# Charmless Quasi-Two-BodyB Decays in Perturbative QCD Approach: Taking B⟶KR⟶K+K− as Examples

Authors: Wen-Feng Liu; Zhi-Tian Zou; Ying Li
Journal: Advances in High Energy Physics
 (2022)

---

## Abstract

Three-bodyB decays not only significantly broaden the study of B meson decay mechanisms but also provide information of resonant particles. Because of complicate dynamics, it is very hard for us to study the whole phase space in a specific approach. In this review, we take B⟶KR⟶K+K− decays as examples and show the application of the perturbative QCD (PQCD) approach in studying the quasi-two-body B decays, where two particles move collinearly with large energy and the bachelor one recoils back. To describe the dynamics of two collinear particles, the S, P, and D-wave functions of kaon-pair with different waves are introduced. By keeping the transverse momenta, all possible diagrams including the hard spectator diagrams and annihilation ones can be calculated in PQCD approach. Most results are well consistent with the current measurements from BaBar, Belle, and LHCb experiments. Moreover, under the narrow-width approximation, we can extract the branching fractions of the two-body decays involving the resonant states and also predict the branching fractions of the corresponding quasi-two-body decays B⟶KR⟶π+π−. All predictions are expected to be tested in the ongoing LHCb and Belle-II experiments.


---

## Body

## 1. Introduction

It is well known thatB meson hadronic decays provide us unique information on three fronts: CP violation and the angles of the CKM matrix, the structure of QCD in the presence of heavy quarks and energetic light particles, and new particles beyond the standard model (SM) physics in the quark sector. In past twenty years, experimental information on nonleptonic B decays has been collected progressively, at CLEO, two B-factories BaBar and Belle [1], the Tevatron, and currently at the LHC, most prominently at LHCb [2]. In addition, the running Belle-II also includes serious plans for analyses of nonleptonic B decays [3] with higher precision. Because of large combinatoric backgrounds, studies of charmless B decays have concentrated mainly on two-body decay processes. Although with complex kinematics, three-body decays could not only significantly broaden the study of B meson decay mechanisms and provide additional possibilities for direct CP violation searches but also provide information of resonant particles. In past decades, more and more analyses of three-body decays have been performed by the BaBar, Belle, CLEO, and LHCb, and the branching fractions and CP violations have been measured with high precision. Motivated by the accumulated experimental results, many theoretical studies of various three-body B hadronic decays have been performed in different frameworks, such as approaches based on the symmetry principles [4–8], the QCD factorization (QCDF) [9–19], the perturbative QCD (PQCD) approach [20–28], and other theoretical methods [29–31].Differing from the two-bodyB decays where the kinematics is fixed, the momentum of each final state in three-body decays is variable. Moreover, both resonant and nonresonant contributions are involved; therefore, how to disentangle the resonant and nonresonant contributions reliably is also very important in studying the multibody decays. For clarity, we define the kinematics of the three-body decay as
(1)BpB⟶Map1Mbp2Mcp3.It is customary to take these variables as two invariant masses of two pairs of final-state particles:(2)m122=p1+p22,m132=p1+p32.Thus, the amplitude of the three-body decay is a function of the two kinematic variables,m122 and m132, and the corresponding distribution in the phase-space region is called a Dalitz plot, which can be divided in different regions with characteristic kinematics, as shown in Figure 1. As usual, we refer to the B-meson rest frame. In the centre of the Dalitz plot, the three final-state particles almost have a large energy (E~mB/3) and none of them flies collinearly to any others. The corners imply that one final particle is approximately at rest, and the other two fly back-to-back energetically, leading to that one invariant mass is large, and the other two are small. Specially, the central part of the edges means that two particles move collinearly with large energy and the other particle recoils back. In the naive factorization, the contribution at the centre of the Dalitz plot is viewed to be both power suppressed and αs suppressed with respect to that at the edge, because two hard gluons are needed. However, recent studies based on QCD factorization showed that the power corrections are large, which means that the centre region maybe as important as the regions at the edge [10, 11]. Assuming that these different regions can be well described by the respective calculations, it is a very challenging work to determine how well these descriptions merge at intermediate kinematical regimes. So, the theory of three-body nonleptonic decays is still in an early stage of development.Figure 1
Phase space of the three-body decayB−⟶K+K−π− in terms of the invariants m12 and m13 [32].In the past decades, theB meson two-body hadronic decays have been explored systematically in the context of QCD factorization, soft-collinear effective theory, or PQCD approach. It is natural to ask if the accumulated experience can be used to study the multibody B decays. Inspired by this, we paid much attention to the edge regions of the Dalitz plot, in which the two energetic particles are collinear and form a moving-fast meson-pair, and the interactions between the meson-pair and the bachelor particle are power suppressed naturally. This kind of process is also called quasi-two-body process. The interactions in the meson-pair can be absorbed into the two-meson wave function. In this case, the obvious generalization of the factorization theorem for two-body decays applies. It is reasonable for us to assume the validity of the factorization for these quasi-two-body B decays. In the PQCD framework that is based on the kT factorization, the decay amplitude of quasi-two-body B decays can be decomposed as the convolution [33].
(3)AB⟶M3R⟶M1M2=Ct⊗ΦB⊗H⊗ΦM1M2⊗ΦM3⊗exp−St,where the ΦB and ΦM3 are the wave functions of B meson and the light bachelor meson, respectively. The newly introduced ΦM1M2 is the two-meson wave function, which describes how four quarks are combined into two mesons. It should be emphasized that both resonant and nonresonant contributions to the hadron-pair system are included into the wave function. The Wilson coefficient Ct covers all physics above mb scale. The exponential term is the so-called Sudakov form factor caused by the additional scale introduced by the intrinsic transverse momenta kT, which suppresses the soft dynamics effectively. The hard kernel H for the b quark decay, similar to the two-body case, starts with the diagrams of single hard gluon exchange, and it can be calculated perturbatively.In the following, we will takeB⟶KR⟶K+K− decay as examples to show how to study quasi-two-body processes in the PQCD approach at leading order, where K+K−-pair move collinearly and combine into resonances with different waves, such as f0980, ϕ1020, and f2′1525. In Section 2, we will introduce the definitions of the two-kaon wave functions with different waves and present the typical Feynman diagrams in PQCD. In Section 3, the numerical results and discussions will be given. At last, we summarize this review in Section 4.


