Anomalies in B-decays and U(2) flavor symmetry

The collection of a few anomalies in semileptonic B-decays invites to speculate about the emergence of some strikingly new phenomena. Here we offer a possible interpretation of these anomalies in the context of a weakly broken U(2)5\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$U(2)^5$$\end{document} flavor symmetry and leptoquark mediators.


Introduction
In the last years quite a few anomalies in semileptonic B-decays have emerged. While individually any of them requires confirmation before being taken under serious consideration, their collection motivates to speculate about the possible emergence of some strikingly new phenomena. The purpose of this paper is to offer a possible interpretation of these anomalies in the context of a weakly broken U (2) nflavor symmetry.
The observations we refer to have received and are receiving a lot of attention. The deviations from the SM that are both statistically more significant and whose theoretical error is negligible (compared to the present experimental error) can be summarized as follows: predicted to be one in the Standard Model (SM) with better than 1 % accuracy.
This last neutral-current anomaly may be related to other tensions with the SM in the branching ratios and in the angular distributions of semileptonic b → s transitions, particularly in B → K ( * ) μ + μ − and B → φμ + μ − (see Refs. [7,8] for an updated discussion). The interpretation of a 30 % deviation from the SM in a tree-level charged-current interaction, Eq. (1.2), calls for an exchange capable to produce at low energy an effective 4-fermion interaction proportional to the operator (c L γ μ b L )(τ L γ μ ν L ). On these grounds one may want to interpret the neutral-current anomaly in Eq. (1.3) as also due to an LL operator of the form (s L γ μ b L )(μ L γ μ μ L ). Although not exclusively, it is known that such an operator can as well improve the fit in the angular distribution of the semileptonic b → s transitions [7,8]. There is, however, a problem to face. While both anomalies hint at a 20 ÷ 30 % deviation from the SM, there is an important difference among them. The charged-current anomaly is a deviation from a SM tree-level amplitude involving the third generation of leptons, whereas the neutral-current one is a putative correction to a SM-loop effect only concerning the first two generations of leptons.
This motivates us to ask whether there is a flavor group G F and a tree-level exchange such that: • With unbroken G F , couples to the third generation of quarks and leptons only; • After G F -breaking, the needed operators, as mentioned in the previous paragraph, are generated as a small perturbation.
The answer is positive with (1.5) in the notation of Refs. [9][10][11][12], and is a leptoquark singlet under G F , carrying either one of the following quantum numbers under the SM gauge group: Dynamical explanations of the above anomalies have already been proposed in the literature both in terms of vector uncolored mediators [13] and in terms of leptoquark mediators [14][15][16]. 2 Here we focus on the specific realization of leptoquark models based on the flavor group G F since: (i) this explains their dominant coupling to the third generation only (in particular only to the left-handed quark and lepton doublets which are the only G F -invariant fermions); (ii) the breaking of G F specifies the source of the flavor violating couplings needed to give rise predominantly to the operator (c L γ μ b L )(τ L γ μ ν L ) and, at a weaker level, to (s L γ μ b L )(μ L γ μ μ L ) as well.
About the needed breakings of G F , we stick to the minimal set of spurions for G q F [9] and for G l F [25,26]. In the following we write down in the three cases above the leptoquark (LQ) couplings to the fermions in their physical bases after inclusion of G F -breaking (Sect. 2) and we calculate the relevant amplitudes at tree level (Sect. 3). Consistency with current data is achieved only by the U μ = (3, 1) 2/3 model above. The dominant loop effects when the tree-level amplitude vanishes are calculated in Sect. 4 for the surviving vector-singlet model. The overall consistency of the model with data is illustrated in Sect. 5, where further expected signals are also examined. A tentative UV completion of the phenomenological model is briefly outlined in Sect. 6. Summary and conclusions are drown in Sect. 7.

Leptoquark Lagrangians after G F -symmetry breaking
The couplings of the three LQ to the SM electroweak doublets Q L and L L are (a is an index in the vector representation of SU (2) L , whereas the color indices are left understood) where F is a matrix in flavor space which, in the G F symmetric limit, is F i j = δ i3 δ j3 . On the other hand, after symmetry breaking along the directions (1.6) and (1.7), F takes the form where, by symmetry transformations, we can write in terms of two small real parameters Q , L , and a, b, c are arbitrary coefficients, generically of order unity, that we shall also take real for simplicity. In Eq. (2.4) we neglect terms proportional to the product y b y τ of the bottom and τ Yukawa couplings or to products of u,d,e . At the same time and in the same bases as Eq. (2.4), the Yukawa matrices for the charged fermions take the form where x b is another unknown coefficient in general of order unity. One goes to the physical bases for all the charged fermions by an approximate diagonalization of these Yukawa matrices. In these physical bases the LQ interaction Lagrangians acquire the form and θ l is the angle (s l = sin θ l , c l = cos θ l ) in the unitary transformation that diagonalizes l on the left side. We are working in the basis of neutrino current eigenstates, where the charged-current leptonic weak interactions are flavordiagonal. We are also neglecting a phase in the 13 and 31 elements of these flavor matrices since it does not play any role in the following considerations.

