Leptoquark Flavor Patterns&B Decay Anomalies

Flavor symmetries that explain masses and mixings of the standard model fermions dictate flavor patterns for the couplings of scalar and vector leptoquarks to the standard model fermions. A generic feature is that couplings to $SU(2)$-doublet leptons are suppressed at least by one spurion of the discrete non-abelian symmetry breaking, responsible for neutrino mixing, while couplings to charged lepton singlets can be order one. We obtain testable patterns including those that predominantly couple to a single lepton flavor, or two, or in a skewed way. They induce lepton non-universality, which we contrast to current anomalies in $B$-decays. We find maximal effects in $R_{D}$ and $R_{D^*}$ at the level of $\sim$10 percent and few percent, respectively, while leptoquark effects in $R_{K^{(*)}}$ can reach order few$\times 10$ percent. Predictions for charm and kaon decays and $\mu-e$ conversion are worked out.


AB QLQL U LŪ L DLDL QEQE U EŪ E DEDE
down-type FCNC ---up-type FCNC ---- Table I: Leptoquark couplings Y AB and YĀ B as they appear in various leptoquark models as well as in tree level down-type quark FCNCs and up-type quark FCNCs. Models S 1,2 and V 1,2 have two yukawas each.
appear in leptoquark models with couplings to SU (2) L doublet quarks Q and leptons L, and SU (2) L singlet quarks U, D and charged leptons E, schematically, where rows and columns correspond to quarks and leptons, respectively. To simplify the discussion, in the following these couplings are denoted Yukawa matrices for both scalar and vector leptoquarks. Table I shows for which leptoquark scenario which type of yukawa is present. Also indicated is by a checkmark which yukawa contributes at tree level to (semi-)leptonic flavor changing neutral current (FCNC) transitions in the down and up-quark sector. Contributions to charged currents, e.g., b → c ν in chirality-preserving four-fermion interactions,Qγ µ (σ a )QLγ µ (σ a )L [5] arise from Y QL , YQ L only. σ a denote the Pauli-matrices. S 1,2 and V 1,2 induce charged currents through a combination of their two couplings present, resulting in chirality-flipping operators.
Patterns based on a U (1) FN -Froggatt-Nielsen (FN) symmetry [6], combined with a non-abelian discrete symmetry, A 4 , have been worked out previously for leptoquarks coupling to lepton doublets [7,8]. Here we provide further details and flavor patterns involving singlet leptons. The U (1) FN explains hierarchies in the quark sector and for the charged lepton masses, while non-abelian discrete subgroups of SU (3) can accommodate neutrino mixing [9]. We stress that leptoquark extensions of the SM are special as they can access both quark and lepton flavor.
would occur for scalar and an increase of hierarchies for vector leptoquarks. Lepton-doublet scenarios would also be affected in models with q(L) = 0. For q(L) = 0, Y AL = YĀ L .
The breaking of the U (1) FN can lead to BSM scalars (flavons) in reach of present or future colliders, with corresponding phenomenology driven by the FN-charges, e.g., [27,28]. Such analysis is interesting, however, beyond the scope of our paper, which focusses on leptoquark-induced BSM effects.

III. FLAVOR SELECTION WITH DISCRETE SYMMETRIES
We employ the discrete symmetry A 4 × Z 3 to model the lepton mixing based on a modification [29] of the original model [25], which introduces an additional field to account for a non-vanishing value of θ 13 . Table II summarizes the charge assignments of the leptons and the flavon fields, adopted from [7]. The FN-spurion is uncharged under A 4 × Z 3 . The VEVs of the flavons are given L e R µ R τ R φ φ ν ξ ξ  as φ /Λ = c (1, 0, 0), φ ν /Λ = c ν (1, 1, 1) and ξ ( ) /Λ = κ ( ) , where Λ denotes a new physics scale related to A 4 -breaking. The values of the VEVs are, in general, model-dependent. Typically, c ,ν , κ ( ) λ few to explain charged lepton and neutrino parameters. Here and in the following we use the term "VEV" for c ,ν , κ ( ) as well. While the latter are dimensionless numbers it should be clear that they do not correspond to renormalizable couplings of the full Lagrangian.
