CP violation tests of alignment models at LHCII

We analyse the low-energy phenomenology of alignment models both model-independently and within supersymmetric (SUSY) scenarios focusing on their CP violation tests at LHCII. Assuming that New Physics (NP) contributes to K0−K¯0\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {K}^0-{\overline{K}}^0 $$\end{document} and D0−D¯0\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {D}^0-{\overline{D}}^0 $$\end{document} mixings only through non-renormalizable operators involving SU(2)L quark-doublets, we derive model-independent correlations among CP violating observables of the two systems. Due to universality of CP violation in ΔF = 1 processes the bound on CP violation in Kaon mixing generically leads to an upper bound on the size of CP violation in D mixing. Interestingly, this bound is similar in magnitude to the current sensitivity reached by the LHCb experiment which is starting now to probe the natural predictions of alignment models. Within SUSY, we perform an exact analytical computation of the full set of contributions for the D0−D¯0\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {D}^0-{\overline{D}}^0 $$\end{document} mixing amplitude. We point out that chargino effects are comparable and often dominant with respect to gluino contributions making their inclusion in phenomenological analyses essential. As a byproduct, we clarify the limit of applicability of the commonly used mass insertion approximation in scenarios with quasi-degenerate and split squarks.


Introduction
The meson systems are among the most interesting low-energy probes of New Physics (NP) and can be regarded as golden channels of the high intensity frontier. However, all the currently available data on K and B d,s systems agree well with the Standard Model (SM) predictions. In turn, this leads to the so-called NP flavor and CP puzzles, that is the tension between the solution of the hierarchy problem, requiring a TeV scale NP, and the explanation of the flavor physics data.
One option to reconcile the above tension without giving up on naturalness is to assume that NP is flavor blind. This could either arise when the flavor mediation scale is very high leading to minimal flavor violation [1][2][3][4][5][6], or possibly when non-abelian flavor symmetries are involved [7]. In both cases, however, flavor non-universality effects involving the first two generations are suppressed, both in the luminosity and energy frontiers (see, e.g., [6,8,9]).
However, another possibility regarding the flavor structure of NP might be realised in Nature. This is due to the fact that most of the information that we have involving low-energy, flavor violating, probes of the SM involve down type fermions. Thus, there is always the possibility that new physics is in fact at the TeV scale and yet it is aligned with the down type Yukawa matrices [10][11][12][13][14]. In such a case flavor universality in the first two JHEP02(2016)178 generations is badly broken, leading to several interesting signatures at the LHC [14][15][16][17]. Somewhat surprisingly such a framework might even be linked to the hierarchy problem leading to flavorful naturalness [18].
In all above cases, D physics observables represent a unique tool to probe NP flavor effects, quite complementary to tests in K and B systems. On general grounds, D systems offer a splendid opportunity to discover CP violating effects arising from NP [19][20][21][22][23] as the SM predictions are expected to be of order O(V * cb V ub /V * cs V us ) ∼ 10 −3 . As a consequence, any experimental signal of CP violation in D 0 −D 0 above the per mill level would probably point towards a NP effect.
In this work, we revisit the phenomenology of alignment models model-independently as well as within SUSY scenarios. Assuming that NP contributes to K 0 −K 0 and D 0 −D 0 mixings only through non-renormalizable operators involving SU(2) L quark-doublets, we derive model-independent correlations among CP violating observables of the two systems. At this era of the beginning of the second run of the LHCb we can safely assume that CP violation effects in the D system are small and thus many of the theoretical expressions are simplified, as we are allowed to work at the linear order in the CP violating parameters.
We briefly summarise here our findings related to the model-independent analysis: i) generically the bound on the allowed amount of CP violation in the Kaon system limits the possible size of CP violation in mixing in the D system; ii) this bound is similar in magnitude to the current sensitivity reached by the LHCb experiment. As such, a discovery of CP violation in D-mixing would be quite challenging for alignment (and many other) models; iii) the expected resolutions at the next LHCb run, as well as other potential experiments, will provide useful information on the parameter space of models where CP violation is controlled dominantly by the left-handed sector.
Then, we focus on SUSY alignment models and the main goals of our study are: i) to perform an analytical computation of all SUSY contributions (pure gluino, mixed neutralino/gluino, chargino, as well as neutralino contributions) for the D 0 −D 0 mixing amplitude; ii) to study the allowed ranges for the squark masses which are compatible with both collider and flavor physics constraints; iii) to study the allowed effects for charm-CPV pointing out possible correlations among D and K meson observables enabling to probe or falsify the NP scenario in question; iv) to clarify the limit of applicability of the commonly used Mass Insertion (MI) approximation comparing the full and approximated results in two relevant squark mass regimes: the quasi-degeneracy and split scenarios.
Our paper is organized as follow: in section 2 we review the main formalism and formulae for D 0 −D 0 mixing observables. In section 3, we derive model-independent JHEP02(2016)178 correlations among CP violating observables related to D 0 and K 0 systems. Section 4 is devoted to the calculation of the D 0 −D 0 mixing amplitude in SUSY, while the study of charm-CP violation is presented in section 5. Our main results and conclusions are summarized in section 6. Finally, in appendix A and B we specify the notation used in the text and report the loop functions, respectively.
The D 0 −D 0 mixing amplitude can be described by means of the dispersive (M 12 ) and the absorptive (Γ 12 ) parts as follow [19][20][21][22][23][24] The mass eigenstates D H,L for the neutral D meson systems are linear combinations of the strong interaction eigenstates, D 0 andD 0 The normalized mass difference x and width difference y are given by with τ = 1/Γ D = 0.41 ps [25] being the neutral D life-time and Γ D the average decay width of the neutral D mesons: The mass difference ∆M D is always taken to be positive by definition. However, the sign of ∆Γ D is physically meaningful. Note that, our definition of ∆Γ D is consistent with the HFAG convention [26].
In addition, we define the decay amplitudes to final state f as The deviation of |q/p| from unity corresponds to CP violation in mixing. An example of this type of CP violation is the semileptonic decay asymmetry to "wrong sign" leptons a SL When the final state f is a CP eigenstate f CP (e.g., π + π − , K + K − ), a CP violating asymmetry A Γ can be constructed taking the difference of the "effective decay width The above expression has been obtained assumingĀ f /A f = 1 and working to linear order in the CP violating parameters. In the absence of direct CP violation A Γ and a SL (or sin φ) are correlated by the model-independent relation [21,27,28] As far as the experimental situation is concerned, the most recent fit results from the UTfit collaboration are collected in table 1. Even if D 0 −D 0 mixing is now firmly established experimentally, there is no evidence yet for CP violation. In particular, current data are

