More flavor SU(3) tests for new physics in CP violating B decays

The recent LHCb measurements of the Bs → K−π+ and Bs → K+K− rates and CP asymmetries are in agreement with U-spin expectations from Bd → K+π− and Bd → π+π− results. We derive the complete set of isospin, U-spin, and SU(3) relations among the CP asymmetries in two-body charmless B → PP and B → PV decays, some of which are novel. To go beyond the unbroken SU(3) limit, we present relations which are properly defined and normalized to allow incorporation of SU(3) breaking in the simplest manner. We show that there are no CP relations beyond first order in SU(3) and isospin breaking. We also consider the corresponding relations for charm decays. Comparing parametrizations of the leading order sum rules with data can shed light on the applicability and limitations of both the flavor symmetry and factorization-based descriptions of SU(3) breaking. Two factorization relations can already be tested, and we show they agree with current data.


Introduction
One of the interesting open questions related to the Belle [1] and BaBar [2] data is the interpretation of the difference of CP asymmetries, A CP [B + → K + π 0 ] − A CP [B 0 → K + π − ] = 0.126 ± 0.022 [3]. This measurement is in tension with the results of calculations using an expansion about the heavy quark limit m b Λ QCD [4][5][6] (see, however, [7,8]). In contrast, the data do not present difficulties if flavor SU(3) symmetry is the only theoretical input used to relate the direct CP asymmetries.
We can hope to achieve a better understanding of the applicability and limitations of these approaches by exploring other relations for CP violation among charmless, two-body B decays. Such an understanding would not only enhance the ability of future B decay measurements to probe for new physics (NP) signals, but also improve our understanding of QCD. For example, the failure of an SU(3) relation at a larger than expected level may be due to a NP signal, and could tell us about the flavor structure of NP. Alternatively, if predictions of factorization fail, then undertanding as well as possible under what circumstances that occurs may in turn improve our understanding of the QCD dynamics. For JHEP01(2014)066 example, one might learn that the relative strong phase of the so-called tree and colorsuppressed tree amplitudes in the diagrammatic picture is large in some cases, despite being power suppressed in the heavy quark limit.
With these motivations in mind, the LHCb Collaboration has recently reported the first evidence of CP violation (CPV) in B s → K − π + decay [9]. This observation has been combined with existing data for B d → K + π − [10] to probe the SM through the parameter ∆ [11][12][13], for which the result is quoted as [9] ∆ = −0.02 ± 0.05 ± 0.04 . (1.1) Here the experimentally measured direct CP asymmetries, A CP , are defined to be where the initial state, i, is conventionally [3,10] a B meson containing ab quark, and In the SU(3) limit ∆ = 0, and thus a measurement of ∆ that deviates significantly from zero may indicate the presence of new physics. For example, such a deviation may arise from enhanced contributions to electroweak penguins. While the present experimental result is consistent with zero, one should also expect deviations from ∆ = 0 due to SU(3) breaking effects. The typical expected size of SU(3) breaking at the amplitude level, parametrized by ε, is of order (m s − m d )/Λ QCD or f K /f π − 1, both of which are O(20%). However, for relations between squared amplitudes, such as ∆, the typical SU(3) breaking should be 2ε, the factor of two arising from the Taylor expansion in ε. Taking into account an additional suppression factor of about 4, one expects ∆ ∼ 10%, in good agreement with the data. This suppression factor arises from a ratio of decay rates prefactor, which is a consequence of the definition of ∆.
In order to examine SU(3) breaking effects, parameters such as ∆ are poorly defined, as they not only carry an arbitrary normalization, but also unnecessarily introduce SU(3) breaking from phase space. A more suitable parameter for the study of SU(3) breaking is the properly normalized and defined combination of these rates and asymmetries, where we defined 5) and the data we used is collected in table 2 in the main text. Here δ CP is the asymmetry of the squared amplitudes for the CP conjugate decays, that is obtained by removing the i → f phase space factor, 1/P (i;f ) , from the rates. The p i→f is the center of mass JHEP01(2014)066 three-momentum of the final state particles; and m i denotes the initial B meson mass. It is advantageous to use ∆-like parameters instead of ∆ to parametrize SU(3) breaking, and we consequently express all SU(3) relations in terms of δ CP rather than ∆ CP . The numerical result in eq. (1.4), obtained using the most recent experimental data [3,9], is in agreement with the naïvely expected size of SU(3) breaking, ε. In refs. [11,12] five other U-spin relations were presented, which lead to testable parameters similar to ∆ or ∆. Recently, ref. [14] presented some SU(3) CP relations for B → P V decays (P denotes a pseudoscalar and V a vector meson). In the present paper, we extend the results of refs. [11,12,[14][15][16], by presenting the full set of SU(3) relations in terms of δ CP for mesons in both the mass and flavor basis, that is, with and without octetsinglet and neutral K meson mixing. We consider both B → P P and B → P V decays.
We further look for relations that hold to second order in SU(3) and isospin breaking by the quark mass spurion. We show that in the flavor basis, apart from isospin relations, there exists one CP relation for B → P P that holds beyond first order SU(3) breaking, and that this relation also holds beyond first order in isospin breaking. Once octet-singlet mixing is included, we find there exist no CP relations beyond first order in SU(3) breaking for either B → P P or B → P V , with the exception of isospin relations. In our analyses, we only consider effects that are first order in the weak interaction (e.g. we neglect electroweak penguins), since SU(3) breaking arising from the quark mass spurion is expected to be much larger than higher-order weak interaction effects.
In parallel to this analysis, we apply QCD and SCET factorization to study SU(3) breaking effects. In this approach, we may derive relations between different parameters that vanish in the SU(3) limit. At present there are two such relations that can be tested, and we show that they are in agreement with the currently available data. This paper is structured as follows. We first recapitulate the U-spin analysis, using the more compact Wigner-Eckart picture, and proceed to consider the effects of U-spin breaking by the strange quark mass. We then present ∆-type parameters for the charged mesons, and introduce natural, well-defined parameters for the characterization of U-spin breaking in CP relations. We derive factorization-based relations between some of these parameters and compare with current data where possible. Finally, we present the full set of SU(3) relations for both B → P P and B → P V decays. Similar relations that hold for the D meson decays are presented in an appendix.