For completeness, we briefly summarize the multiplication rules for A 4 . For further information on the basis and group theory of A 4 see [30]. The group has three singlet representations 1, 1 , and 1 which form a Z 3 subgroup with the usual multiplication rules. Additionally, A 4 has a triplet representation. Denoting two triplets as A = (a 1 , a 2 , a 3 ) and B = (b 1 , b 2 , b 3 ) the product reads with a symmetric (s) and an antisymmetric (a) triplet.
Firstly, all quarks are considered A 4 singlets (Section III A). In Section III B we discuss patterns for individual quark generations in non-trivial singlet-representations of A 4 .
A. Quarks trivial under A 4

Flavor patterns
If all quarks have a trivial A 4 -charge and identical Z 3 -charges, one needs to distinguish only between the couplings to right-handed leptons Y AE (YĀ E ) and to left-handed leptons Y AL (YĀ L ). The column structure of the patterns is governed by the A 4 and Z 3 -charges of the leptoquark. The A 4 -charge determines to which lepton generation(s) the leptoquark can couple, while the Z 3 -charge selects the flavon field that mediates the coupling. We denote the leptoquarks S † i , V † i generically by ∆ and the charge assignments by [∆] A 4 etc.
For the left-handed couplings the crucial flavons are the A 4 -triplets φ and φ ν , which produce patterns that either isolate a single lepton generation or couple equally to all generations [7].
For the right-handed leptons, terms of the form A∆E are Z 3 -invariant without any additional flavon insertion for [∆] Z 3 = 2. (Here and in the following, as in Eq. (1), A (B) generically denotes quark (lepton) fields.) In this case one isolates a single lepton generation, depending on the leptoquark's A 4 -representation. Additionally, and in contrast to the respective pattern for the left-handed coupling, the isolated column is suppressed by powers of λ due to the FN-charges of the right-handed leptons. For [∆] Z 3 = 0 one additional flavon, ξ or ξ , is needed. Since the latter have identical Z 3 -charge but transform under different singlet representations of A 4 , two lepton generations are isolated.
To summarize these findings we introduce the following lepton flavor isolation textures from which all patterns can be constructed. Here, " * " denote non-zero entries whose parametric flavor dependence is given by the U (1) FN . Table III shows the resulting patterns for the Yukawa matrices Y AL (YĀ L ) and Y AE (YĀ E ) as linear combinations of the k -matrices, = e, µ, τ . For instance, It is manifest from these patterns that generational hierarchies can be inverted relative to the ones of the fermion mass terms. Neglecting terms of order λ 2 the pattern R eµ (Ū E), which can appear in theṼ 1 scenario, closely resembles patterns leading to sizable LFV in rare charm decays [8]. Contributions with [A∆B] Z 3 = 2 arise at second order in the A 4 -flavon expansion, and yield democratic patterns, L d and R d , see Table III.
For the leptoquarks S 1 , S 2 , V 1 and V 2 both left-and right-handed couplings can be present simultaneously. Since the lepton and quark mass terms must be Z 3 -invariant, both interaction terms of the respective leptoquark must have identical Z 3 -charge Quite generally, and beyond the explicit A 4 ×Z 3 model, the flavon VEV suppression in leptoquark couplings to lepton doublets cannot be avoided, once the three generations of doublets are in a triplet representation of the non-abelian group in order to give the Pontecorvo-Maki-Nakagawa-Sakata (PMNS)-matrix. This feature is of course manifest [7] in the A 4 × Z 4 model [29,31]. Requiring invariance of the term A∆L one therefore needs an insertion of a triplet flavon VEV. The other alternative would be to make the leptoquark a triplet, which leads to a democratic pattern and does not give rise to LNU. Note, in see-saw models, terms with right-handed neutrinos, which are triplets of A 4 and carry Z 2 = 2 [31] result in VEV-suppressed, democratic patterns.