## 2. Framework

In the quasi-two-body region of phase space, the Dalitz plot analysis allows one to describe the decay amplitude in the isobar model, where the decay amplitude is represented by a coherent sum of amplitudes fromN individual decay channels with different resonances,
(4)A=∑j=1NcjAj,where the Aj is the amplitude corresponding to certain resonance and cj is the complex coefficient describing the relevant magnitude and phase of the different decay channel.When we calculate the amplitudeAj in PQCD, the most important inputs are the nonperturbative wave functions. For the decay B0⟶K0R⟶K+K−, the wave functions of the B meson and the bachelor meson K0 have been well determined by comparing the theoretical predictions with those well-measured experimental data of the two-body B decays. For the sake of brevity, we shall not discuss them anymore, and their explicit expressions can be found in refs. [34–36]. As aforementioned, in the quasi-two-body decays, the newly introduced ingredient is the two-meson wave function corresponding to different resonances with different spin [22].We firstly discuss theS-wave two-meson wave function of the kaon-pair,
(5)ΦKK,S=12NcPϕSz,ζ,ω2+ωϕSsz,ζ,ω2+ωnv−1ϕStz,ζ,ω2,where z is the momentum fraction of the spectator quark and ζ is the momentum fraction of one kaon in the pair. Nc=3 is the number of colors, and ω and P are the invariant mass and momentum of the kaon-pair, respectively. n=1,0,0T and v=0,1,0T are two dimensionless vectors. The ϕS, ϕSs, ϕSt, are the twist-2 and twist-3 distribution amplitudes, and they are parameterized as [37]
(6)ϕSz,ζ,ω2=92NcFSω2aSz1−z2z−1,(7)ϕSsz,ζ,ω2=122NcFSω2,(8)ϕStz,ζ,ω2=122NcFSω21−2z.The Gegenbauer momentaS=−0.8 is determined with the experimental data [38]. We have to adopt the asymptotic form within the SU(3) symmetry, as the reliable theoretical studies are still absent.Specially, the functionFSω2 is the S-wave time-like form factor, which contains the interactions between the two kaons in the kaon-pair. For most resonances, the form factors are usually taken to be relativistic Breit-Wigner (RBW) line shapes [39]
(9)FSω2=mj2mj2−ω2−imjΓjω,where mj is the mass of the resonance and Γω is the mass-dependent width [39, 40]. However, the case of f0980 is complicated. Because there is an anomalous structure corresponding to the enhancement from the KK system found around 980 MeV in the π+π- scattering [41, 42], it can be interpreted as a two-channel resonance combining the ππ and KK channels. In order to include these effects, Equation (9) is modified to the Flatté form [43–45] as
(10)FSω2=mf09802mf09802−ω2−imf0980gππρππ+gKKρKKFKK2,where gππ and gKK are the f0980 coupling constants to the ππ and KK final states, respectively. The phase space factors ρππ and ρKK are given as