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compatible with the hypothesis of CP conservation, i.e. |q/p| = 1 and φ = 0 to a better than 10% accuracy. This justifies our linear expansion of CP violating quantities. Eq. (2.9) can be further used to constrain the phase of a heavy NP. We shall assume here that the SM contributions are dominated by the first two generations and thus can be brought to be real without loss of generality. Thus, any CP violation can only arise due to the presence of an imaginary component of the dispersive part of the ∆c = 2 amplitude, Im (M 12 ) , see [20,23] for more details. NP effects for D 0 −D 0 mixing can be described in full generality by means of the ∆F = 2 effective Hamiltonian where C i are the Wilson Coefficients (WCs) of the operators Q i given by where P R,L = 1 2 (1 ± γ 5 ) and α, β are colour indices. The operatorsQ 1,2,3 , which we have omitted, are obtained from Q 1,2,3 through the replacement L ↔ R.
For the calculation of the observables, we have used the hadronic matrix elements and the magic numbers from [30].

Model-independent analysis
In general, NP effects for ∆F = 1, 2 transitions in the up-and down-quark sectors are unrelated. As such, the very stringent constraints arising from FCNC processes like / or K do not necessarely imply similar constraints on FCNC processes involving D mesons. Yet, there are many NP scenarios in which the dominant effects are encoded in operators involving only the quark-doublet q L . In such cases, FCNC contributions for K and D meson systems stem from the fermionic bilinear q L γ µ q L and therefore are approximately SU(2) L invariant [31].
Focusing on these scenarios, the relevant ∆F = 1, 2 operators are, respectively