Mass basis rotation
We consider modifications of the patterns derived in the flavor basis from changing to the mass basis. The corresponding transformations of the fermion fields by the unitary matrices U, V read from which the Cabibbo-Kobayashi-Maskawa (CKM) and PMNS mixing matrices are obtained as In leptoquark models also other combinations become physical. In particular, the leptoquark yukawas transform as Quark rotations therefore only mix rows, whereas lepton rotations only mix columns.
The parametric dependence of the rotation matrices in the quark sector can be obtained by perturbative diagonalization [32] as 1 The resulting mixing of the rows does not spoil the patterns as the hierarchical suppression of the leptoquark yukawas stays parametrically intact. Note, that this does not hold true anymore for quarks charged non-trivially under A 4 , as discussed in Section III B.
Since the transformations U, V are unitary and neutrinos are inclusively reconstructed in collider experiments, the rotation V ν has no impact on such observables. Furthermore, in the A 4 × Z 3 framework considered in this work, the charged lepton Yukawa matrix Y is already diagonal at leading order. However, higher order flavon insertions can induce non-diagonal entries in Y [33].
We discuss this in the next section together with other higher order effects.

Higher order flavon corrections
It is easy to compute Y including next-to leading order corrections from which the rotation matrices follow as, using perturbative diagonalization [32], Here, we introduced a parameter δ < 1, of the order (VEV) 2 , The effect of transforming the left-handed charged leptons is therefore O(δ), at second relative order in the flavon expansion and modifies Y AL,ĀL . This implies, for instance, for the tau-isolation Rotations stemming from the right-handed leptons contribute at higher orders in λ. E.g., this effect modifies single and double lepton isolation patterns in Y AE,ĀE such as those given in Eq. (9) For the R τ -pattern mass rotation effects amount to The patterns given in Table III [7]. In terms of δ introduced before these higher order effects amount to the same as what we got from the mass basis rotation, Eq. (21). The democratic pattern L d is subject to next-to leading order corrections from φ ν → φ plus one additional A 4 -singlet. However, because of the unknown O(1) coefficients, these corrections are immaterial.
The explicit higher order flavon corrections to the patterns of right-handed leptons arise universally for each entry at third order: two times φ ν plus one singlet flavon or three singlet flavons. Denoting If there are cancellations between the FN charges of the quarks and leptons, these corrections can be larger than the mass rotation effect Eq. (23). For phenomenology one therefore has to take the maximum of each entry of Eq. (23) and (24). Similarly, for the double lepton isolation patterns where δ = O(VEV 4 ).

B. Quarks non-trivial under A 4
Single quarks in a non-trivial A 4 × Z 3 -representation allows to construct further flavor patterns for the leptoquarks. In Ref. [7] this has been discussed for A 4 × Z 4 models. Here, to formally restore A 4 × Z 3 -invariance of the SM yukawa terms of the quarks insertions of ξ are necessary. In order to not destroy the quark masses and mixings, the A 4 -VEV suppression κ ∼ λ m needs to be compensated by a corresponding change in FN-charge. Additionally, the Z 3 charge of the inserted flavon fields has to be cancelled. The following choices leave the SM Yukawa matrices of the quarks intact: or, with two insertions, Here, A can be any of the quark fieldsQ, U, D of first or second generation, i = 1, 2. For the third generation this leads to a suppression of third generation yukawas.
