Phenomenological study of heavy hadron lifetimes

The lifetimes of bottom and charmed hadrons are analyzed within the framework of the heavy quark expansion (HQE). Lifetime differences arise from the spectator effects such as weak W-annihilation and Pauli interference. Spectator effects originating from dimension-7 four-quark operators are derived. Hadronic matrix elements of four-quark operators are parameterized in a model-independent way. Using the dimension-6 bag parameters recently determined from HQET sum rules and the vacuum insertion approximation for meson matrix elements of dimension-7 operators, the calculated B meson lifetime ratios τ(B+)/τ(Bd0) = 1.074− 0.016+ 0.017 and τ(Bs0)/τ(Bd0) = 0.9962 ± 0.0024 are in excellent agreement with experiment. Likewise, based on the quark model evaluation of baryon matrix elements, the resulting baryon lifetime ratios τ(Ξb−)/τ(Λb0), τ(Ξb−)/τ(Ξb0), τ(Ωb−)/τ(Ξb−) and the Λb − B0 lifetime ratio τ(Λb0)/τ(Bd0) = 0.953 also agree well with the data. Contrary to the bottom hadron sector where the HQE in 1/mb works well, the HQE to 1/mc3 fails to give a satisfactory description of the lifetimes of both charmed mesons and charmed baryons. This calls for the subleading 1/mQ corrections to spectator effects. The relevant dimension-7 spectator effects are in the right direction for explaining the large lifetime ratio of τ(Ξc+)/τ(Λc+). However, the destructive 1/mc corrections to Γ(Ωc0) are too large to justify the validity of the HQE, namely, the predicted Pauli interference and semileptonic rates for Ωc0 become negative. Demanding these rates to be positive for a sensible HQE, we find the lifetime pattern τ(Ξc+) > τ(Ωc0) > τ(Λc+) > τ(Ξc0), contrary to the current hierarchy τ(Ξc+) > τ(Λc+) > τ(Ξc0) > τ(Ωc0). We conclude that the Ωc0, which is naively expected to be shortest-lived in the charmed baryon system owing to the large constructive Pauli interference, could live longer than the Λc+ due to the suppression from 1/mc corrections arising from dimension-7 four-quark operators. The new charmed baryon lifetime pattern needs to be tested in forthcoming experiments.

Abstract: The lifetimes of bottom and charmed hadrons are analyzed within the framework of the heavy quark expansion (HQE). Lifetime differences arise from the spectator effects such as weak W -annihilation and Pauli interference. Spectator effects originating from dimension-7 four-quark operators are derived. Hadronic matrix elements of fourquark operators are parameterized in a model-independent way. Using the dimension-6 bag parameters recently determined from HQET sum rules and the vacuum insertion approximation for meson matrix elements of dimension-7 operators, the calculated B meson lifetime ratios τ (B + )/τ (B 0 d ) = 1.074 +0.017 −0.016 and τ (B 0 s )/τ (B 0 d ) = 0.9962 ± 0.0024 are in excellent agreement with experiment. Likewise, based on the quark model evaluation of baryon matrix elements, the resulting baryon lifetime ratios τ ) and the Λ b − B 0 lifetime ratio τ (Λ 0 b )/τ (B 0 d ) = 0.953 also agree well with the data. Contrary to the bottom hadron sector where the HQE in 1/m b works well, the HQE to 1/m 3 c fails to give a satisfactory description of the lifetimes of both charmed mesons and charmed baryons. This calls for the subleading 1/m Q corrections to spectator effects. The relevant dimension-7 spectator effects are in the right direction for explaining the large lifetime ratio of τ (Ξ + c )/τ (Λ + c ). However, the destructive 1/m c corrections to Γ(Ω 0 c ) are too large to justify the validity of the HQE, namely, the predicted Pauli interference and semileptonic rates for Ω 0 c become negative. Demanding these rates to be positive for a sensible HQE, we find the lifetime pattern τ (Ξ + c ) > τ (Ω 0 c ) > τ (Λ + c ) > τ (Ξ 0 c ), contrary to the current hierarchy τ (Ξ + c ) > τ (Λ + c ) > τ (Ξ 0 c ) > τ (Ω 0

