently, the perturbative mass shift does not mix different channels, so the only operator which mixes them is the potential in . However, as will be detailed below, the molecular wave function is dependent on different meson channels.
The previous coupled channel equations can be solved in a more elegant way through the matrix, solution of the LippmannSchwinger equation,where is the RGM potential.
Using the matrix, we end up with a Schrödingerlike equation for the coefficients,
In the previous equation we identify as the energydependent complete massshift matrixwhere is the potential dressed by the RGM mesonmeson interaction,which can be decomposed in the GEM basis as in Eq. (13).
In order to find molecular states above and below thresholds in the same formalism we have to analytically continue all the potentials for complex momenta. Therefore, resonances are solutions of Eq. (17), with the pole position solved by the Broyden method [25].
The molecular wave function is related with the coefficients of the meson state,with the normalization given by
The partial decay widths can be defined through the complete Smatrix of the mix channel, as detailed in [26].
3. Calculations, Results, and Discussions
In order to compare the results of the proposed scheme with the perturbative one we perform a similar calculation as in Ref. [13], namely, a coupled channel calculation including the sector and the and channels. We, first of all, perform a calculation with the same parameters as [13] in the charge basis
Isospin symmetry is explicitly broken taking the experimental threshold difference into account in our equations and solving for the charged and the neutral components.
One can see in Table 2 that when we use the value of we get three states with energies close to the , the , and the MeV. The first two states are mixtures of and components, being the predominantly and the mostly . The third state is clearly a state. If we project the component in the base of bare states (Table 3) we realize that this third state is an almost pure state whereas the other two are predominantly . In order to compare with the bare spectrum we show in Table 1 the charmonium states in the vicinity of the , only up to the first radial excitation.



One can analyze the isospin content of the component of the different states. The only one which shows a sizable component is the one we have identified with the . The other two are basically states. Notice that all the interactions are isospin conserving interactions and the reason to have a nonzero component for the is that the binding energy of the component for this state is smaller than the isospin breaking of the and masses which enhances the component at large distances.
As in Ref. [13], we have finetuned the parameter to get the right binding energy of the . The results are shown in the second part of Table 2. We get again three states. The first one, with a mass of MeV, can be identified with the [28] and is a mixture of of and of molecule with isospin . The component is basically a state. The second state has now the right energy of the resonance. The clearly dominates its structure with a probability, giving a probability for the isospin component and for isospin , which is enhanced in this case because the binding energy is much smaller compared with mass difference of the neutral and charged components. As the isospin breaking is a threshold effect, it grows as we get closer to the physical mass. The component is, as in the previous state, a bare state. Finally we get an almost pure state with a mass of MeV.
The scenario drawn by these results consists of two bare states (a molecule and a state), which mix together to give the two physical states, and a third state which participates slightly into the game, although, as we will see, its contribution is important. The result is similar to those of Ref. [13], within the uncertainties of the model, but now it appears dynamically without the need to make educated guesses about the bare states involved in the calculation. In this way we are confident that all the physics is included into the model.
Although not addressed in Ref. [13], we have calculated with our wave functions the two decay rates that represent a challenge in the description of the structure, namely, has been measured by BaBar Collaboration [29] obtaining . A value of has been recently reported by LHCb Collaboration [30].
Whereas , which showed a large isospin symmetry breaking, has been used to justify that the should be hadronic molecule, the high value of was interpreted as a strong evidence that the cannot be a pure hadronic molecule, based on the claim that the contributions of the molecular component to this ratio should be small [31].
Our wave function allows for a simultaneous description of both ratios. To calculate we have assumed that the decay proceeds through the component, obtaining the value which is clearly far from the experimental value. A similar result is obtained in [32], where it is shown that if the states are neglected the ratio approaches to the experimental value. In our approach the appears automatically. Then, it seems that a more careful calculation of this decay in the line of Ref. [33, 34] should be done.
The obtained value for the first ratio is that is close to the experimental result, similar to the values obtained in Ref. [35–37].
4. Summary
In this work we present a method to coupled quarkantiquark states with mesonmeson channels, taking into account effectively the nonperturbative coupling to all quarkantiquark states with the same quantum numbers. Instead of expanding the wave function of the system in eigenstates of the Hamiltonian and then solving the coupled channels equation with the mesonmeson channels, we use a general wave function for the system to solve the coupled channels problem and then develop the solution of the system in the base of the bare states. The method is applied to the coupling of the resonance to the states and the results were compared with those of the perturbative calculation of Ref. [13].
Data Availability
The data used to support the findings of this study are included within the article.
Conflicts of Interest
The authors declare that they have no conflicts of interest.
Acknowledgments
This work has been funded by Ministerio de Economía, Industria y Competitividad under Contract No. FPA201677177C22P. Pablo G. Ortega acknowledges the financial support from Spanish MINECO’s Juan de la CiervaIncorporación program, Grant Agreement No. IJCI201628525.
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Copyright
Copyright © 2019 Pablo G. Ortega et al. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited. The publication of this article was funded by SCOAP3. The publication of this article was funded by SCOAP^{3}.