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where O µ = q qγ µ q, γ µ , etc. Since X is an hermitian matrix it can be diagonalised through a unitary matrix V as X = V †X V whereX = diag(X 1 ,X 2 ) andX 1,2 are the eigenvalues of X. In the down mass basis it turns out that where c K (z K ) and c D (z D ) are related through the CKM matrix V CKM as follow Working in a two-generation framework, which is appropriate for our purposes, V CKM and V can be parametrised as follows As a result, the coefficients c K(D) governing ∆F = 1 transitions read In particular, the relation Im c K = Im c D implies that, within our framework, CP violating effects in ∆F = 1 transitions are universal in the up-and down-quark sectors, in agreement with [32]. Passing to ∆F = 2 transitions, we find the following results Let us simplify the above expressions remembering that cos θ C ≈ 1, sin θ C ≈ λ C ≈ 0.22 and taking the limit of almost alignment where θ q 1. We find that (3.14) The expressions above show that CP violating effects entering K and D meson systems are not universal for ∆F = 2 transitions. Yet, it is still possible to obtain a model-independent upper bound for charm CP violating effects. In order to see this, we notice that that above relations imply where the upper bound on |Im z D | has been obtained assuming the bounds on |Im z K | and |Re z D | from refs. [33] and [34], respectively. Since we are interested in a relation among physical observables, we exploit the model-independent results of the previous section in the limit of small CP violation. In particular, from eq. (2.9) and (2.10), and remembering that in D-physics we are interested in the two generation limit, where all the SM couplings can be made real without loss of generality, we have As a result, it is straightforward to find the following expression for |A Γ |  Table 2. Lower and upper bounds on SUSY flavor mixing angles in alignment models [12].
where ∆ K ∼ Im z K . Finally, imposing the experimental bounds on x and ∆ K , we can find the desired theoretical upper bound for |A Γ | in agreement with the bound quoted in ref. [33]. Therefore, the current experimental resolutions (see table 1) are testing right now the natural predictions of alignment models.
In figure 1 on the left, we show the model-independent correlation between A Γ and ∆ K within alignment models. As we can explicitly see, positive NP effects for ∆ K at the level of 20% − 30% (which would even improve the current UTfit analyses) naturally imply values for A Γ close to the present bound A Γ 4.4 × 10 −4 . In figure 1 on the right we show also the correlation between Im C D  We shall now move to consider SUSY alignment models [10,11]. It amounts to aligning the squark and quark mass matrices either in the up-or down-sector, so that FCNC effects are kept under control without requiring any degeneracy in the squark spectrum.
As argued in ref. [12], within alignment models it is possible to predict both lower and upper bounds for the SUSY flavor mixing angles (s q M ) ij entering the couplingsg−q M i −q M j , with M = L, R. In particular, by making use of holomorphic zeros in the down quark mass matrix to suppress the mixing angles of the first two generations, one can find the predictions of table 2.
The most prominent feature of these models is the appearance of a large left-handed mixing between the first two families. In particular, in the so-called super-CKM basis, the left-handed squark mass matrices are related by the SU(2) L relation M 2 u,LL = JHEP02(2016)178 A leading order expansion in the Cabibbo angle leads to the following expression Therefore, even assuming a perfect alignment in the down sector, that is (M 2 d,LL ) 21 = 0, we always end up with a large flavor violating entry in (M 2 u,LL ) 21 proportional to λ C as long as the left-handed squarks are non-degenerate.
The usual prescription is to start from eq. (4.1) and define the following MI [35] ( where, considering only the first two generations, (δ L u,d ) 21 , ξ and mq read Here, M 2 Q is the squark mass matrix squared for the left-handed squark-doublets. As a result, flavor constraints translate into constraints on SUSY masses and the mass splitting parameter ξ. If the mass splittings among squarks is sizable, i.e. ξ ∼ 1, the MI approximation is not in general a good approximation, as we will discuss quantitatively in the following.
The main goal of the following section is twofold: • to derive exact analytical expressions for C i , see eq. (2.11), working in a twogeneration framework and performing an analytical diagonalization of the squark mass matrices. We account for the full set of SUSY contributions which include pure gluino, mixed neutralino/gluino, chargino, as well as neutralino effects; 3 • to derive the expressions for C i in the MI approximation in two relevant limits for the squark masses: the quasi-degeneracy and split scenarios, clarifying the extent to which the commonly used MI approximation (so far known only for the gluino contributions) agrees with the exact computation.