(11)ρππ=1−4mπ2ω2,ρKK=1−4mK2ω2.The factorFKK=e−αq2 with α≈2.0GeV−2 is introduced to suppress the KK¯ contribution [45], q being the momentum of each kaon in the KK¯ rest frame.It should be noted that we only consider the contributions from three scalar resonancesf0980, f01500, and f01710, which have been well analyzed by BaBar experiments [38, 46]. The coefficients of the coherence summation of these three resonances in Equation (4) are set to be cf0980=2.9, cf01500=1.0, and cf01710=0.5, which have been determined by the experimental measurements already [38, 46].Next, we come to theP-wave two-kaon wave function. Because the third bachelor kaon in B0⟶K0K+K− decay is a pseudoscalar one, therefore only the longitudinal part contributes, and its form can be expressed as
(12)ΦKK,P=12NcPϕPz,ζ,ω+ωϕPsz,ζ,ω+p1p2−p2p1ω2ζ−1ϕPtz,ζ,ω,where p12 is the momentum of each kaon in the KK¯-pair. The corresponding twist-2 and twist-3 distribution amplitudes that can be decomposed as Gegenbauer polynomials are given as
(13)ϕP0z,ζ,ω=3FP∥ω22Ncz1−z1+aP0C23/22z−12ζ−1,(14)ϕPsz,ζ,ω=3FP⊥ω222Nc1−2z1+aPs1−10z+10z22ζ−1,(15)ϕPtz,ζ,ω=3FP⊥ω222Nc2z−121+aPtC23/22z−12ζ−1,with aP0=−0.6, aPs=−0.8, and aPt=−0.3. Similarly, the P-wave time-like form factor FP∥ω2 is also taken to be the RBW line shape in Equation (9). As for FP⊥ω2, the relation [47]
(16)FP∥ω2FP⊥ω2≈fVfVT,will be used, where fV and fVT are the vector and tensor decay constants.At last, we will discuss the wave function ofD-wave kaon-pair in which the information of tensor meson resonances is included. In previous studies of B meson decays involving a tensor [48, 49], it is found that the polarization components ±2 of tensor meson do not contribute of the amplitudes, due to the conservation of the angular momentum. Hence, the form of D-wave two-kaon wave function is the same as that of the P-wave,
(17)ΦKK,D=12NcPϕDz,ζ,ω+ωϕDsz,ζ,ω+p1p2−p2p1ω2ζ−1ϕDtz,ζ,ω.The distribution amplitudes are given as(18)ϕDz,ζ,ω=239FD∥ω22Ncz1−zaD02z−1P2ζ,(19)ϕDsz,ζ,ω=−239FD⊥ω242NcaD01−6z+6z2P2ζ,(20)ϕDtz,ζ,ω=239FD⊥ω242NcaD02z−11−6z+6z2P2ζ,with aD0=0.6 and P2ζ=1−6ζ+6ζ2. Likewise, we use the RBW line shape for describing the time-like form factor FD∥ and determine the FD⊥ by the similar relation as Equation (16).According to the effective Hamiltonian ofb quark decay, we can draw the possible Feynman diagrams as shown in Figure 2. In diagram (a), the spectator quark enters to the bachelor particle, and the KK-pair is emitted. In order to make the spectator quark from soft to hard, the hard gluon is needed, and it can come from any quark participating in the four-quark weak interaction. So, with three wave functions, we could calculate amplitude with different operators in the PQCD approach. In practice, we keep the transverse momenta of each quark for smearing the end-point singularities.Figure 2
Typical Feynman diagrams for the quasi-two-body decayB⟶KR⟶K+K− in PQCD, where the black squares stand for the weak vertices, large (purple) spots on the quark lines denote possible attachments of hard gluons, the green ellipse represents kaon-pair, and the red one is the light bachelor K meson [20].
(a)(b)(c)(d)For decaysB±⟶K±R⟶K+K−, the spectator quark can also enter into the recoiled meson pair, as shown in diagram (b). Besides these two kinds of contributions, the annihilation diagrams (c) and (d) also play important roles, which can be calculated quantitatively without introducing new parameters. Due to the space limit, we cannot list all amplitudes of these diagrams, and one can find them in ref. [20].