The different charges for one generation of quarks lead to a mixing of rows between patterns characterized by different [A∆B] Z 3 and [∆] A 4 and a modified hierarchy in the entries " * " of the lepton flavor isolating textures, k . If the quark generations j = i are trivially charged and couple to the pattern characterized by see also Table III, then the ith row corresponding to the non-trivially charged quark is given by the pattern with and the total A 4 -charge [A∆] A 4 of the quark and the leptoquark. Note that since the FN-charge of quarks has been changed, corresponding mass basis rotations Eq. (17) do matter. Choosing , that is, a = 0 and m = 2 gives a modification of the µ-isolation pattern, asL where for QL the second row has [A∆B] Z 3 = 2 and correspondingly couples to L d and forQL the second row has [A∆B] Z 3 = 1 and correspondingly couples to L d . Including mass basis corrections where we note that due to Eq. (2) the FN-suppression of the first row is λ 2 . The FN-suppression of the second row present in L µ is inL µ turned into a VEV-suppression. TheL µ -patterns are relevant for b → sµµ processes. Similarly, modifications of τ -isolation patterns can be obtained for which is an example for a pattern that potentially maximizes the effect from doublet quarks and leptons in R D , R D * . Relevant leptoquarks are V 1 and V 3 . After mass basis rotations For V 1 and V 3 constraints from µ − e-conversion data apply as λ 4 c 2 c 2 ν λ 2 5 · 10 −6 (M/TeV) 2 , that is, c ν 0.01(M/TeV), somewhat stronger than µ − e-conversion. This prohibits noticeable effects in b → sµµ transitions, which are induced at parametrically the same order of magnitude as the kaon decay. Constraints on scalar Wilson coefficients, which involvẽ L τ · R τ , exist from the B s → µµ branching ratio. They read δc ν < 2 · 10 −3 (M/TeV) 2 and can be evaded naturally for δ 0.1.
A similar pattern can be obtained forŪ L-couplings, by charging up-quark singlets non-trivially, however, with an additional suppression of the second row by κ relative to Eq. (32).L τ (Ū L) is relevant for model S 2 . Including mass basis corrections, There are no kaon bounds onL τ (Ū L). The branching ratios of D → µµ and similarly D → πµµ [8] impose κc ν 0.02(M/TeV).

IV. FLAVOR PHENOMENOLOGY
The flavor patterns obtained in Section III can be used directly for predictions in flavor physics.
Contributions to dimension six operators induced by tree level leptoquark exchange can be read-off from Tables V and VI for scalar and vector leptoquarks, respectively, updating [2] with signs and tensor operators. To discuss LNU in the B-system and explore possible signatures in charm we additionally provide the Wilson coefficients for the semileptonic transitions b → cτ ν in Table XI, for b → s , νν in Table XII and for c → u , νν in Table XIII. We discuss in Section IV A leptoquark effects in B → D ( * ) ν decays and in Section IV B LNU signals in b → s processes within flavor models. In Section IV C we work out signatures for charm and kaon decays and µ − e conversion.
where in the denominator = µ at LHCb and = e, µ at Belle and BaBar. In Table IV experimental findings and SM predictions for R D , R D * and the τ -polarization P τ , as measured in the rest frame BaBar [37] 0.440 ± 0.058 ± 0.042 0.332 ± 0.024 ± 0.018 --Belle [38] 0.375 ± 0.064 ± 0.026 0.293 ± 0.038 ± 0.015 -- D and the τ -polarization. † Error weighted average; we added statistical and systematical uncertainties in quadrature. For R ave D * we used [36][37][38][39][40]. Without [36], of the B-meson, are given. Formulae for the branching ratios involving left-and right-polarized τ -leptons, B − and B + , respectively, are given in Appendix B. SM predictions for P τ (D * ) and P τ (D) are obtained by using the form factors of Refs. [10] and [35], respectively. Our SM value of P τ (D * ) is in very good agreement with the one quoted in [36], P τ (D) has larger uncertainties due to the lattice form factors.

