On the two-body decay processes of the predicted three-body K*(4307) resonance

In a recent theoretical work, Phys. Lett. B785, 112 (2018), we proposed that a K* resonance with hidden charm content arises from the KDD¯∗\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ KD{\overline{D}}^{\ast } $$\end{document} dynamics, where the DD¯∗\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ D{\overline{D}}^{\ast } $$\end{document} system is treated as a Zc(3900) or X(3872). With the motivation of determining its further properties, which can be observed in experiments, we now present a calculation of the decay processes of this K*, namely K*(4307), to two-body channels. Particularly, we consider the decay channels J/ψK*(892), D¯Ds\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \overline{D}{D}_s $$\end{document}, D¯Ds*\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \overline{D}{D}_s^{*} $$\end{document} and D¯∗Ds*\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {\overline{D}}^{\ast }{D}_s^{*} $$\end{document}. The mechanisms of the decay to these channels involve triangular loops and are a consequence of the internal structure of the state. Thus, the values found for the decay widths of the proposed K*(4307) are related to its nature and should be valuable for carrying on an experimental study of the K*(4307). A K* state with such a mass (in the charmonium region) and quantum numbers is a clear manifestation of an exotic meson, since, having hidden charm (i.e., a cc¯\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ c\overline{c} $$\end{document} pair), its mass and quantum numbers can not be explained within a quark-antiquark description.


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decay [23]. Similarly, in the vector sector, the latest I(J P ) = 1/2(1 − ) K * state listed in ref. [21] is the K * (1680), whose existence dates to experiments and partial wave analysis performed during 1978-1988 [24][25][26][27]. As in the case of K(1830) also, the LHCb collaboration has recently considered its existence in the analysis of the amplitude for the decay process B + → J/ψφK + [23]. And, overall, the final excited state in the meson sector, with nonzero strangeness quantum number, reported in the PDB corresponds to K(3100), whose quantum numbers are unknown, and which was observed in several Λp(Λp)+pions reactions during the years 1986-1993 [23].
In view of such a panorama, it is worth to explore whether or not there could be another family member to be added to the already known X, Y , Z families whose members will also have masses in the charmonium mass range, i.e., ∼ 3-4 GeV, but nonzero strangeness. Such states are manifestly exotic, since within a quark description, we will need at least a cc pair as well as a s quark and a light antiquark (ū,d) to account for their masses and quantum numbers. Surprisingly, although being currently accessible, the existence of such states has not been yet explored experimentally. But formation of such states has been claimed theoretically very recently using different models: in ref. [28], the DD * K system was studied by solving the Schrödinger equation and considering a pion exchange potential model to describe the interactions between the pairs forming the three-body system. As a result, a bound state with mass 4317.92 +3. 66 −4.32 MeV was obtained. Considering G-parity arguments, the authors of ref. [28] claim also the existence of a DD * K bound state with basically the same mass. In ref. [29], the DD * K system was studied by solving the Faddeev equations under the fixed center approximation [30][31][32][33][34][35][36][37]. In this case, the interaction between the particles in the two-body subsystems were obtained by solving the Bethe-Salpeter equation in coupled channels with a kernel determined from an effective field theory implementing symmetries like the chiral symmetry [38,39] or the heavy quark spin symmetry [40][41][42]. Under such an approach, the states D * s0 (2317), X(3872) and Z c (3900) are generated from the coupled channel dynamics and are mainly DK bound states in isospin 0, DD * states in isospin 0 and 1, respectively [43][44][45][46]. As a consequence of the dynamics involved, a theoretical evidence for an I(J P ) = 1/2(1 − ) K * state with a mass of (4307 ± 2) − i(9 ± 2) MeV was obtained when the DD * system clusters as X(3872) or Z c (3900).
Theoretically, the attraction in the DK and DD * subsystems, which leads to the generation of the D * s0 (2317), X(3872) and Z c (3900) states, constitutes a compelling argument in favor of the existence of such exotic K * state with a mass around 4.3 GeV and hidden charm. Experimentally, observation of such K * state should be possible in the current facilities and it would constitute an exciting novelty in the Kaonic spectroscopy and in that of the exotic mesons.
In the present work, we continue with the investigation of the properties of the K * state predicted in ref. [29] and calculate the decay widths to several open two-body channels. Particularly, we consider the channels J/ψK * (892),DD * s ,D * D * s andDD s , which are the most relevant ones, based on the nature of K * (4307). This information should be reliable for experimental searches of the K * state proposed in ref. [29], since the decay mechanism of the state is linked to the internal structure of the decaying particle. Figure 1. Decay mechanisms of the K * R state predicted in ref. [29] to the J/ψK * channel. The vertex X → J/ψρ(ω) on the diagram (b) involves yet another triangular loop, as shown in figure 3.

