Doubly-charged scalar in four-body decays of neutral flavored mesons

In a previous paper [1], we studied the lepton number violation decays of the ${B}_{c}^{-}$ meson induced by a doubly-charged Higgs boson. There are both experimental and theoretical motivations to study this kind of particle. Although the Higgs boson has been found, whether it is the one predicted by the Standard Model still needs more confirmation. It is possible that an extended Higgs sector exists, and that there are additional isospin multiplet scalar fields. For example, theSU(2)_Ltriplet scalar, which contains a doubly-charged component, is introduced to generate small neutrino mass in the Type-Ⅱ seesaw modes [2-5]. Generally, such a triplet representation is needed in the left-right symmetric models [6-8] to break the extendedSU(2)_L×SU(2)_R×U(1)_B−Lsymmetry in the Standard Model. The doubly-charged scalar also appears in other models, such as little Higgs models [9] and Georgi-Machacek model [10]. As it can decay into two leptons with the same charge, indicating lepton number violation, such processes for top quark,τ⁻[11], and charged mesons, such asK⁻,D⁻, ${D}_{s}^{-}$ ,B⁻[12-15] have been investigated extensively. As the lower bound of the mass of the doubly-doubly charged Higgs boson is around 800 GeV [16,17], these low energy processes have extremely small branching ratios. Although it is not likely that these channels will be detected soon, as experiments collect more data, the upper limits of the branching ratios for such decay processes will become more stringent. One can also use them to derive further constraints for the effective short-range interactions [18].

In Ref. [1], we considered both the three-body and four-body decay channels of ${B}_{c}^{-}$ meson, in which the lepton number is not conserved. In this paper, we investigate the lepton number violation processes of the neutral flavored mesons induced by the doubly-charged Higgs boson. Contrary to the charged meson case, where the annihilation-type diagram and the twoWmeson emitting diagram both contribute to the amplitude, in the case of the neutral meson, the light antiquark is just a spectator (seeFig. 1). Theoretically, this makes the calculation simpler, as there is no complexity brought by the cascade decay. As for the decay products, the two leptons have the same charge, and so do the two mesons. These decay modes have no equivalent in the Standard Model, which makes them also interesting experimentally.

Figure 1.Feynman diagrams of the decay processes $h\to {h}_{1}{h}_{2}{l}_{1}^{-}{l}_{2}^{-}$ .

These channels can also be induced by Majorana-type neutrinos. Their Feynman diagrams are similar toFig. 1, but theschannels should be replaced bytchannels. If the neutrino mass were around GeV, it could be produced on-shell, which has attracted much attention [19-22]. For the cases when the neutrino mass is very small or very large, the branching ratios will have the same order of magnitude as in the case of the doubly-charged Higgs boson [15,23]. Therefore, the theoretical analysis of the low energy processes induced by the doubly-charged Higgs boson also provides a useful complement to the Majorana neutrino scenario.

This paper is organized as follows. In Sec. 2, we give the Lagrangian which describes the couplings between the Higgs triplet and the Standard Model particles, and present the amplitudes and phase space integrals. In Sec. 3, we give the branching ratios of all decay channels and compare the results forD⁰with experimental data. We summarize our results in the last section. Some details of the meson wave functions are presented in the Appendix.

The hypothetical Higgs triplet Δ in the 2 × 2 representation is defined as [12]

It mixes with the usualSU(2)_LHiggs doublet by a mixing angleθ_Δ, from which we defines_Δ= sinθ_Δandc_Δ= cosθ_Δ.

The Lagrangian which describes the interaction between Δ andW⁻gauge boson or SM fermions has the following form [12,15]

whereC=iγ²γ⁰is the charge conjugation matrix;ψ_iLrepresents the leptonic doublet;h_ijis the leptonic Yukawa coupling constant;gis the weak coupling constant. The third and fourth terms represent the interactions between the singly-charged boson and the other particles. Compared with the second term, their contributions can be neglected.

Ifq=q₃, all four diagrams inFig. 1contribute to the decay:

where the factor $\displaystyle \frac{1}{3}$ in ${ {\mathcal M} }_{B}$ and ${ {\mathcal M} }_{D}$ is introduced by the Fierz transformation; ⟨lepton⟩ is the leptonic part of the transition matrix element;V_qiqjis the Cabibbo-Kobayashi-Maskawa matrix element. The definition of the decay constantf_h1of a pseudoscalar meson

is used. For vector mesons, it should be replaced by

The values of the decay constants are given inTable 1. It should be pointed out that we have used the factorization assumption in Eqs. (3)-(6), which is not quite appropriate when both final mesons are light. However, as only the order of magnitude is important in such processes, we anticipate that the effects of nonfactorization and final meson interactions do not change the results significantly.

Finally, we get the transition amplitude

Ifq≠q₃, onlyFig. 1(a)and(b)contribute:

The hadronic transition matrix can be expressed as [27]

whereh₁is a pseudoscalar meson, andf₊andf₋are form factors. Ifh₁is a vector meson, we have

wheref_Vandf_i(i= 0, 1, 2) are form factors;MandM₁are the masses of corresponding mesons; the definitionQ=p−p₁is used.