## 3. Results and Discussions

With the calculated amplitudeA, we then obtain the differential branching fraction
(21)d2Bdζdω=τBωp⟶1p⟶332π3mB3A2,where τB is the lifetime of the B meson. The magnitudes of three momenta of one kaon and the bachelor particle in the rest frame of the KK-pair are given by
(22)∣p⟶1∣=λω2,mK2,mK22ω,p⟶3=λmB2,mK2,ω22ω,with the standard Källén function λa,b,c=a2+b2+c2−2ab+ac+bc.Integrating out the variablesζ and ω, we could obtain the branching fractions of the quasi-two-body decays B⟶KR⟶K+K−, and the CP averaged branching fractions are presented in Table 1. As aforementioned, the theoretical studies of multibody B hadronic decays are on the early stage, so there are many uncertainties in our calculations. The first and foremost parameters uncertainties are from nonperturbative parameters, including the shape parameter in the heavy B wave function, the Gegenbauer moments in the distribution amplitudes of kaon-pair and kaon. We call for the results with higher precision from nonperturbative approaches, such as QCD sum rules and lattice QCD. The second uncertainties originated from the PQCD approach itself, including the unknown QCD radiative corrections and the power corrections. Although some higher order and higher power corrections have been explored, the complete calculations are still in absence. The last kind of uncertainties is caused by the CKM matrix elements. In the table, the currently available experimental measurements are also given for comparison. It is obvious that within the uncertainties, most of our results are in good agreement with experimental results, except decay mode B0⟶K0f01710⟶K+K−.Table 1
CP averaged branching fractions (in 10−6) of B⟶KR⟶K+K− decays in PQCD [20] together with experimental data [39].
Decay modesPQCDEXP [39]B+⟶K+ϕ1020⟶K+K−3.81−1.03−0.33−0.00+1.44+0.64+0.274.48±0.22−0.24+0.33B+⟶K+f0980⟶K+K−10.13−4.38−2.44−0.00+5.60+2.22+0.719.4±1.6±2.8B+⟶K+f01500⟶K+K−0.60−0.24−0.06−0.02+0.24+0.07+0.050.74±0.18±0.52B+⟶K+f01710⟶K+K−1.64−0.70−0.46−0.02+0.89+0.42+0.081.12±0.25±0.50B+⟶K+f2′1525⟶K+K−0.68−0.29−0.14−0.00+0.37+0.13+0.070.69±0.16±0.13B+⟶K+f22010⟶K+K−1.18−0.50−0.19−0.00+0.65+0.26+0.12B0⟶K0ϕ1020⟶K+K−3.22−0.98−0.18−0.08+1.36+0.48+0.183.48±0.28−0.14+0.21B0⟶K0f0980⟶K+K−9.10−3.89−2.11−0.00+5.12+2.19+0.697.0−1.8+2.6±2.4B0⟶K0f01500⟶K+K−0.57−0.22−0.15−0.00+0.26+0.09+0.040.57−0.19+0.25±0.12B0⟶K0f01710⟶K+K−1.48−0.63−0.42−0.00+0.82+0.39+0.114.4±0.7±0.5B0⟶K0f2′1525⟶K+K−0.58−0.27−0.13−0.01+0.31+0.12+0.050.13−0.08+0.12±0.16B0⟶K0f22010⟶K+K−1.09−0.48−0.23−0.00+0.57+0.26+0.11In Figure3, we show the K+K− invariant mass-dependent differential branching fractions for the quasi-two-body decays B0⟶K0ϕ1020⟶K+K−. It can be seen that the contribution of ϕ1020 is dominate in the region near 1 GeV. Under the narrow-width approximation, the three-body decay and corresponding two-body one satisfy the relation
(23)BB⟶P3R⟶P1P2≈BB⟶P3R×BR⟶P1P2,with R being the resonance. With the experimental results Bϕ⟶K+K−=49.2±0.5% [39], we obtain BB0⟶K0ϕ=6.4−2.0+2.9×10−6, which is in agreement with above experimental results with uncertainties.Figure 3
Theω-dependence of differential branching fractions for the B0⟶K0K+K− decay [20].Although the conventional quark model has achieved great success, the quark structures of scalar particles are still quite controversial, especially for the light scalar ones. Although there are many hints that the light scalars are four-quark states, the wave functions of these particles have not established, and we left it as our future work. Currently, we here still regardf0980 as a two-quark structure. Many experimental evidences indicate that both ss¯ and qq¯ are involved in the f0980, so the mixing form is supposed to be