CP sum rules
Let us first derive the Wigner-Eckart decomposition for direct CP asymmetries in the general group theoretic case. This decomposition is well-suited for expansions in symmetry breaking parameters.
We are interested in matrix elements of the form where P α denotes the final state mesons, B µ is the initial state and H is the effective Hamiltonian. The Wigner-Eckart theorem ensures that we can write these amplitudes in terms of reduced matrix elements, where X w are reduced matrix elements, and I w are group theoretic invariants, formed from the effective Hamiltonian, initial and final state tensors. In general, I w contain both strong and weak phases arising from the effective Hamiltonian, so it is convenient to write, without loss of generality, where χ q w,αβµ contain weak phases and group theoretic coefficients that depend on the particular initial and final states and the effective Hamiltonian, while σ q w are strong phases from the effective Hamiltonian alone.
The corresponding decay rate for each process is The symmetry factor 1/2 arises when the two final state particles are identical, which will be relevant in section 4. We are interested in relations involving the difference of CP conjugate square amplitudes, δ CP , which are pure group theoretic objects: they do not involve phase space factors. That is, we seek sum rules among Dropping explicit inclusion of the symmetry factor of 1/2, we then have Now, a CP sum rule is a symbol -i.e. an array of numerical coefficients -S such that It follows from eq. (2.6) that a sufficient condition for sum rules is S αβµ Im χ q * w,αβµ χ r v,αβµ = 0 . (2.8)

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That is, one needs only compute the kernel of χ q * w,αβµ χ r v,αβµ with respect to the basis of modes, indexed by αβµ. The structure of χ q * w,αβµ χ r v,αβµ is determined in part by the group theoretic indices w, v, which encode the group theoretic structure of the initial, final states and effective Hamiltonian. It is further determined by the strong phase indices q, r, which encode the strong phase structure of the effective Hamiltonian. However, the sum rules are independent from particular values of these strong phases. Moreover, the sum rules are independent from the reduced matrix elements X w , and consequently any strong phase structure carried by these.
In eq. (2.6), we also see that if the amplitude (2.2) for a CP violating mode involves n invariants, then the corresponding δ CP involves n 2 . It is therefore reasonable to expect that it is more difficult to obtain CP relations, compared with amplitude relations.