Vector-like contributions
We begin with some general considerations on the order of magnitude of leptoquark effects induced by a dimension six operator with doublet quarks and leptons, O V 1 , see Appendix B for details. Such a vector-type operator is induced for the representations V 3 , S 3 , and, together with a Here n(∆) = −1/2, +1, −1 are Fierz factors for S 3 , V 1 , V 3 , respectively. InR D * contributions from , and the expression holds for V 1 at this level. For S 3 , V 3 holds exactlyR D =R D * .
Confronting Eq. (38) to data (37), one obtains We learn that, model-independently, i) M 3 TeV or perturbativity breaks down and ii) to avoid collider search limits for "third generation leptoquarks" decaying to tτ M > 685 GeV [42] the yukawa couplings need to be not too suppressed, does not couple to tτ , but rather to tν. Corresponding mass limits are similar [15]. For scalar leptoquarks decaying 100 % into a muon (an electron) and a jet, the limits are M > 1160 GeV [43] (M > 1755 GeV [44] Limits for vector leptoquarks are model-dependent and read M > 1200 − 1720 GeV (M > 1150 − 1660 GeV) for 100 % decays to muon plus jet (electron plus jet) [45].
A maximal prediction from flavor models is The suppression at second order in the flavon VEV is unavoidable in couplings to lepton doublets which are triplets of the non-abelian discrete group, and holds beyond the A 4 × Z 3 model considered here, see Section III A. An explicit realization is given by the model with non-trivially charged quarks, as, for instance, for the τ -isolation patterns, L τ , given in Eq. (21).
We are therefore led to conclude that flavor models cannot explain the few×0.1 enhancement in R D ( * ) relative to the SM as in present days data with vector-type operators, that is, within the models S 3 , V 3 . V 1 is discussed separately in Section IV A 3. On the other hand, the possible effects can show up at the level few percent for "maximal" and few permille for the generic case. The τ -polarization for BSM in the operator O V 1 only is SM-like, andR D =R D * .
We consider now the leptoquarks S 1 , S 2 , which induce scalar and tensor operators, O S 2 and O T , respectively. Their Wilson coefficients are related as C τ ντ S 2 = ∓r C τ ντ T , r = 7.8, where the upper sign (lower sign) corresponds to S 1 (S 2 ) at renormalization scale around m b , see Appendix B for details.
As in Eq. (38) for the vector-type operators, we linearize the LNU-sensitive observables, In both last rows of Eqs. (42) and (43) we neglected the contributions from = e or µ as they enter with mass suppression relative to the τ -contribution. A Fierz factor of −1/2 is included. In general R D =R D * and in particular for S 2 , corresponding to the bottom sign,R D andR D * cannot be both simultaneously enhanced. To fit the data (37) in this leptoquark model, one has to go beyond the linear approximation and introduce imaginary parts [10,11]. This is illustrated in Fig. 1, where we show the 1 σ allowed regions for R D and R D * for S 1 (plot to the left) and S 2 (plot to the right). In The best fit points read The hierarchy required for S 1 can be explained naturally with the flavon VEVs. In L τ (QL), R τ (U E) the ratio is ∼ c .
In contrast to the lepton doublets, the leptoquark yukawas to the lepton singlets do not require a flavon VEV insertion and can be order one. The resulting flavor model prediction for chirality-flipping operators is therefore subject to a single VEV suppression from the doublets only, Figure 1: Preferred regions for the coupling Y Y * | τ in leptoquark model S 1 (plot to the left) and S 2 (plot to the right). In the fit to S 1 we fixed Y QL Y * QL | τ to its conservative, upper limit given by Eq. (44). The red and green bands show the 1 σ allowed regions by R D and R D * , respectively. Also shown is the induced Wilson coefficient C τ ντ S2 . Dark and light blue bands correspond to the best fit regions at 1 and 2 σ, respectively. This is realized in the scalar contribution of leptoquark V 1 byL τ (QL), Eq. (32), and the τ -isolation patterns, R τ (DE), the maximum of Eq. (23) and (24). The corresponding VEV is c ν . We discuss this further in Section IV A 3. Generic predictions for chirality-flipping contributions in flavor models are given by for instance, with the patterns L τ and R τ , given in Eq. (21) and the maximum of Eq. (23), (24), respectively. For leptoquark V 2 the contributions are induced by L τ (DL) (orL τ (DL)) and R τ (QE) and of the order Y Y * | τ ∼ c λ 4 , further FN-suppressed than the generic case.