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Main two-body decay channels for the K * R state found in the theoretical investigation of ref. [29].

Theoretical framework
The coupled channel calculation of ref. [29] shows that the rescattering of a Kaon with the D andD * , which cluster to form X(3872) in isospin 0 and Z c (3900) in isospin 1, generates a I(J P ) = 1/2(1 − ) K * state with a mass around 4307 MeV, which is below the KDD * threshold, thus, it is a bound state. When considering the width of Z c (3900), which is around 28 MeV, a width close to 18 MeV is found for the K * (4307) state. A K * state with such an internal structure can naturally decay to three-body channels, like J/ψπK, since the state itself is obtained as a consequence of the three-body dynamics involved in the KDD * system. However, it can also decay to two-body channels. In this latter case, due to the nature found for K * (4307) in ref. [29], such a decay mechanism can proceed through triangular loops (see figure 1) and we can have as main decay channels J/ψK * (892),DD * s ,D * D * s , andDD s (see figure 2). In order to avoid confusion between K * (4307) and K * (892) and to simplify the notation, we shall, henceforth, denote the former as K * R and the latter as K * . From the results of ref. [29], the coupling of K * R to KZ c (3900) is around 4 times bigger than that to KX(3872), thus, when calculating the decay width of K * R (which is proportional to the squared coupling of K * R to KZ c or KX), the contribution arising from the diagram shown in figure 1 Figure 3. Decay mechanism of X to the J/ψρ channel in an approach in which X is obtained from the DD * interaction [47]. Figure 5. Contributions related to the diagram (a) of figure 2 for the decay mechanism K * 0 R → J/ψK * 0 .
the diagram in figure 1(a). On top of that, for the decay process K * R → J/ψK * , the vertex X → J/ψρ(ω) shown in figure 1(b) involves yet another triangular loop [47] (see figure 3) and such a vertex produces a contribution much smaller than that of the vertices Z c → J/ψπ,DD * ,D * D, since Z c (3900) couples directly to J/ψπ,DD * − c.c (where c.c means complex conjugate) [46], at the tree level. It is also interesting to notice that, with the internal structure found in ref. [29] for the predicted K * R , the decay process K * R →D * D s could also be contemplated, but it would involve a three pseudoscalar vertex (see figure 4), resulting in a null amplitude.

Determination of the vertices
Let us then start evaluating the contribution arising from the diagrams shown in figure 2. Considering the decay of a neutral K * 0 R into a J/ψ and a π 0 , we have two diagrams contributing to each of the processes shown in figure 2: in one of the diagrams, the primary vertex is K * 0 R → K 0 Z 0 c while in the other it is the vertex K * 0 → K + Z − c . We illustrate these two contributions in figure 5 for the decay process K * 0 R → J/ψK * 0 . To evaluate these diagrams, we need several vertices involving vector and pseudoscalar mesons. The contribution for the K * R → KZ c vertices in figure 5 can be written in terms of the polarization vectors µ respectively, and the coupling of K * R to the KZ c (3900) channel as where the four momenta and masses assigned to the particles are as shown in figure 6. The couplings g K * 0 c in eq. (2.1) can be obtained from the isospin 1/2 scattering matrix, T (KZc) 1 2 , determined in ref. [29]. To do this, we consider, a Breit-Wigner expression for this T -matrix in an energy region around the mass m K * R of the state, i.e., Once we have the value of g K * R →(KZc) 1 2 , the couplings g K * 0 by using the fact that where we use the phase convention |K − = −| 1 2 , − 1 2 . In this way, from eq. (2.4), (2.5) Using isospin average masses for the particles belonging to the same isospin multiplet and eq. (2.5), we can write eq. (2.1) as