U-spin analysis
We may now present a compact recapitulation of the derivation of ∆ and other similar relations in the U-spin limit. Our results agree with those of [11,12], but are presented in a different way. In the remainder of this section we only consider decays into a pair of charged pseudoscalars, so that P α = (K, π) are the charged kaon or pion final states and First, the neutral B mesons furnish a U-spin anti-doublet while the two-particle final states furnish singlet and triplet U-spin representations, Next, the Hamiltonian is a ∆U = 1/2 operator. Using CKM unitarity it can be written in its most general form as Here λ j q ≡ V qj V * qb carry weak phases, and T and P are complex numbers containing strong phases. While the notation T and P is suggestive of 'tree' and 'penguin', we emphasize that certain penguins with the same weak phase and flavor transformation properties as the trees have been absorbed into H t .
The Wigner-Eckart theorem ensures that we can write the amplitudes in terms of two reduced matrix elements in the U-spin limit (cf., eq. (2.2)),

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where the summations over tensor indicies i and j are implicit. In the present U-spin case, since the Hamiltonian has only ∆U = 1/2 terms, we can further partition the amplitudes into the form where we have defined the following which we hereafter refer to as 'partial invariants', since they form part of the group theoretic invariants. Note for all charged meson final state and B initial state combinations, the partial invariants happen to have the property that We now have from eqs. (2.11) and (2.13), with w = 0, 1 in the U-spin limit. Applying eq. (2.6), we have χ 1,2 w = |T |λ j u C w,j , |P|λ j c C w,j , and σ 1,2 w = arg[T ], arg[P] so it immediately follows that where δ ≡ arg[P T * ], and we defined Contributions to δ CP are generated by interference between terms which carry a relative weak and strong phase. Here, the only such interference terms are cross terms between λ j u and λ k c , which is precisely the term that appears in eq. (2.17). Contributions such as Im[λ j * u λ k u ] or Im[λ j * c λ k c ] do not occur because eq. (2.15) enforces j = k, so these imaginary parts are zero.
Explicitly, the operator that generates CP violation

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Note that the off-diagonal terms of O CP are basis dependent, while the diagonal, Jarlskog, terms are independent of the choice of up-type quark basis for the Hamiltonian. That is, they are independent of which term is chosen to be eliminated when applying CKM unitarity. However, a consequence of eq. (2.15) is that the off-diagonal, basis dependent terms in eq. (2.19) do not appear in the physical relations, as desired.
The full set of the invariants, [M CP ] w,v , is shown on the left side of table 1 for B decays to charged mesons. From the general construction of CP sum rules in eq. (2.8), one may derive U-spin CP sum rules in the basis of amplitudes {A µ→αβ } by solving S αβµ [M CP ] w,v;αβµ = 0. That is, we need to find the null space of a matrix whose entries are the invariant matrices [M CP ] w,v;αβµ (see ref. [17] for analogous amplitude and rate sum rule constructions). For the present analysis, the U-spin relations may be read off table 1. For example, we have in the U-spin limit Explicitly, and applying eq. (2.17) yields In the U-spin limit, the phase space factors for both modes are the same, so that eq.
Finally, one may also see from table 1 that in the U-spin limit, we have two other relations, These relations generate other ∆-type parameters, discussed further in section 3.

First order U-spin breaking
U-spin breaking arises from the mass splitting between the d and s quarks, and may be encoded in the effective Hamiltonian by an expansion in a strange quark mass spurion. This spurion transforms as a U-spin triplet, with vacuum expectation value where ε parametrizes U-spin breaking.