Full results
In the following, we provide the relevant expressions for C i andC i in SUSY alignment models under the following approximations: 1. we work in a two-generation framework. Such an approximation is justified if the underlying c → u transition is not significantly affected by flavor mixings with the third generation, that is if the direct c → u transition dominates over the double flavor transition (c → t) × (t → u). This is an excellent approximation in alignment models, as one can check from table 2; 2. we neglect the small Yukawa couplings for the first two generations and therefore the corresponding LR/RL soft terms while we keep the full dependence on the chargino and neutralino mixings; 3. we neglect U(1) Y interactions since they are safely negligible compared to SU(2) L interactions, as we have explicitly checked numerically.
The most important effects for D 0 −D 0 mixing in alignment models arise from the operators Q 1 and Q 4,5 since their (different) sensitivity to the large MI (δ L u ) 21 ∼ λ C . Our results for C 1 are given by the following expressions where a sum over the indices a, b = 1, 4 (for neutralinos) and a, b = 1, 2 (for charginos) is undesrtood. The matrices Z N and Z − , which stem from the diagonalization of the chargino and neutralino mass matrices, as well as the mixing angles s L c L e iφ L are defined in appendix A while the loop functions B(x, y) and C(x, y) are defined in appendix B. The WCs C gg stand for the pure gluino, chargino, neutralino, and mixed neutralino/gluino effects, respectively.
If in addition to left-handed mixings right-handed mixings might also be present, thus for completeness we present the relevant functions,C 1 and C 4,5 10)

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Notice that C 2,3 andC 2,3 are vanishing in the limit of vanishing LR/RL flavor mixings, which we assume. Few comments are in order: • Cgg 1 , C χ 0 χ 0 1 , and Cg χ 0 1 receive two contributions, corresponding to crossed and uncrossed gluino and/or neutralino lines, as a result of the Majorana nature of the gluino and neutralinos. Such contributions have opposite sign and therefore tend to cancel to each other, the extent of cancellations depending on the parameter space. By contrast, C χ + χ + 1 is not affected by any cancellation since charginos are Dirac particles and therefore there are no crossed diagrams for C χ + χ + 1 .
• Even if C χ + χ + 1 is parametrically suppressed compared to Cgg 1 by a factor of α 2 w /α 2 s ≈ 1/10, it might still provide important/dominant effects whenever the gluino is sufficiently heavier than squarks and charginos or when the above cancellations in Cgg 1 are significant. Similar comments apply also to the case of C χ 0 χ 0 1 , as long as we are far from the cancellation regions for C χ 0 χ 0 1 . Finally, Cg χ 0 1 can also provide significant effects especially when Cgg 1 (but not Cg χ 0 1 ) is suppressed by large cancellations. 4 • Assuming the upper and lower bounds for the flavor mixing angles of table 2, we find that C 1 ∝ (ξλ C ) 2 while C 4,5 ∝ ξλ 3−5 C and therefore ξ/λ C |C 1 |/|C 4,5 | ξ/λ 3 C . Taking into account that Q 4,5 have larger hadronic matrix elements than Q 1 and that QCD runnings further enhance C 4,5 with respect to C 1 , it turns out that the contributions of C 4,5 to the D 0 −D 0 mixing amplitude are very important even for ξ ∼ O(1).
• In the limit of complete alignment, i.e. for (M 2 d,LL ) 21 = (M 2 u,RR ) 21 = 0, CPV effects in D 0 −D 0 mixing are vanishing [40]. Possible CPV sources can arise only in the presence of a misalignment either in the LL or RR sectors. In the former case, the underlying SU(2) L symmetry links CPV effects in D-and K-meson systems. In the latter case, the above CPV effects are generally unrelated.
• Naively, one would expect that flavor violating sources in the LL up-squark sector are felt by the down sector through chargino up-squark contributions. However, the chargino amplitude is such that Aχ ij ∼ (V † M 2 u,LL V ) ij ≡ (M 2 d,LL ) ij and therefore down-quark FCNCs turn out to be sensitive to M 2 d,LL and not M 2 u,LL [40].  Here, we have neglected the mixings in the chargino and neutralino mass matrices keeping only the dominant pure Wino contribution (see the following section for more details). On general grounds, from figure 3 we learn that there is a very significant sensitivity on the Wino mass M 2 . In turn, this means that chargino/neutralino effects are extremely important and therefore their inclusion in phenomenological analyses of SUSY alignment models is mandatory.