Tree-level amplitudes
In the three models defined in Sect. 1 the tree-level exchanges of the corresponding LQ give rise to effective Lagrangians relevant to charged-current and neutral-current semileptonic B and K decays. For b → cτν 3 one has to be compared with the SM result In both cases (SM and LQ exchange) the b → uτν 3 effective Lagrangians are obtained from the above ones with the exchange c → u and V cb → V ub .
For the neutral-current processes b → s ¯ , with = e, μ, τ , the LQ exchange gives whereas the lepton-universal local b → s ¯ effective interaction present in the SM reads Finally, for b → sν 3ν3 and s → dν 3ν3 amplitudes, the LQ exchange gives (3.5) to be compared with where C SM ν ≈ −6.3 (and we have omitted the subleading charm contribution in the s → dνν case). Note the absence of a tree-level contribution to b → sνν from the SU (2)singlet vector LQ (model 1), as noted first in Ref. [14].
Similarly from Eqs. (3.5) and (3.6) one has where for the various models it is (3.10) A similar formula holds for R πνν = B(K → πνν)/B(K → πνν) SM , in the limit where we neglect the subleading charm contribution and replace a). This puts a strong constraint on models 2 and 3 of Sect. 1, shown in Fig. 1 (for R K ( * ) ν we use the bound R K ( * ) ν < 4.3 [27]), making them highly disfavored [14]. From now on we therefore concentrate our attention on model 1 with a vector-singlet LQ.
For later use, R while the corresponding τ/e and τ/μ ratios are The result in Eq. (3.12) holds for any b → sττ rate, e.g. also for B(B → τ + τ − ) and B(B → K * τ + τ − ), normalized to its corresponding SM value. At present this does not represent a significant constraint given that the experimental upper bounds on these modes are still 3 orders of magnitude above the SM level [27], but in the future this large enhancement could provide a striking low-energy signature of the model. To conclude this section, it is worth comparing the treelevel effects induced by the LQ exchange (model 1) with those analyzed in Ref. [13] assuming a vector uncolored mediator. The structure of the semileptonic operators generated is the same, but the relative weight of charged-and neutral-current terms is different: in Ref. [13] the neutralcurrent operators receive an additional overall suppression factor. This is why in Ref. [13] the non-standard effects are much smaller in the case of b → sνν and b → sττ transitions. Another difference is the absence, at the tree level, of LQ contributions to B-meson mixing. However, as we will discuss next, this different is only apparent: quadratically divergent contributions to F = 2 amplitudes are generated in the LQ case at the one-loop level and, similarly to the case of Ref. [13], B-meson mixing represents a significant constraint on the model.

Loop effects
Several processes exist which do not take place in the leptoquark models under consideration at tree level, but appear only at the one-loop level. A relevant example, as already noticed, is the b → sνν amplitude in the SU (2)-singlet vector leptoquark model 1 of Sect. 1. Since several of these processes can give significant constraints, a one-loop calcu-lation is necessary, especially, but not only, when there are quadratically divergent contributions.
For the Lagrangian that describes the free propagation of the leptoquark U μ and its interactions with the SM gauge bosons we take and with obvious meaning of the symbols. L U is gauge invariant under the SM group for any value of k s and k Y . The overall interaction Lagrangian of the leptoquark with the B μ field is therefore As a non-trivial check of our calculations it will be useful to notice that, for k Y = 1 and 2/3g = g, Eq. (4.4) becomes the triple vertex among the W bosons in the SM with the identifications for a fixed color component of the leptoquark field.

Quadratically divergent loop effects
From exchanges of the U μ vector quadratically divergent corrections appear: (i) in the 2-point function of the B μ field, (ii) in the 3-point function between B μ and the fermion fields, (iii) in box-diagram contributions to various 4-fermion interactions. Below we list the relevant corrections.

Two and three-point functions
In the LQ model we have the following contribution to the B μ propagator: We do not include a correction to B B μν at q 2 = 0, which vanishes by electromagnetic gauge invariance, nor a contribution proportional to q 2 since it is reabsorbed in a redefinition of g .
Similarly one has 2 -divergences in the 3-point correlation functions with an external B μ field As remarked above, this implies the presence in the SM in the unitary gauge of similar contributions in the 2 and 3-point functions of the W a μ field, at g = 0, where F = Q or L and T a is the weak isospin. We have explicitly checked that quadratically divergent contributions to physical amplitudes vanish in this limit of the SM, as they should, with the inclusion of box diagrams as well. with the process-dependent effective operators and the corresponding coefficients (F a W a ) given in Table 1.