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Decay mode U-spin limit U-spin breaking Table 1. Invariant matrices describing CPV in the U-spin limit and at first order in U-spin breaking in B d,s decays to K ± and π ± . The 2×2 (2×3) blocks should be read as matrices in indices w and v, that are multiplied on the left by leading order reduced matrix elements and on the right by leading (first order in U-spin breaking) conjugate reduced matrix elements to produce a contribution to the corresponding δ CP . For example, the top 2 × 2 block is multiplied on the left by (X 0 , X 1 ) and on the right by (X 0 , 12 ) † on the right (see eq. (2.26) for definitions of the subscripts), so that it contributes The CP asymmetry result in eq. (2.17) follows immediately from eqs. (2.11) and (2.13), which hold for arbitrary numbers of spurion insertions in the Hamiltonian. Hence eq. (2.17) holds to arbitrary order in U-spin breaking by this spurion: for each insertion we just gain more group theoretic invariants, indexed by w. In particular, the first order, O(ε), effects arise from a single insertion of this spurion into the effective Hamiltonian. This is equivalent to three new U-spin breaking partial invariants Furthermore, since [m s ] i j is diagonal, eq. (2.15) continues to hold, so the unphysical offdiagonal terms in O CP do not appear in CP asymmetries. As a consequence of this, and JHEP01(2014)066 applying eq. (2.17), the first order in U-spin breaking contributions to δ CP are The latter equality holds, because only the diagonal components of O CP are physical. The matrices M

Natural parameters
We see from Eq (2.20) that the ∆ parameter, defined in eq. (1.4), vanishes in the U-spin limit. In group theoretic notation and in terms of phase space factors, the ∆ parameter, quoted by LHCb and defined in eq. (1.1), has the form As mentioned above, in the U-spin limit the phase space factors are the same, so ∆ = 0, too. Furthermore, table 1 and eqs. (2.24) imply that there are two other ∆-type U-spin breaking parameters involving charged kaon and pion final states that vanish in the U-spin limit. If one were to enforce an analogy with eqs. (1.1) and (3.1), these parameters should be similarly written in the form Diagrammatically, the decays in Ξ only receive contributions involving W -exchange, penguin annihilation, or rescattering, which are power suppressed in the heavy quark limit. The B s → π + π − decay was observed recently [18], and its rate is probably much larger than B d → K + K − , which has not yet been seen with more than 2σ significance.

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The key point here is that the values of ∆, ∆ , and Ξ are not only determined by the U-spin breaking in the square amplitude relations (eq. (2.20) and its analogs (2.24)), but also by the ratios of decay rates and phase space factors. Such normalizations lead to additional enhancements or suppressions, so we expect that (3.4) The factors of two arise from the Taylor expansion in ε, the amplitude level breaking, of relations between squared amplitudes. The branching ratios collected in table 2 then imply that we should in turn expect With a canonical magnitude for U-spin breaking, ε ∼ 0.2, we then expect ∆ ∼ 0.10, in good agreement with the data shown in eq. (1.1). The recent first LHCb measurement, A CP [B s → K + K − ] = −0.14 ± 0.11 [19] and the world averaged [3,19], provides ∆ = −0.26±0.38, which agrees with the expectation ∆ ∼ 0.08.
(Note that ref. [19] , under the extra assumption |q/p| = 1.) These extra normalization and phase space factors render ∆, ∆ , and Ξ somewhat arbitrary parameters to characterize the magnitude of U-spin breaking. A set of better-defined quantities are In contrast with eq. (3.5), U-spin breaking with its canonical magnitude predicts For this reason, it is more natural to consider these parameters to study U-spin breaking. Recent data (see table 2 Both values are in agreement with U-spin breaking expectations.