No chargino/neutralino mixing
The expressions of the Wilson coefficients C χ + χ +  breaking, Higgino/Wino mixings will induce corrections to the pure Wino contribution of order v 2 /max(µ 2 , M 2 2 ) which are sizable only for relatively light Higgsinos and Winos. Thus, the leading chargino/neutralino and gluino-neutralino contributions, as obtained by neglecting chargino/neutralino mixings and U(1) Y interactions, are given by the compact expressions 14)

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Eqs. (4.13)-(4.15) together with the expressions of Cgg 1,4,5 andCgg 1 of section 4.1, provide the full set of Wilson coefficients describing D 0 −D 0 mixing. These expressions, which provide an excellent approximation of the full results of section 4.1, are entirely expressed in terms of physical parameters, i.e. masses, mixing angles and CPV phases, and do not require any numerical diagonalization of the squark and chargino/neutralino mass matrices to be used.

21)
where x gq = m 2 g /m 2 q , x wq = M 2 2 /m 2 q , and the loop functions f 6 (x),f 6 (x), f 6 (x, y), and f 6 (x, y) are given in the appendix. The above expressions extend the results of Gabbiani et al. [36] where only the pure gluino contributions were considered.

Split squarks
When the squark mass splittings are sizable, the results obtained in the MI approximation are not trustable. As an illustrative example, we consider the limit of split squark families where it is assumed that the heaviest squark is completely decoupled, i.e. mq 1 → ∞. In this scenario, the prescriptions for (δ L u ) 21 and (δ R u ) 21 are (4.24) Starting again from the full results of section 4.1, we end up with the following expressions where x gq = m 2 g /m 2 q 2 , x wq = M 2 2 /m 2 q 2 , and the loop functions D 0,2 (x) are defined in the appendix.
In the limit of mq 1 → ∞, the Wilson coefficients of eqs. Our numerical results confirm that neutralino/chargino mixing effects are indeed rather small. Yet, we find that for light Wino and Higgsino, (M 2 , µ) v, corrections up to 50% are still possible. On the other hand, for large squark mass splittings, we observe significant departures of the MI approximation from the exact results. This is also evident in the right plot where we show the ratio between x in the MI approximation, x MI , and in the full computation, x full , as a function of |ξ|: for |ξ| 0.1 the two computations nicely agree while they can differ very significantly for |ξ| ∼ O (1).
Concerning the case of split-squarks, we have explicitly checked that the MI approximation formulae reproduce quite accurately the full results provided |ξ| 0.6.

CPV in D 0 −D 0 mixing
We are ready now to analyse possible CPV effects for D 0 −D 0 mixing in SUSY alignment models. On general ground, we notice that in the limit of complete alignment, that is for (δ L d ) 21 = (δ R u ) 21 = 0, CPV effects in D 0 −D 0 mixing are vanishing as (δ L u ) 21 , which is the only source of flavor violation can be taken to be real without loss of generality [40].
On the other hand, possible CPV sources stem from (δ L d ) 21 and/or (δ R u ) 21 . In the former case, CPV effects in D 0 −D 0 and K 0 −K 0 mixings are correlated due to the underlying SU(2) L symmetry and the leading effects are generated through the SM operator Q 1 , see eq. (2.12). By contrast, in the latter case, the effects in D 0 −D 0 and K 0 −K 0 mixings are not correlated and the leading effects for D 0 −D 0 arise typically from the operator Q 4 .
For a qualitative understanding of CPV effects in D 0 −D 0 mixing, it is convenient to consider the CPV phase in the mixing in the approximation that the SM contributions are dominated by the first two generations and are made real, as explained above, see eqs. (2.9), (2.10) and (3.16). In that case we can bound the amount of CPV by setting the contributions of the SM to M 12 to zero (not allowing for accidental cancellations) hence in the following M 12 is assumed to be totally dominated by the NP contributions. In this case we can write (omitting for simplicity the SM ∈ Real subscript in (3.16)) Again, we emphasise that it is assumed that M 12 = M NP 12 , to maximise the contributions. We are going now to analyse two distinct cases where either (δ L d ) 21 = 0 and (δ R u ) 21 = 0 or (δ L d ) 21 = 0 and (δ R u ) 21 = 0 outlying their peculiar phenomenological features.