Dipole operators
Unlike the previous cases, the coefficients of the dipole operators are not quadratically divergent. Yet they are logarithmically divergent and yield potentially relevant constraints given the stringent experimental bounds on τ → μγ , μ → eγ and b → sγ . The leading LQ contributions to these processes are encoded by (4.14)

Electroweak precision tests
At the one-loop level in the leptoquark vector-singlet model there are no corrections to the S, T, U parameters. This is due to the fact that U μ only couples to B μ and not to the W a μ -fields. There are, however, corrections to the electroweak Precision Tests (EWPT) due to higher dimensional operators, which are at least in principle important due to 2 -divergent effects.
The most effective way to see these effects is by considering the i -parameters, as defined in [28,29], and their expressions in terms of vacuum-polarization, box-diagram, and vertex corrections for S, T, U = 0 [30]. More specifically, in the limit where one neglects the small G F -breaking, the first two generations receive corrections only from B B μν = −ig μν (q 2 ): and To estimate A, we take ≈ 4π M U /g U , which gives Given the bounds on the deviations from the SM of the i at the 10 −3 level, with R U ≈ 0.1 and g 2 U /(gg ) 2 ÷ 3, this is a mild constraint on k Y .
Still without any G F -breaking, a vertex correction intervenes in Z -decays to the third generation. Specifically, from Eq. (4.8), the corresponding amplitudes get corrected as which can be estimated as Consistency with the few per mille measurement of B(Z → τ + τ − ) and R U ≈ 0.2 requires

Box diagrams and dipole operators
Some of the box-diagram contributions shown in Table 1 give extra significant constraints on the parameter space of the leptoquark vector-singlet model. Such constraints are given in the last column of Table 1 in the leptonic processes. The bound on the flavor coefficient relevant to τ → μγ (obtained in the limit k Y = 0) is whereas the one on μ → eγ is

Overall constraints
As apparent from Sects. 3.1 and 5.2 the leptoquark effects in R τ/l D ( * ) (at tree level), R K ( * ) ν , B(K + → π + νν) and bs →bs (at loop level) are predicted in terms of two single effective parameters, R U and β = 1 − (1 − a)r u , for a cutoff ≈ 4π M U /g U . The consistency with data of all these effects is shown in Fig. 2

Leptoquark pair production at LHC
The LQ production at the LHC is dominated by the QCD pair production and it depends only on M U . A compilation of results relevant to our model 1 can be found, for instance, in the recent CMS analysis [31]: the cross-section varies from about 1 pb for M U ≈ 0.5 TeV to 3 × 10 −3 pb for M U ≈ 1.0 TeV. 3 In order to determine the LHC sensitivity to various LQ searches we need to evaluate the branching ratios in the different decay channels. At the tree level one has and, to a good accuracy, the total decay width is given by the sum of the two leading decays (U → tν τ , bτ ): tot = g 2 U M U /(12π). The branching ratios are then just given by For the searches in the second-generation channels performed in Ref. [31] (UŪ → μμj j and UŪ → μν j j, where j denotes a light-quark jet) we find from which we deduce that these searches do not put any significant constraint on the model. On the other hand, a relevant constraint is obtained by the dedicated search for the UŪ → ttν τντ decay chain performed by ATLAS [32]. In our model B(UŪ → ttν τντ ) = 0.25 that implies the limit M U > 770 GeV. (5.14) By a naive scaling of the statistics and the cross-section, we estimate that this limit could improve up to 1.3 TeV, in absence of a signal, with 300 fb −1 at 13 TeV.
Taking into account the constraints on R U in Fig. 2, the bound on M U can be turned into a bound on g U . For R U > 0.2 we get g U > 1.4, which would increase to g U > 2.4 in the absence of a direct signal with 300 fb −1 at 13 TeV.