Heavy quark limit and factorization
It has been shown that in the m b Λ QCD limit, the amplitudes of many B decays to pairs of light mesons can be factorized into calculable short distance factors: the B → X form
In the QCD factorization (BBNS) approach [4,21] the dominant contributions to the amplitudes with possibly large strong phases arise from power-suppressed effects, which are modeled. We find 12) or, in terms of the natural CP parameters,

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Here we used the simplified expressions adopted in ref. [21], and kept only the dominant source of direct CP violation proportional to α 1α c 4 , which is a good approximation numerically, since β c 3 is several times larger than β c 4 : see [4,21] for definitions. (Similar results were also stated in ref. [14].) One may then eliminate the form factors from eq. (3.12) to obtain where we used the numerical inputs collected in table 2. Alternatively, one can eliminate the form factors from eq. (3.13) to obtain, from the present value for ∆. These are in agreement with the recent LHCb measurements, that imply ∆ = −0.26 ± 0.38 and ∆ = 0.40 ± 0.34 respectively. The uncertainties are expected to be reduced significantly in the future.
In the SCET (BPRS) approach [5,22] (see also [23]) charm penguin amplitudes are described as unsuppressed nonperturbative quantities, A M 1 M 2 cc , where M 1,2 are the final meson states, while other amplitudes with strong phases (relative to the leading amplitudes) are O(α s , Λ QCD /m b ). If SU(3) breaking in the charm penguin amplitudes is small, then to a good approximation A Kπ cc = A ππ cc = A KK cc [22], so that one obtains eq. (3.13) with all the squares removed. Instead of eq. (3.15), we obtain  figure 1, compared with present data for these parameters. It shows that if factorization is a good approximation then ∆ and ∆ can only have comparable magnitudes in a relatively small region. In particular, if ∆ is close to zero, as is its central value with the current data, then ∆ should deviate from zero substantially if subleading corrections to factorization are small. We see in figure 1 that this factorization picture conforms with the current data, with the relations in eqs. (3.15) and (3.16) both intersecting the present 1σ confidence region for ∆ and ∆ . In contrast, observe that the U-spin limit prediction ( ∆, ∆ ) = (0, 0) does not agree as well with the current data; as already shown in eqs. (3.9) and (3.10), the prediction including first order U-spin breaking effects is in concordance with the data. Future comparisons of ∆ and ∆ with these relations will probe the factorization picture with greater precision. Note that no serious lattice QCD calculation of the B s → K form factor exists yet, and these tests of factorization should increase the motivations for such a calculation (besides the hope of measuring |V ub | at LHCb fromB s → K + eν).
Due to the lack of leading order contributions to the amplitudes in Ξ in the heavy quark limit, and the complexity of the contributing power-suppressed terms (see also ref. [24] and referenecs therein), this U-spin relation may be expected to receive larger corrections, and Ξ is expected to deviate from zero more significantly than ∆ and ∆ . If Ξ is measured in the future to be comparably close to zero as ∆ or ∆ , that would be a success of SU(3) flavor symmetry, and be puzzling from the point of view of the heavy quark limit.

SU(3) relations
Let us now proceed to consider full SU(3) and the CP relations that hold to zeroth and first order in SU(3) breaking. We do not make any assumptions about the size of the hadronic reduced matrix elements (see, e.g., ref. [25] for such studies). However, we do make one assumption that goes beyond flavor SU (3): we only consider effects that are first order in the weak interaction. In practice, this amounts to neglecting electroweak penguin operators and b → dds-type decays. This is well-justified as corrections from higher order weak interactions corrections are expected to be smaller than those from the SU(3) breaking induced by the quark mass spurion.