Maximal effects inR D andR D * from chirality-flipping operators are therefore possible at the level of a few percent (D * ) and reaching 0.1 (D) (for S 2 ), and one order of magnitude lower for the generic case. In S 2 an enhancedR D implies a suppressedR D * and vice versa.
For the τ -polarization, we find where the upper (lower) sign corresponds to leptoquark S 1 (S 2 ).

Leptoquark V 1
For V 1 withL τ (QL) and R τ (DE) 2 exist both vector-like and chirality-flipping operatorŝ If the chirality-flipping contribution dominates, bothR D andR D * can be enhanced, and at the same time differ as the deviation from the SM is larger inR D . Kaon decay constrains c ν 0.01(M/TeV), which has been taken into account above. Corresponding µ − e conversion bounds are very close, c ν 0.02(M/TeV). It would therefore require the tuning of both the first and the second quark generation coefficients to ease these constraints. While B → Kνν constraints do not apply to V 1 at the matching scale µ ∼ M , a contribution is induced by renormaliztion group running from M to the weak scale [47]. Corresponding constraints are, however, weaker than the ones from kaon decays and µ − e conversion.
For the τ -polarization, we find where in the last steps we imposed kaon constraints.

Synopsis of leptoquark models for R D ( * ) and the τ -polarization
Maximal predictions forR D ( * ) − 1 from leptoquarks V 1 , V 3 and S 2 in flavor models are shown in We learn that present data onR D andR D * cannot be explained within 1.6σ and 3.1σ, respectively.
Difficulties in explaining sizable BSM in R D * have also been encountered within the context of Two-Higgs doublet models once conditions on the flavor structure are imposed [48].
The Belle II projection for the uncertainty on R D is 5.6% (3.4%) with 5 ab −1 (50 ab −1 ) and for R D * is 3.2% (2.1%) for 5 ab −1 (50 ab −1 ) [49]. This suffices to probe all leptoquark models on the basis of branching ratio measurements even close to SM values.
The predictions for the τ -polarization are similar to the ones for R D ( * ) with contributions from vector-like operators removed. P τ (D * ) can differ from the SM by at most a percent. Deviations from the SM in P τ (D) can reach up to several percent. Present data on the τ -polarization, given in (37), are in agreement with the SM and are not sensitive to leptoquark flavor models yet.
We analyze tree level leptoquark effects in b → s within the representations S 3 , V 1,2,3 andS 2 .
We do not consider S 2 andS 1 because they induce only contributions onto operatorssγ µ b γ µ (1+γ 5 ) , whose impact on B → K ( * ) branching ratios is very small. We focus on explaining the measurement of R K [50] by LHCb for dilepton masses squared between 1 and 6 GeV 2 [51] A model-independent analysis points, at 1σ, to modifications to the vector-type operators O ( ) 9,10 with couplings to = e, µ as [21], where the operators are defined in Appendix C. Eq. (56) can be satisfied with C NPµ with the leptoquarks S 3 , or V 1,3 , respectively, and Simple flavor patterns such as the µ-isolation one L µ [7] can accommodate this   V 1,3 ). The values of κc ν and c ν are set to the upper limit allowed by kaon decays, induced at order c 2 ν κ 2 λ 2 and c 2 ν λ 2 , respectively. As c cannot be much larger a value of R K around (55) implies that the next round of LFV kaon and µ − e-experiments should see a signal. BSM effects as in Eq. (56) can therefore be accommodated naturally with S 3 , V 3 with both L µ andL µ -patterns. Both leptoquark models induce also LFV in charm, however, due to the constraints from the kaon sector, effects in charm are very small. In V 1 both left-and right-handed couplings are present. The latter, R µ (DE), moreover exhibits inverted flavor hierarchies, such that kaon decays are induced at order λ, which seem to rule out V 1 with µ-isolation patterns. However, as discussed in Section II, it is viable to flip the sign of the charges q(E). In this case the hierarchies in R µ (DE) would increase. Contributions to kaon decays arise at O(λ 9 ), which can be safely neglected. One-loop contributions to µ → eγ arise in V 1 from L µ · R µ andL µ · R µ , which are enhanced by the top mass.