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with (2.7) Next, we need the vertices Z c → J/ψ π,DD * ,D * D for different charge combinations. As shown in ref. [46], a state with mass around 3872 MeV and 30 MeV of width is generated from the dynamics present in the DD * + c.c. (c.c. means complex conjugate) and J/ψπ coupled channel system in isospin 1 and positive G-parity. This state can be related to Z c (3900) [46].
A comment regarding this latter state is here in order: the nature of Z c (3900) is still under debate. Experimental investigations seem to report two states with J P = 1 + around 3900 MeV, Z c (3900) [49][50][51] and Z c (3885) [52,53]. It is still not clear if these states are two different ones or are the same. The lattice investigations [54][55][56], on the other hand, do not seem to find an evidence for the existence of a molecular state around 3900 MeV. However, the analysis made in ref. [57] shows that the lattice data is compatible with the existence of the Z c (3900) resonance. Further, the latest experimental investigations continue to find signals of a state with mass near 3900 MeV in different processes, such as B-decays [58], η c ρ invariant mass spectra [59], etc. In spite of the debate, both experimental and theoretical investigations indicate that the DD * interaction in isospin 1, spin-parity 1 + is attractive in nature and produces a peak in the cross sections of the relevant processes. In our study, the Z c (3900) we refer to is the state arising from the DD * and coupled channel dynamics found in ref. [46].
Following the approach of ref. [46], we can write where we have defined The subscript 1 in the above equation indicates the total isospin of theDD * system. The CD D * and CD * D coefficients in eq. (2.8), which relate the Z c state to theD D * and DD * states in the charge basis, are given by where we have used the isospin phase convention |D * 0 = −| 1 2 , − 1 2 and |D 0 = −| 1 2 , − 1 2 . In case of pions, we follow the isospin phase convention |π + = −|1, 1 . In this way, C J/ψπ = 1 for the processes Z 0 c → J/ψπ 0 and Z − c → J/ψπ − .

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The couplings in eq. (2.8) can be obtained from the residue of the isospin 1 two-body scattering matrix determined in ref. [46] in the complex energy plane. We have calculated them and obtain Other vertices needed to evaluate the contribution of the diagrams shown in figure 2 are K π → K * , D * K → D s and DK → D * s . To determine these contributions, we use the effective Lagrangian L P P V [60,61] involving two pseudoscalars and a vector meson with V µ and P being matrices containing the corresponding vectors and pseudoscalar fields, respectively. The coupling g in eq. (2.12) is given by m V /(2f π ) 4.41, with m V 815 MeV being an average mass for the vector mesons ρ, ω and K * and f π = 92.4 MeV being the pion decay constant. While this value of the coupling produces a theoretical width of the K * + meson, which comes basically from the decay processes K * + → K 0 π + , K + π 0 , compatible with the experimental result, it underestimates the width of the D * + meson, obtained from the processes D * + → D 0 π + , D + π 0 . In this latter case, as shown in ref. [62], arguments based on the heavy quark symmetry establish that g → m D * g/m K * 9.9 when using the Lagrangian in eq. (2.12) for describing processes involving heavy pseudoscalar and vector mesons. Having this in mind and using eq. (2.12), we get the following amplitudes for the above mentioned vertices . In the above equations, g L = 4.41 and g H = 9.9, and the coefficients C Kπ , C KD and C KD * are given by (2.16)

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The last vertex whose contribution needs to be determined corresponds to D * K → D * s . To do this, we consider the effective Lagrangian L V V P [60,63] involving two vectors and a pseudoscalar meson where the coupling G is given by 3g 2 4π 2 fπ with g = − Mρ 2fπ = −4.14. Using eq. (2.17), we can write

Triangular loops
Once we have all the vertices associated with the decay mechanisms of K * R , we can evaluate the contributions related to the diagrams in figure 2. We start with the process shown in figure 2(a) and the two Feynman diagrams shown in figure 5 (for the K * 0 R decay). Using the vertices given in eqs. (2.1), (2.8), (2.14), the corresponding amplitude can be written as, where we have introduced the three tensor integrals I 1 α , I 2 µν , I 3 µνα , which are defined as with m 1 , m 2 and m 3 being the masses of the particles in the triangular loops shown in figure 2 (see figure 6 for the corresponding four momenta labels). Based on the Lorentz covariance, eq. (2.21) can be written in terms of the external momentum P and k. In particular, we have