(24)f0980=qq¯sinθ+ss¯cosθ,with qq¯=uu¯+dd¯/2 and the mixing angle θ=40° [50]. For the heavier scalar mesons, there are glueball contents in isosinglet scalar mesons f01370, f01500, and f01710. It is commonly accepted that f01710 is dominated by the scalar glueball, while f01500 is an approximately SU(3) octet with negligible glueball component. So, the glueball content of f01500 can be neglected.In Figure4, we show the dependencies of the differential branching ratios dBB+⟶K+R⟶K+K−/dω on the kaon-pair invariant mass ω with the S-wave resonances f0980, f01500, and f01710 and the D-wave particles f2′1525 and f22010. From the figure, it is obvious that the f0980 production is apparently dominant, and it is about ten times larger than that of f01710. In fact, it has been shown that within present experimental and theoretical uncertainties, the narrow peak at 980 MeV in the KK¯ system may be interpreted as a cusp phenomenon with large width and does not necessarily imply that there exists a narrow resonance in that region. Because of large width, the contribution of the tail of f0980 is still larger than the total effect of f01500. We also find that the contributions of f01710 and f01500 overlap with each other, so that it is very hard for us to disentangle two resonances at the region about 1.5 GeV. Unlike S-wave, the contributions from D-wave resonances do not overlap anymore because of the narrow width of f2′1525. As for the f21270, although there are some studies on it [51], the mixing between different quark components is quit complicated, so its contribution has not been included.Figure 4
Theω-dependence of differential branching fractions from f0980, f01500, f01710, f2′1525, and f22010 for the B0⟶K0K+K− decay [20].As aforementioned, the narrow-width approximation is invalid in describing the scalar particlef0980, but it still holds in the processes B⟶Kf01500⟶K+K−. Again, we could obtain the branching fractions of B⟶Kf01500 as
(25)BB0⟶K0f01500=13.7±6.1×10−6,(26)BB+⟶K+f01500=13.9±5.8×10−6,within Bf01500⟶K+K−≃4.3%. For the decay B0⟶K0f01500, our result agrees with experimental data 1.3−0.6+0.7×10−5 [39]. As for the decay B+⟶K+f01500, the centre value of prediction is about 3.7 times larger than that averaged experimental data 3.7±2.2×10−6 [39], but both theoretical and experimental uncertainties are very larger.Under the narrow-width approximation, we get a ratio as(27)R1=Bf01500⟶K+K−Bf01500⟶π+π−≈BB⟶Kf01500⟶K+K−BB⟶Kf01500⟶π+π−.Using the experimental dataBf01500⟶K+K−=4.3% and Bf01500⟶π+π−=23.27% [39], we can get the fraction R1=0.185. Thereby, the branching fractions of B⟶Kf01500⟶π+π− decays are estimated to be
(28)BB+⟶K+f01500⟶π+π−=3.24±1.35×10−6,(29)BB0⟶K0f01500⟶π+π−=3.15±1.40×10−6.Similarly, we also define another ratio as(30)R2=Bf01710⟶K+K−Bf01710⟶π+π−≈BB⟶Kf01710⟶K+K−BB⟶Kf01710⟶π+π−.With the experimental resultΓf01710⟶ππ/Γf01710⟶KK¯=0.23±0.05 [39], we then predict the branching fractions of B⟶Kf01710⟶π+π− decays as
(31)BB+⟶K+f01710⟶π+π−=5.0−3.4+3.9×10−7,BB0⟶K0f01710⟶π+π−=4.5−3.4+3.9×10−7.All above predictions are expected to be measured in LHCb and Belle-II experiments.


## 4. Summary

In this review, we tookB⟶KR⟶K+K− decays as examples and showed the application of PQCD in studying the quasi-two-body B decays. In this approach, we here only discussed the region at the central part of the edges, where two particles move collinearly with large energy and the other particle recoils back. In order to describe the dynamics of two collinear particles, the wave functions of kaon-pair with different spins are introduced. By keeping the transverse momenta, all possible diagrams at leading order were calculated, including the hard spectator diagrams and annihilation ones. Most of our numerical results are well consistent with the current experimental data. Under the narrow-width approximation, we extracted the branching fractions of the corresponding two-body decays involving the resonances, such as the B⟶Kϕ, whose branching fractions agree with the current experimental data well. We also predicted the branching fractions of the corresponding quasi-two-body decays B⟶KR⟶π+π−. All predictions are expected to be tested in the ongoing LHCb and Belle-II experiments.



---

*Source: 5287693-2022-02-22.xml*