Introduction
It was realized since the late 1970s and 1980s that the lifetime differences of singly heavy hadrons containing a heavy quark Q arise mainly from the spectator effects like W -exchange and Pauli interference due to the identical quarks produced in heavy quark decay and in the wave function of the heavy hadron [1][2][3][4]. The spectator effects were expressed in 1980s in terms of local four-quark operators by relating the total widths to the imaginary part of certain forward scattering amplitudes [5][6][7]. With the advent of heavy quark effective theory (HQET), it was recognized in early 1990s that nonperturbative corrections to the parton picture can be systematically expanded in powers of 1/m Q [1][2][3][4]. Within the QCD-based framework, namely the heavy quark expansion (HQE), which is a generalization of the operator product expansion (OPE) in 1/m Q in the Minkowski space, some phenomenological assumptions in 1980s acquired a firm theoretical footing in 1990s and nonperturbative effects can be systematically studied (for a review, see [8]). On the basis of the OPE approach for the analysis of inclusive weak decays, the inclusive rate of the heavy hadron H Q is schematically represented by

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where V CKM is the relevant CKM matrix element. The A 0 term comes from the decay of the heavy quark Q and is common to all heavy hadrons H Q . There is no linear 1/m Q corrections to the inclusive decay rate due to the lack of gauge-invariant dimension-four operators [1,9,10], a consequence known as Luke's theorem [11]. Nonperturbative corrections start at order 1/m 2 Q and are model independent. Spectator effects in inclusive decays due to the Pauli interference and W -exchange contributions account for 1/m 3 Q corrections. The estimate of spectator effects is model dependent; the hadronic four-quark matrix elements are usually evaluated by assuming the factorization approximation for mesons and the quark model for baryons. Moreover, there is a two-body phase-space enhancement factor of 16π 2 for spectator effects relative to the three-body phase space for heavy quark decay. This means that 1/m 3 Q corrections can be quite significant. Moreover, spectator effects in charm hadron decays, being of order 1/m 3 c , can be comparable to and even exceed the A 0 term. Based on the HQE approach for the analysis of inclusive weak decays, the first correction to bottom hadron lifetimes is of order 1/m 2 b and it is model independent. For example, it was found in [12]  . The 1/m 3 b corrections can be expressed in a modelindependent manner [12] τ ≃ 0.98 − 0.17ε 1 + 0.20ε 2 − (0.012 + 0.021B)r, (1.2) where ε i , B i ,B, r are the hadronic parameters to be introduced below in section 3.1. Experimentally, the Λ 0 b lifetime was significantly shorter than the B meson one in the early measurements. Taking the current B 0 meson lifetime τ (B 0 ) = (1.520 ± 0.004) ps [13] as a benchmark, τ (Λ b ) was found to be (1.14 ± 0.08) ps in 1996 [14]. The world-averaged lifetime ratio then was τ (Λ 0 b ) τ (B 0 ) = 0.79 ± 0.06 (1996), (1.3) dominated by CERN e + e − collider LEP experiments [15]. This lifetime ratio remained essentially unchanged even in 2004 [16] τ (Λ 0 b ) τ (B 0 ) = 0.803 ± 0.047 , HFAG 2004. (1.4) Since the two parameters ε 1 and ε 2 obey the constraint ε 1 ≈ 0.3ε 2 [12] and they vanish under vacuum insertion approximation, it is very difficult to employ the HQE prediction (1.2) to accommodate the experimental value of τ (Λ b )/τ (B d ) without invoking too large a value of r and/orB. It is thus reasonable to conclude that the 1/m 3 b corrections in the HQE do not suffice to describe the observed lifetime difference between Λ b and B d .
Motivated by the conflict between theory and experiment for the lifetime ratio τ (Λ b )/τ (B d ), it was suggested in [17] that the assumption of local duality is not correct for nonleptonic inclusive width and that the presence of linear 1/m b corrections prohibited in the HQE is strongly implied by the data. As shown in [18] and [19], the simple ansatz of replacing Γ NL by Γ NL (m Λ b /m b ) 5 not only solves the lifetime ratio problem but also provides the correct absolute decay widths for the Λ b baryon and the B meson. However,