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which correspond to the standard Passarino-Veltman decomposition for tensor integrals [64]. The coefficients a i j are scalars to be determined. Considering the Lorenz gauge and using P = p + k, the amplitude t a in eq. (2.20) can be further simplified to and we need to determine seven coefficients, a 1 1 , a 2 1 , a 2 3 , a 3 1 , a 3 2 , a 3 4 , and a 3 6 . To do this, the way of proceeding is: first, by using eq. (2.22), we can contract the expressions in eq. (2.22) with the different Lorentz structures present there and get a system of coupled equations which can be solved. For example, from the expression of I 1 α in eq. (2.22), we have (2.24) By solving this system of coupled equations, we can write a 1 1 as where Equation (2.25) clearly shows that the a i j coefficients depend on the mass of the decaying particle, m K * R , the masses of the particles in the loops, m 1 , m 2 and m 3 , and the masses m a and m b of the particles to which K * R can decay (see figure 6). For all the diagrams shown in figure 2, m 1 = m K and m 3 = m Zc , and for the particular case of the diagram in figure 2(a), m 2 = m π , m a = m J/ψ and m b = m K * . The next step consists in calculating the Lorentz scalar terms appearing in eq. (2.26) directly from the definition in eq. (2.21). For example, using eq. (2.21), PI 1 is given by with where we have used the rest frame of the decaying particle, for which P µ = (P 0 , 0) = (m K * R , 0) and Next, we can use Cauchy's theorem to determine the q 0 integration of eq. (2.27), and we get Similarly, we can continue with the evaluation of the other a i j coefficients of eq. (2.23). The results are given in the appendix A. Note that some of these a i j coefficients, after performing the integration on the q 0 variable, involve integrals in d 3 q which are divergent. In such a case, we regularize the corresponding integral by introducing a cutoff Λ = 700 MeV, which corresponds to the value used in ref. [29] to get the resonance K * R from the threebody KDD * system. It is also interesting to notice that for the cases in which the d 3 q integration does not involve divergences, the upper limit for such integration is also naturally provided [65], in this case, by the value of the cut-off used when regularizing the two-body loops involved in the generation of the Z c state from the interaction of DD * and coupled channels, and which is also ∼700 MeV [46].
Let us consider now the decay mechanism shown in figure 2(b) and the two Feynman diagrams contributing to it, which are shown in figure 7. In this case, considering eqs. (2.1), (2.8) and (2.18), the amplitude describing the process is given by where the Lorenz gauge and the antisymmetric properties of the Levi-Civita tensor have been used to get the last line. Using the decomposition in eq. (2.22) and considering once again the antisymmetric properties of the Levi-Civita tensor, eq. (2.31) can be written as where the coefficient a 1 1 can be obtained from eq. (2.25), where now, from figure 2(b), m 3 = m D * , m a = mD, m b = m D * s , and the expression for a 2 1 can be found in the appendix A. Next, we continue with the evaluation of the process depicted in figure 2(c). In this case, considering the diagrams shown in figure 8 and using the results in eqs. (2.1), (2.8), (2.14), the amplitude associated with such decay mechanism reads as Note that the above expression is analogous (up to a phase) to the expression of t a in eq. (2.20) changing g L → g H , J/ψ →D * , π → D, K * → D * s in the couplings and in the products of four momenta, i.e., we have now m 2 = m D (instead of m π ), m a = mD * (instead of m J/ψ ) and m b = m D * s (instead of m K * ). This result is expected since we are, basically, changing a light pseudoscalar (the pion) by a heavy pseudoscalar (the D meson) and light vector mesons (J/ψ and K * ) by heavy ones (D * and D * s respectively). At last, considering the vertices in eqs. (2.1), (2.8), (2.14) and the diagrams in figure 9, we get the following amplitude for the description of the process shown in figure 2(d), . Using the Lorenz gauge, we can write eq. (2.34) as .
We could proceed as in the previous cases and use the Lorentz covariance to write the tensor integrals in terms of the possible Lorentz structures and some a i j coefficients. However, the presence of the tensor integrals I µαβσ 4 and I µαβσλ 5 makes such a method inconvenient, since many different Lorentz structures would appear. We adopt then a different strategy: although the particles in the triangular loop are off-shell, their interactions give rise to the K * R and Z c states. In such a situation, the momenta associated with the particles generating such states are much smaller as compared to their energies. In this way, the temporal component of the polarization vector (of the order momentum/mass) is negligible as compared to the spatial components. Thus, when summing over the internal polarizations of the particles, if we call Q µ and m the four-momentum and mass, respectively, of the vector meson whose interaction with the corresponding pseudoscalar generates K * R or Z c , with i and j being spatial indices. Considering such an approach, the amplitude in eq. (2.34) can be written as

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where I 0 is given by eq. (2.21) (with m 1 = m K , m 2 = m D * and m 3 = m Zc ) and (2.37) Note that the approach shown in eq. (2.35) could have also been used when calculating the amplitudes in the diagrams depicted in figure 2(a)-(c). There, however, such an approach would not lead to a significant simplification in the calculations, and we have not implemented it. In any case, for completeness, in section 3, we discuss the validity of such an approach by comparing the results obtained with and without the substitution of eq. (2.35) for the diagram shown in figure 2(a). The next step to get t d consists in performing the q 0 integration in eq. (2.37). The details of this integration are given in the appendix A. After that, since in the rest frame of the decaying particle P = 0, the integral in eq. (2.37) is a function of k. In such a case, to perform the integration in d 3 q, it is more convenient to introduce the dot product between q and k, which can be done by replacing (2.38)