By applying the Bethe-Salpeter method with the instantaneous approximation [28], the hadronic matrix element is written as

whereφ⁺⁺is the positive energy part of the wave function; $\overrightarrow{q}$ and ${\overrightarrow{q}}_{1}$ are the relative three-momenta between the quarks and antiquarks in the initial and final mesons, respectively.

The partial decay width is obtained by evaluating the phase space integral

where

We also use the definitionss₁₂= (p₁+p₂)²ands₃₄= (p₃+p₄)². The meanings ofθ₁₂,θ₃₄, andϕare shown inFig. 2.δ_l1l2is 1 ifl₁andl₂are identical particles, otherwise it is 0. The same is true forδ_h1h2. The integral limits are

Figure 2.Kinematics of the four-body decay ofhin its rest frame.P₁andP₂are respectively the momenta ofh₁andh₂in their center-of-momentum frame;P₃andP₄are respectively the momenta ofl₁andl₂in their center-of-momentum frame.

whereM₂,m₁, andm₂are the masses ofh₂,l₁, andl₂, respectively.

The Bethe-Salpeter method has certain advantages when calculating the form factors, especially in the case when both initial and final mesons are heavy. In the first step, the wave functions of the mesons, which include relativistic corrections, are obtained by solving numerically the corresponding instantaneous Bethe-Salpeter equation. Their pole structure is important for describing the properties of heavy mesons. Subsequently, the form factors for the physically allowed region are calculated using Eq. (13) without any analytic extension. Although the instantaneous approximation is reasonable for the double heavy mesons and acceptable for the heavy-light mesons, it results in large errors for the light mesons, such asπandK. For example, when we change the parameters by ±5%, the form factors atQ²= 0 for the channels with heavy mesons change by less than 10%, while for those withπorK, the errors can be larger than 50%. For processes with light mesons, such asB→π(ρ), other methods are more appropriate, for example the light-cone sum rules. Nevertheless, we use this approximation also for the light mesons as the decay channels we consider are related to new physics, for which the branching ratios are expected to be very small, and only the order of magnitude is important.

The parameters of the doubly-charged Higgs boson have no definite values at present, only the lower or upper limits from experiments are available. For example, the latest results of the ATLAS and CMS Collaborations [16,17] show that the mass of Δ⁺⁺is larger than 800 GeV. From Ref. [12], the upper limit fors_Δis 0.0056. The constraints for the couplingh_eecan be extracted from thee⁺e⁻annihilation process [29]: $\displaystyle \frac{{h}_{ee}^{2}}{{m}_{\Delta }^{2}}\le 9.7\times {10}^{-6}\ {{\rm{GeV}}}^{-2}$ . Forh_μμ, the Muong− 2 experiment provides the limit [30]: $\displaystyle \frac{{h}_{\mu \mu }^{2}}{{m}_{\Delta }^{2}}\le 3.4\times {10}^{-6}\ {{\rm{GeV}}}^{-2}$ . Theh_eμis related toμ⁻→e⁻e⁺e⁻andμ⁻→e⁻γprocesses [12], which give $\displaystyle \frac{{h}_{e\mu }{h}_{ee}}{{m}_{\Delta }^{2}}\le 3.2\times {10}^{-11}\ {{\rm{GeV}}}^{-2}$ and $\displaystyle \frac{{h}_{e\mu }{h}_{\mu \mu }}{{m}_{\Delta }^{2}}\le 2.0\times {10}^{-10}\ {{\rm{GeV}}}^{-2}$ , respectively. Takingm_Δ= 1000 GeV as an example, we can estimate the upper limits of the quantity ${(\displaystyle \frac{{s}_{\Delta }{h}_{ij}}{{m}_{\Delta }^{2}})}^{2}$ for theeeandμμcases as 3.0 × 10⁻¹⁶and 1.1 × 10⁻¹⁶, respectively. For theeμcase, following the method applied in Ref. [12], we leth_eeandh_μμequal to their upper bound, and geth_eμ≤ 1.1 × 10⁻¹⁶, which leads to ${(\displaystyle \frac{{s}_{\Delta }{h}_{e\mu }}{{m}_{\Delta }^{2}})}^{2}\le 3.3\times {10}^{-27}$ .

For ${\bar{K}}^{0}$ , there are only three channels allowed by the phase space, namely ${\pi }^{+}{\pi }^{+}{l}_{1}^{-}{l}_{2}^{-}\ ({l}_{i}=e, \ \mu )$ . The corresponding diagrams areFig. 1(a)-(d). Theπ⁺π⁺e⁻e⁻channel has the largest branching ratio, which is of the order of 10⁻³⁰(seeTable 2). Experimentally, $Br({K}^{+}\to {\pi }^{-}{l}_{1}^{+}{l}_{2}^{+})\lesssim {10}^{-10}$ [31], which is the most precise result for lepton number violation. However, lepton number violation in four-body decay channels of this particle has not been experimentally found. In Refs. [32,33], the channelsK_L,S→π⁺π⁻e⁺e⁻are investigated. We hope that the ${K}_{L, S}\to {\pi }^{+}{\pi }^{+}{l}_{1}^{-}{l}_{2}^{-}$ channels will be experimentally studied in the future.