One may employ the τ -isolation patterns of model V 3 discussed in the context of R D ( * ) in Section IV A 1 to predict b → sµµ processes. The resulting effects are very small, further VEV-suppressed for L τ (QL) as ∼ δ 2 c 2 λ 2 or constrained by b → sνν and low energy physics inL τ (QL) as ∼ δc c ν + c 2 ν λ 2 . In either case, the effects are by orders of magnitude too small to match Eq. (56).
We consider now leptoquarksS 2 and V 2 , which induce right-handed currents C µ 9 = −C µ 10 in b → s transitions. This is disfavored by global fits to data (excluding R K ) on b → s transitions, which suggests predominantly BSM in SM-type operators [52]. Let us nevertheless entertain this possibility as this line of research has not reached final conclusions yet. Right-handed currents would be signaled by R K = R K * [53], where R K * denotes the ratio of branching fractions of B → K * µµ over the one into electrons. This part of our work is sensitive to the FN-charges of the down quark singlets, q(D). Let us therefore be here more general than the benchmark Eq. (2) and introduce Explaining R K (first row) while obeying limits from K → µµ [34] (second row) strongly constrains the allowed values for the q i : which prefers q 1 ≥ q 3 + 2. By perturbativity and lower limits on M , q 2 + q 3 = 0, 1, 2, 3. This In supersymmetric or multi-Higgs extensions, a viable set reads q(D) = (q 3 + 1, q 3 , q 3 ), where q 3 = 0, 1, 2, 3, all of which are in mild conflict with Eq. (62). When the charges of the quark doublets and up-type quarks are also changed, two viable solutions are q(Q) = q(U ) = (3, 2, 0) and q(D) = (2, 0, 0) or q(D) = (3, 1, 1) [26]. Smaller charges generically give smaller VEVs. Choosing Similar to the situation for V 1 discussed previously, in V 2 rapid kaon decays arise through R µ (QE).
This can be avoided once the sign of q(E) is flipped. In this case the constraint from µ → eγ reads c δλ 3 10 −4 (M/TeV) 4 [3], which is always satisfied for perturbative δ.
We learn that improved bounds on kaon decays together with b → sµµ data can strongly constrain or rule out BSM models with flavor patterns. If solutions with down quark singlets can be ruled out, this leads to testable predictions, the equality of LNU ratios R K and R K * , as well as those of other b → s induced decay modes [53]. We checked that the impact of leptoquark models explaining R K at tree level on the observable B(B → D ( * ) µν)/B(B → D ( * ) eν) [54] is at permille level. We further recall that R K -explaining leptoquarks can induce percent-level contributions to b → sγ and subsequently b → s spectra [21], which can be accessed at a future high luminosity facility (with 75ab −1 ) [55].
LFV in b → s transitions related to R K [7,54,56,57] arises in the patterns studied in Eqs. (58) - (61). Relative to b → sµµ the effects on the amplitudes read TheL µ pattern predicts sizable LFV rates for leptonic and semileptonic B (s) -decays which can be searched for at future hadron colliders and e + e − -machines, see [7] for details, We investigate the implications of the flavor patterns studied in the previous sections for rare charm decays, K decays and µ − e-conversion.