Results and discussion
The decay width of the K * R state to the two-body channels shown in figure 2 can be obtained from the amplitudes determined in the previous section as where the index i = a, b, c, d is associated with the processes shown in figure 2  It is interesting to notice that the process depicted in figure 2(b) involves an anomalous vertex [66,67], the D * D * s K vertex, whose contribution is given by the Lagrangian in eq. (2.17). It is sometimes argued that processes involving anomalous vertices should give smaller contributions that those in which no anomalous vertices are involved. However, the importance of the anomalous vertices in different contexts, like in the determination of production and absorption cross sections of several processes, calculation of radiative decays of scalar and axial resonances and kaon photo-production, has been shown [68][69][70][71][72][73][74][75].
In the present work, as can be seen, the decay width found for theDD * s channel, which,

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as stated above, involves an anomalous vertex, is comparable to the result obtained for theD * D * s channel, which does not involve anomalous vertices, but has smaller phase space thanDD * s . We can study the sensitivity of the results to the cut-off used when regularizing the integrals appearing in the a i j coefficients of eqs. (2.23), (2.32), (2.33), (2.36). Changing Λ in the range 700-800 MeV, we get the following values for the decay widths Γ a = 6.97 ± 0.27 MeV, Γ b = 0.54 ± 0.08 MeV, Γ c = 0.54 ± 0.07 MeV, Γ d = 1.14 ± 0.17 MeV. (3.3) We can also study the uncertainty produced in the results under changes in the coupling constant of K * R → KZ c . If we allow a variation of ±1% in this coupling, for a fixed cut-off Λ = 700 MeV, we get Γ a = 6.71 ± 0.14 MeV, Γ b = 0.47 ± 0.02 MeV, In case of the diagram shown in figure 2(a), when calculating the decay width of K * R → J/ψK * , we can also consider the fact that the K * meson has a width Γ K * ∼ 47 MeV from its decay to the Kπ channel. This can be done by convoluting the expression in eq. (3.1) with the spectral function associated with the K * meson, in which case the expression for Γ a (m 2 ) in eq. (3.5) is given by eq. (3.1), and Note, however, that since the mass of the K * R resonance is far from the J/ψK * threshold, even when the width of K * is taken into account, a significant change in the results is not expected. We indeed find almost the same value for the decay width Γ a .
It is also interesting to establish the validity of the approach in eq. (2.35). If we would have considered such an approach when determining the amplitude in eq. (2.20), the terms related to the coefficients different to a 1 1 would have vanished. In such a case, we would have got for Γ a the value of 6.66 MeV instead of the result in eq. (3.2). This clearly shows that the approach in eq. (2.35) is, in fact, reliable.

JHEP05(2019)103 4 Conclusion
In this work we have calculated the decay width of the K * (4307) predicted in ref. [29] to the two-body channels J/ψK * ,DD * s ,D * D * s andDD s . These channels, as well as the decay mechanism, are related to the internal structure of the proposed K * (4307), which, as found in ref. [29], corresponds to a KDD * system in which the DD * subsystem clusters as X(3872) or Z c (3900). The possible formation of vector meson resonances with strangeness at the charmonium energy region has been, so far, unexplored. The mass and quantum numbers of the state invoke a clear non quark-antiquark structure for it. The results presented in this work constitute a prediction for the decay properties of this K * (4307) and should serve as a motivation for conducting experimental investigations of this state.
A Determination of the a i j coefficients involved in the triangular loops depicted in figure 2 In this appendix we give the details of the calculation of the a i j coefficients appearing in eqs. (2.20), (2.32), (2.33), which are related to the Lorentz decomposition of eq. (2.22), and to determine eq. (2.37). By contracting I 1 α , I 2 µα and I 3 µνα with the corresponding Lorentz structures, we can get a set of coupled equations whose solution, in each case, allow us to write the a i j coefficients in terms of scalar integrals. We obtain (the expression for the a 1 1 coefficient can be found in eq. (2.25) but, for convenience, we write it here again)

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× k 2 P 2 +2(P ·k) 2 GKI 3 −5k 4 (P ·k)PPPI 3 +3k 2 k 2 P 2 +4(P ·k) 2 PPKI 3 +P 2 k 2 P 2 +4(P ·k) 2 KKKI 3 −3(P ·k) 3k 2 P 2 +2(P ·k) 2 KKPI 3 , where, Note that the a i j coefficients in eq. (A.1) and the scalars in eq. (A.2) depend on the masses m 1 , m 2 and m 3 of the particles involved in the triangular loop as well as of the mass of the K * R state and the masses of the particles to which it can decay, which we represent by m a and m b (see figure 6).