ForD⁰, the final mesons can be pseudoscalars or vectors. The results for the case whenh₁andh₂are both pseudoscalars, that isππ,πK, orKK, are given inTable 3. The largest value is of the order of magnitude of 10⁻²⁹. We note that the Fermilab E791 Collaboration presented the upper limits of the branching ratios for these channels [34], which are of the order of 10⁻⁵. By comparing the theoretical predictions and experimental data, we find the upper limit of the constant $\displaystyle \frac{{s}_{\Delta }{h}_{ij}}{{m}_{\Delta }^{2}}$ of the order of 10⁴GeV⁻². One can also extract this upper limit from the three-body decay processes, such asD⁻→π⁺e⁻e⁻, which gives about 10²GeV⁻²by using the results in Ref. [12]. The branching ratios ofD⁰decay channels, whereh₁andh₂are 0⁻1⁻or 1⁻1⁻, are given inTable 4; the largest value has the order of magnitude of 10⁻²⁹.

The results for ${\bar{B}}^{0}$ and ${\bar{B}}_{s}^{0}$ are given inTables 5-10. The largest value is of the order of 10⁻²⁸. In Ref. [35], the four-body decay channelB⁻→D⁰π⁺μ⁻μ⁻was measured to have a branching ratio of less than 1.5 × 10⁻⁶. There are no experimental values available at present for the neutralBmeson decay channels. However, as LHCb is continuing to run, more data will be available. We expect that the LHCb Collaboration will detect such decay modes and will set more stringent constraints on the parameters of doubly-charged Higgs boson. Besides, the future B-factories, such as Belle-Ⅱ, will also have the possibility of providing more information about these channels.

In this paper, we studied the lepton number violation in four-body decays of neutral flavored mesons, including ${\bar{K}}^{0}$ ,D⁰, ${\bar{B}}^{0}$ , and ${\bar{B}}_{s}^{0}$ . They are assumed to be induced by a doubly-charged scalar. For ${\bar{K}}^{0}$ , the channel ${\bar{K}}^{0}\to {\pi }^{+}{\pi }^{+}{e}^{-}{e}^{-}$ has the largest branching ratio, of the order of 10⁻³⁰. ForD⁰, the channel ${D}^{0}\to {\pi }^{-}{K}^{-}{l}_{1}^{+}{l}_{2}^{+}$ has the largest order of magnitude of 10⁻²⁹. By comparing with the E791 experimental data, we find the upper limit for $\displaystyle \frac{{s}_{\Delta }{h}_{ij}}{{m}_{\Delta }^{2}}$ of the order of 10⁴GeV⁻². For ${\bar{B}}^{0}$ and ${\bar{B}}_{s}^{0}$ , the largest values of the branching ratio is also about 10⁻²⁸. As these values are extremely small, there are no prospects for detection of such processes in the near future. However, the constraints for such channels may provide guidance for the studies of neutrino-less double beta decays of mesons. We expect more experimental data for such processes from the LHCb and Belle-Ⅱ Collaborations.

Wave functions of mesons

With the instantaneous approximation, the Bethe-Salpeter wave function of the meson fulfills the full Salpeter equations [36]

where ${q}_{\perp }^{\mu }={q}^{\mu }-\displaystyle \frac{P\cdot q}{{M}^{2}}{P}^{\mu }$ , ${\omega }_{1}=\sqrt{{m}_{1}^{2}-{q}_{\perp }^{2}}$ , and ${\omega }_{2}=\sqrt{{m}_{2}^{2}-{q}_{\perp }^{2}}$ ;m₁andm₂are the masses of quarks and antiquarks, respectively; ${\Lambda }_{i}^{\pm }=\displaystyle \frac{1}{2{\omega }_{i}}[\displaystyle \frac{\rlap{/}{P}}{M}{\omega }_{i}\mp {(-1)}^{i}({\rlap{/}{q}}_{\perp }+{m}_{i})]$ is the projection operator. In the above equation, we have defined

and

whereϕ_P(q_⊥) is the wave function, which is constructed using ${\rlap{/}{q}}_{\perp }$ , $\rlap{/}{P}$ , and the polarization vector. Here we only show the expression for the positive energy part of the wave function. For the 1⁻state, it has the form

For the 0⁻state, it has the form

A_iandB_iare functions of ${q}_{\perp }^{2}$ , whose numerical values are obtained by solving Eq. (A1).

The interaction potential used in this work has the form [36]

where

The parameters involved area=e= 2.71828,α= 0.06 GeV,λ= 0.21 GeV², Λ_QCD= 0.27 GeV;V₀is obtained by fitting the mass of the ground state. The constituent quark masses used arem_b= 4.96 GeV,m_c= 1.62 GeV,m_s= 0.5 GeV,m_u= 0.305 GeV, andm_d= 0.311 GeV.