Using [8] we with leptoquarks in flavor models, but the largest associated with models addressing R D ( * ) and R K .
In scenarioṼ 1 with the skewed pattern R µe (Ū E), which could have a large impact on rare charm decays, the FN-suppression of the (1, 2) element is not strong enough to effectively evade the µ − e conversion constraint, while, at the same time, keep the diagonal ones sizable. Similarly, effects in rare charm processes from , and negligible compared to the foreseeable experimental sensitivity. With the skewed pattern R eτ and leptoquarkṼ 1 µ−e conversion constraints can be evaded and c → ueτ transitions can be induced at order κκ λ 2 1 · 10 −3 . This leads to B(D → eτ ) 1 · 10 −13 .

V. CONCLUSIONS
We obtain patterns for leptoquark couplings to SM fermions based on flavor symmetries. In addition to those for lepton doublets [7], we find lepton isolation patterns for charged lepton singlets.
These are particularly relevant for contributions to R D ( * ) involving both chiralities. We argue on general terms that chirality-flipping contributions are generically larger than the ones based on SM-like operators involving doublet lepton couplings.
The flavor symmetry puts strong constraints on the leptoquark reach in flavor observables. We find that it is not possible to explain the present data on R D and R * D from tree level leptoquark exchange. The reason is that these BSM effects of few×0.1 are too large given lower mass bounds on the leptoquarks, perturbativity of the flavor symmetry breaking and flavor constraints, importantly, b → sνν, rare kaon decays and µ − e-conversion. We give predictions for R D , R D * and the τpolarization, which are summarized in Section IV A 4. At least the maximal leptoquark models, shown in Fig. 2, can be tested at Belle II with 50ab −1 [61].
On the other hand, R K together with the preferred global fit in b → s observables can be explained naturally using muon isolation patterns and S 3 , V 3 . If one abandons the constraints from the global fit, which prefers predominantly V − A-structure, modelS 2 accommodates as well a few×0.1 BSM effect in semileptonic b → sµµ processes.S 2 also predicts R K = R K * .
In our analysis we require the non-abelian flavon VEVs to remain perturbative, or we constrain In the SM, all Wilson coefficients C ν i vanish. Tree level contributions from leptoquarks are given in We use the CRunDec package [65] to evaluate α s . Assuming M ∼ 1TeV we find a modification of the Fierz relations between scalar and tensor operators, C S (M ) = ∓4C T (M ), at the b-and c-quark mass scale, µ b and µ c , respectively, where the minus sign (plus sign) refers to scenario S 1 (S 2 ). The overall running of C S and C T is negligible compared to the unknown O(1) coefficients of the flavor patterns and will not be considered further.
The branching fractions of B → D ( * ) ν decays can be written as where the coefficients A i and B i generally depend on the lepton and its polarization. Corresponding indices are suppressed in Eqs. (B8), (B9) to avoid clutter. The coefficients can be expressed in terms of hadronic matrix elements provided in Ref. [10]. Using lattice data from [35] for the B → D form factors and the HQET form factors from [10] for B → D * , we find the numerical values given in Tables VII and VIII by  Here we use the lifetime τ B 0 = (1.520 ± 0.004) · 10 −12 s of the B 0 meson [46]. In order to estimate the uncertainties, we draw 10 5 random samples of the form factor parameters provided in the respective references and calculate the coefficients A i and B i for each sample. The mean and standard deviation of the resulting distributions are then considered as the central value and uncertainty. We assume that the form factor parameters are normally distributed and incorperate all correlations provided by [10,35].
Additionally, we provide the coefficients for given τ -polarizations in Tables IX and X, where          −13 and C SM R is negligible. The strongest bound on new physics (NP) in b → sνν transitions is provided by B(B + → K + νν) < 1.7 · 10 −5 at 90 % CL [66], which, using [67], implies an enhancement over the SM of at most a factor of 4.3. Therefore, Solving this for a single, dominant diagonal coupling C NPνν