B → P P
We consider first B decays to two pseudoscalars. The initial states furnish a flavor antitriplet, and the final states an octet and singlet The effective Hamiltonian is a four-quark current-current tensor operator, in which q i = (u, d, s) T and q = c, b. The terms corresponding to charmless decays transform as 3 ⊗3 ⊗ 3 = 3 ⊕ 3 ⊕6 ⊕ 15. Enforcing charge conservation together with CKM unitarity, the non-zero, independent components of each irrep are Here X and Y are O(1) complex numbers. As already mentioned we work to first order in the weak interaction and thus in eqs. (4.3) we have neglected electroweak penguin operators as well as operators of the form (qq )(db) with q = q . It is this assumption that is responsible for the fact that the6 and 15 do not have terms proportional to V * cb V cd . Note that the extra penguin operator (q q )(q ib ) in (4.2) furnishes a triplet proportional to the 3, and is therefore subsumed by eqs. (4.3).
Applying the Wigner-Eckart theorem, as in section 2.1 and in particular eq. (2.6), and assuming an arbitrary mixing angle between the η and η mass eigenstates, we now present all possible SU(3) CP relations. The first two are due to isospin The next eight use only U-spin, of which the first three are the familiar charged meson relations from section 2.2, and the last two require full SU(3) The six relations (4.4c)-(4.4h) correspond to those found in refs. [11,12], while the first two relations, (4.4a) and (4.4b), are isospin relation previously presented in refs. [26,27]. The relations (4.4i)-(4.4l) are, to our knowledge, novel to this work. (For completeness, in appendix A we present relations in the flavor basis. One may check these are consistent with the SU(3) decompositions contained in ref. [15].) It should be noted that we have chosen to present these sum rules in a particular basis, such that the U-spin and isopsin sum rules are manifest. Of course, any linear combination of these sum rules is also a sum rule. Let us now incorporate K 0 -K 0 mixing. Since we work to first order in the weak interaction, we neglect CPV effects in K 0 -K 0 mixing and also neglect operators which produce b → dsd -type decays. Within this approximation, for each non-zero mode B → K 0 X (B →K 0 X) the corresponding conjugate mode B →K 0 X (B → K 0 X) is zero. Here X denotes all pseudoscalar mesons with correct charges and B denotes B d , B s , or B + as appropriate. It follows that for all pseudoscalar mesons X. One further obtains the following relations for all pseudoscalar mesons X = K S,L with correct charges. Note that these relations arise from the properties of K S,L , rather than from SU(3) symmetry. In order to rotate to the K meson mass basis, we see from eq. (4.5) that we need only replace K 0 andK 0 in each of eqs. (4.4) by K S (or K L ), with an extra factor of two in front of the corresponding δ CP . Thus, in the mass basis we obtain the isospin relation (4.6c) and the U-spin relations where X 0 = π 0 , η, or η . The six relations in eqs. (4.7) The isospin relations should hold to all orders in breaking by m sm s does not further break isospin -but are clearly sensitive to isospin breaking. In the flavor basis, we find that the isospin relations (4.4a) and (4.4b), together with hold to O(ε 2 ). Furthermore, we find that eq. (4.8) holds to second order in isospin breaking. This is result is novel to this work: while such a CP relation is untestable, it is interesting to note such a relation exists in principle, given the large number of cancellations required among the group theoretic invariants.
In the presence of η-η mixing, we find that only the isospin relations (4.4a) and (4.4b) hold to O(ε 2 ). If one includes K 0 -K 0 mixing, then the relations (4.4a) and (4.6c) hold to O(ε 2 ), along with the mixing relations (4.6a) and (4.6b), which do not arise from SU(3). Once isospin breaking is introduced, there exists no CP relation that survives at first order. In summary, the B → P P isospin relations (4.4a) and (4.6c) are expected to hold to the O(1%) level, while all other mass basis CP relations should fail at O(ε).

B → P V
We may also derive CP relations for charmless two-body B decays to a pseudoscalar and a vector meson. It should be noted that, experimentally, these decays are measured via construction of Dalitz plots, and it is not always possible to identify the P V final state.
The vector mesons furnish an SU(3) singlet and octet, the B and pseudoscalars furnish the same representations as in eq. (4.1). The effective Hamiltonian (4.3) and strange quark spurion (4.7) are unchanged. Assuming ideal mixing between the ω and φ mass eigenstates, such that φ is pure ss, and arbitrary mixing between η and η , one finds eighteen relations, corresponding to the following zero sums. This first three are isospin relations

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The next ten are generated by U-spin Finally, there are a further five SU (3) relations Note that the K * 0 andK * 0 can be tagged, so we need not consider K * -K * mixing. (As for the B → P P case, in appendix A we present relations in the flavor basis. These are consistent with the SU(3) decompositions contained in ref. [15].) Including K 0 -K 0 mixing with the same approximations as in section 4.1, leads to a further twelve relations that do not arise from SU(3). Just as for the PP case, eq. (4.5) holds for all vector mesons X, so that the SU(3) CP relations for kaon mixing are obtained by replacing all the K 0 andK 0 mesons in eqs. (4.10) with K S , and including an extra factor of two in front of the corresponding δ CP . In particular, eq. (4.10c) becomes