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where the first approximation is valid at the leading-order expansion in (M 2 u,LL ) 21 while the last one, obtained by using eqs. (4.1)-(4.2), is valid for Re(δ L d ) 21 4λ C ξ. Interestingly, eq. (5.2) shows that, for a given value of x, the largest effects in A Γ are expected for small values of ξ, i.e. for relatively degenerate squarks. The maximum value for A Γ is found by imposing the constraints from K and x which have the following parametric expressions In particular, in the quasi-degenerate scenario (see section 4.2.2) and assuming that gluino effects are dominant, we end up with the following estimates where we have set m g =m Q = 1 TeV, (δ L d ) 21 = e iφ L |(δ L d ) 21 |, and assumed again that Re(δ L d ) 21 4λ C ξ. Therefore, imposing the constraint |∆ K |/ SM K 0.4, and setting φ L = 45 • , we find the upper bound as confirmed by the lower plot on the right of figure 5. Notice that A Γ ∼ sin φ L while ∆ K ∼ sin 2φ L and therefore the constraint from ∆ K can be relaxed for φ L ≈ 90 • while maximizing A Γ .
2. (δ L d ) 21 = 0 and (δ R u ) 21 = 0. In this case we find that where the first approximation holds in the limit where Re (δ L u ) 21 (δ R u ) 21 Re (δ L u ) 2 21 . Comparing eq. (5.2) with eq. (5.6), we learn that (δ R u ) 21 is potentially much more effective than (δ L d ) 21 to generate large CPV effects in D 0 −D 0 mixing. In particular, for Im(δ R u ) 21 ≈ Im(δ L d ) 21 (notice that in alignment models (δ R u ) 21 might be even larger than (δ L d ) 21 , see table 2) the effect driven by (δ R u ) 21 is typically more than two orders of magnitude larger than that from (δ L d ) 21 . The reason of this can be traced back remembering that C 4 is highly enhanced with respect to C 1 by a larger hadronic matrix element, larger QCD-induced RGE effects, and also by a larger loop function. Moreover, from a pure phenomenological perspective, we remember that (δ R u ) 21 does not suffer from the K 0 −K 0 mixing constraints, in contrast with (δ L d ) 21 .
In figure 5, we show the predictions for A Γ vs. ∆ K (upper plots) and A Γ vs. ξ (lower plots) in the case 1. The plots on the left (right) include only EW-ino (gluino) effects. Green, red and black points correspond to arg(δ L d ) 21 = 20 • , 45 • , 70 • , respectively. An intriguing feature emerging by these plots is the growth of A Γ for decreasing values of JHEP02(2016)178 ξ which might be traced back from eq. (5.2). Given the collider bounds on mq 1 1TeV, this implies that A Γ is maximum for mq 2 ≈ 1TeV, well above the current experimental bound from direct search. Moreover, the maximum values for A Γ are reached for arg(δ L d ) 21 approaching 90 • as in this case the indirect constraint from ∆ K can be relaxed, as already discussed.

Conclusions
In spite of the remarkable success of the SM in describing all the available flavor data on K and B d,s systems, it is still possible that New Physics (NP) affects the up-quark sector in a significant manner. This is the case for instance of models of alignment, in which the flavor structure of the NP does not satisfy two-generation universality. In this work, we have revisited the phenomenology of alignment models both model-independently and within supersymmetric scenarios. Assuming that NP contributes to K 0 −K 0 and D 0 −D 0 mixings only through non-renormalizable operators involving SU(2) L quark-doublets, we have derived model-independent upper bounds on CP violating effects in D meson system. Interestingly enough, we have found that the current experimental resolutions are starting to probe the natural predictions of alignment models. Our main finding is that within the above framework the bound from K and the current value of x (see table 1) constrain CP violation in the D −D mixing to below the per-mil level, A Γ 0.1% (see figure 1 and eq. (3.18)).

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we can perform an exact diagonalization of the 2 × 2 squark mass matrices M 2 q,LL and M 2 u,RR by means of the unitary matrices U L and U R defined as where U L and U R read The flavor mixing angles s L,R , c L,R and the CPV phases φ L,R are defined as while the squark masses read where f = q, u and m 2 ij stands for (M 2 q,LL ) ij or (M 2 u,RR ) ij when f = q, u, respectively. For the chargino and neutralino mass matrices, we have