A naive composite leptoquark picture
Needless to say the phenomenological model described so far cries out for a UV completion. Here we describe an attempt in the direction of composite Higgs models that will at least serve to illustrate the difficulties to comply with the various constraints. It does not take much to anticipate that the main such constraint comes from the value of R U as implied by Fig. 2.
Let us consider a strongly interaction sector with a global symmetry SU (4)×SO (5) spontaneously broken down to the Pati-Salam group SU (4)×SU (2) L ×SU (2) R , so as to generate a composite pseudo-Goldstone Higgs boson. As usual the SM group is gauged inside the residual global group. Within SU (4) this structure leads to composite quasi-degenerate vectors: the composite gluons, a vector singlet carrying B −L and, most importantly, the U μ leptoquark vector.
The strong sector will also contain composite vector-like fermions in multiplets of the Pati-Salam group occurring in three flavor species. The important thing is that these composite fermions have components that match the quantum numbers of the SM fermions with respect to the SM gauge group. The requisite to make contact with the phenomenological model described in the previous Sects. is that the mass mixing terms between the elementary and the composite fermions respect, up to small breaking terms, the symmetry in flavor space U (2) × G F . 4 With = (4, 2, 1) ⊕ (4, 1, 2) (plus complex conjugate states) it is easy to convince oneself that this structure shall lead, in the unbroken U (2) × G F limit, to Eq. (2.1) with g U = g * sin θ Q3 sin θ L3 (6.1) and F i j = δ i3 δ j3 as the only interaction of U μ with the standard fermions. Here g * is the coupling of the LQ to the composite fermions and θ Q3 , θ L3 are the mixing angles of Q 3 , L 3 with the same composite fermions in . Other choices of , phenomenologically motivated, shall lead to a relation between g U and g * involving more parameters but always respecting g U ≤ g * .
The "standard" interpretation of the composite Higgs models also gives a similar mass M ≈ g * f for the composite vectors in the adjoint of SU (4), among which is U μ , and f is the breaking scale of SO(5) down to SO (4). As a consequence the phenomenological parameter R U becomes independent from g * .

Summary and conclusions
Being the heaviest particle in the SM, the top quark plays a special role in many processes and/or mechanisms of the greatest relevance in particle physics. It is not surprising therefore that the top quark is thought to be equally important in several BSM speculative considerations. Flavor physics is no exception to this rule. In the SM top exchanges dominate many of the observed flavor changing neutral current effects. In BSM, taking minimal flavor violation as a relevant example, it is the relatively large top Yukawa coupling that controls many of the new observable phenomena that might occur. This is the basis to consider a U (2) 3 approximate symmetry as a ruling symmetry of the flavor quark sector of any putative extension of the SM. More precisely U (2) Q × U (2) u × U (2) d × U (1) d3 , a residual symmetry of the SM with all the Yukawa coupling switched off but the top one, can allow, suitably broken, for mild deviations from the SM itself. Decays of the B mesons, in particular through the b Lcomponent, which is the only singlet under U (2) 3 × U (1) d3 other than t L ,R , are obvious candidates where such deviations might occur and be observable.
It is therefore natural to ask if and how the recently emerged anomalies in semileptonic B-decays can be accommodated in this context. As we have shown this is possible by: (i) invoking the exchange of a vector-singlet LQ with a relatively large value of the parameter R U = 4M 2 W g 2 U / g 2 M 2 U ≈ 0.2, i.e. a ratio well below 1 TeV between its mass M U and its dominant coupling g U to the third generation of left-handed quarks and leptons; (ii) extending the U (2) 3 × U (1) d3 symmetry of the quark sector, with its breaking, to the lepton sector as well, via a U (2) L × U (2) e × U (1) e3 flavor symmetry.
The observed anomalies arise as relatively small effects of the breaking of the overall U (2) 5 symmetry, thus allowing non-vanishing couplings of the LQ to the lighter generations as well.
The deviation from the SM in the charged-current observable R τ/l D ( * ) is due to a tree-level exchange of the LQ controlled, other than by R U , by a single combination of dimensionless parameters β, as shown in Fig. 2. The same effective parameter controls the quadratically divergent one-loop contributions to B → K ν 3ν3 , K → πν 3ν3 and bs →bs, as well as the tree-level effect in b → sττ . All of these processes can corroborate or exclude the LQ model by future measurements.
The lepton flavor violation emerging in the neutral-current observable R μ/e K can also arise from a tree-level exchange of the leptoquark, although suppressed by the intervention in the final state of muons or electrons. In this case the relevant parameters control as well the log-divergent one-loop dipole moment contributions to τ → μγ and μ → eγ . The current limits on both these processes are close to saturate the observed deviation of R μ/e K from unity, at least in a natural range of the relevant parameters, as illustrated in Figs. 3 and 4.
To discuss the possible manifestation of the vector LQ in direct production strongly depends on being able to go beyond the low energy phenomenological picture that we have used in this paper. This is because the constraint on R U ≈ 0.2 only fixes the ratio M U /g U between the mass and the coupling of the LQ. The current LHC searches bound M U to be bigger than about 700 GeV, independently from the value of g U , which is therefore constrained to be bigger than about 1.4. Larger values of g U , and therefore of M U as well, are indirectly hinted by the constraints from τ → μγ and μ → eγ . All this points toward the need of a UV completion of the phenomenological model used so far, perhaps along the lines outlined in Sect. 6. It will be interesting to see if and how such UV completion can be accomplished consistently with the numerous constraints.