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We find that only the three isospin CP relations, eqs. (4.10a)-(4.10c), hold to second order in SU(3) breaking by the strange quark mass spurion, with or without η − η mixing. Including kaon mixing, the relation (4.10c) is replaced by eq. (4.12). Finally, with or without mixing, no CP relations hold at first order in isospin breaking. Similarly to B → P P , we conclude that the three B → P V isospin relations (4.10a), (4.10b) and (4.12) are expected to hold to the O(1%) level, while all other mass basis CP relations should fail at O(ε).

Conclusions
New data on B s decays and CP asymmetries have made it possible to test several U-spin and SU(3) relations. We have derived the complete set of leading order isospin, U-spin, and SU(3) CP relations, some of which are novel to this work. We further found that there are no relations for CP asymmetries that hold at first order in SU(3) breaking, except for isospin relations. These latter relations fail at first order in isospin breaking. While isospin relations are expected to hold at the percent level, this is not the case with SU(3) relations, where the breaking effects are expected to be ∼ 20%.
For the purposes of parametrizing SU(3) or U-spin breaking with these relations, one must construct parameters that are properly normalized. Furthermore, the CP relations themselves are formally constructed in terms of the phase space-stripped decay rate splittings, δ CP , which are well-defined in a group theoretic sense, rather than in terms of the decay rate splittings, ∆ CP . Therefore, any such parameters that are designed to test the breaking of flavor symmetries should be similarly constructed in terms of δ CP , becuase they do not admit extra breaking from phase space factors.
Factorization at leading order in the heavy quark limit predict relations between the U-spin parameters ∆ and ∆ , given in eqs. (3.15) and (3.16) and shown in figure 1. We see that these factorization-based descriptions of U-spin breaking are in good agreement with the data. We hope that future data will test this picture with better precision.
From the flavor symmetry point of view, a third parameter Ξ, defined in eq. (3.8), is on the same footing as ∆ and ∆ : we expect corrections of O(ε). However, while the modes relevant for ∆ receive leading contributions in the heavy quark limit, those in Ξ are power suppressed. Hence in the factorization picture, Ξ may be expected to receive larger SU(3)-breaking corrections. Thus, measurements of these parameters will help us understand which theoretical tools are reliable.
In terms of future study, we have considered here only two-body decays. While this is appropriate for decays into two pseudoscalars, B → P V decays are measured through Dalitz analyses. The Dalitz plots include the dominant resonance regions, but also other features, such that a full study of the B → 3P decays would be well-motivated.

A CP sum rules in flavor basis
In this appendix we present CP sum rules in the flavor basis, that is, without K-K, or singlet-octet mixing. Clearly, these cannot be tested experimentally, but we include them here for the sake of completeness.
There are 19 linearly independent B → P P sum rules in this basis, namely, Similarly, there are 32 linearly independent B → P V sum rules in the flavor basis, which are,

JHEP01(2014)066 B Charm decays
Similarly to B decays, we can compute CP relations for charmless D → P P and D → P V . In this case, the initial states furnish an SU (3)  The charmless terms transform as3 ⊗ 3 ⊗3 =3 p ⊕3 t ⊕ 6 ⊕15. Enforcing QED charge conservation together with CKM unitarity, the non-zero, independent components of each irrep are Here X is an O(1) complex number. Penguin contributions carrying strong phases arise purely in the3 irreps, and note that the [3 t ] and3 irrep produced by the charm term in eq. (B.1) are both subsumed by [3 p ]. One finds, including η-η and K 0 -K 0 mixing, the following leading order D → P P CP relations. There are two U-spin relations,  3a) is a well-known U-spin relation [29]. No SU(3) relations hold at first order in breaking by the strange quark mass spurion or isospin breaking, with or without mixing.

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Similarly, for D → P V , we have, in the presence of neutral meson mixing, five U-spin relations Once again, no SU(3) relations hold at first order in breaking by the strange quark mass spurion or isospin breaking, with or without mixing.
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