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there exist several insurmountable difficulties with this scenario and some of them were already discussed in [18].
Nowadays we know that the issue with the low value of Λ b − B 0 lifetime ratio or the short Λ b lifetime was on the experimental side. The first direct measurement of the lifetime ratio τ (Λ 0 b )/τ (B 0 ) was carried out by the D0 Collaboration in 2005 with the result 0.87 +0. 17 −0.14 ±0.03 [20]. Also, the CDF experiment measured the Λ b lifetime in exclusive decay to J/ψΛ [21] and showed that the Λ b lifetime is significantly longer than either previous Λ b lifetime measures or state-of-the-art calculation based on the HQE at the time. The world averages as of today are [13] τ (Λ 0 b ) = (1.470 ± 0.010) × 10 −12 s , τ (Λ 0 b )/τ (B 0 d ) = 0.964 ± 0.007 . (1.5) As we shall see in section 4.1 below, the current value of the Λ b − B 0 lifetime ratio can be explained nicely in the HQE approach. The major theoretical uncertainties of the HQE predictions for hadron lifetimes come from the hadronic matrix elements of four-quark operators. In the meson sector, the meson matrix elements can be expressed in a model-independent manner in terms of four bag parameters B 1,2 and ǫ 1,2 . These parameters have been calculated using lattice QCD and QCD sum rules (see [8] for a review). Based on HQET sum rules, they have been updated recently in [22]. For the baryon matrix elements, they can be parameterized in terms of four parameters L 1,··· ,4 , but only two of them are independent.
Although the heavy quark expansion in 1/m b works well for B mesons and bottom baryons, the HQE in 1/m c fails to give a satisfactory description of the lifetimes of both charmed mesons and charmed baryons. First of all, to order 1/m 3 c , the destructive Pauli interference in D + decay overcomes the c quark decay rate so that the inclusive rate and the lifetime of D + become negative. Hence, it is not meaningful to discuss the lifetime ratio τ (D + )/τ (D 0 ) at this level. Second, the lifetime pattern of charmed baryons is understandable only qualitatively, but not quantitatively. The quantitative estimates of charmed baryon lifetimes and their ratios are still rather poor [18]. For example, τ (Ξ + c )/τ (Λ + c ) is calculated to be 1.03 (see section 4.2 below), while experimentally it is measured to be 2.21 ± 0.15 [13]. Therefore, it is natural to consider the effects stemming from the nextorder 1/m c expansion. Specifically, we shall consider the subleading 1/m c corrections to the spectator effects.
The 1/m Q corrections to the spectator effects are computed by expanding the forward scattering amplitude in the light-quark momentum and matching the result onto the operators containing derivative insertions. Dimension-7 terms are either the four-quark operators times the spectator quark mass or the four-quark operators with an additional derivative [23,24]. Dimension-7 operators were first studied in [25] for the width difference in the B s −B s system, in [23,24] for the lifetime differences of heavy hadrons and in [26] for D-meson lifetimes.
In this work we will study spectator effects in inclusive nonleptonic and semileptonic decays, analyze the lifetime pattern of heavy hadrons, and pay attention to the effects of dimension-7 operators on the heavy hadron lifetimes, especially for the charmed mesons and baryons. Our goal is to see if the aforementioned problems such as the negative lifetime JHEP11(2018)014 of the D + meson and the closeness of Ξ + c and Λ + c lifetimes can be resolved by the inclusion of subleading 1/m Q corrections to the spectator effects.
This work is organized as follows. In section 2 we give general heavy quark expansion expressions for inclusive nonleptonic and semileptonic widths. We then study lifetimes of B and D mesons in section 3 and bottom and charmed baryons in section 4 with the evaluation of hadronic four-quark matrix elements. Discussions and conclusions are given in section 5. In appendix A we sketch the derivation of dimension-7 four-quark operators relevant for the spectator effects in heavy baryon decays. Appendix B is devoted to the evaluation of baryon matrix elements in the quark model.

Framework
In this section we write down the general expressions for the inclusive decay widths of heavy hadrons and leave the evaluation of the relevant hadronic matrix elements to the next section. It is known that the inclusive decay rate is governed by the imaginary part of an effective nonlocal forward transition operator T . When the energy released in the decay is large enough, the nonlocal effective action can be recast as an infinite series of local operators with coefficients containing inverse powers of the heavy quark mass m Q . Under this heavy quark expansion, the inclusive nonleptonic decay rate of a singly heavy hadron H Q containing a heavy quark Q is given by [1][2][3][4] where the second T appearing in the integral is a time-ordering symbol. Under the operator product expansion, the transition operator T can be expressed in terms of local quark operators where ξ is the relevant CKM matrix element, the dimension-6 T 6 consists of the four-quark operators (QΓq)(qΓQ) with Γ representing a combination of the Lorentz and color matrices, while a subset of dimension-7 T 7 is governed by the four-quark operators containing derivative insertions (see section 2.2 below). Since σ · G = −2 σ · B, theQσ · GQ term describes the interaction of the heavy Q quark spin with the gluon field. Explicitly,

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has been made with In heavy quark effective theory, the mass of the heavy hadron H Q is of the form where the three nonperturbative HQET parametersΛ H Q , λ 1 and λ 2 are independent of the heavy quark mass andΛ H Q can be regarded as the binding energy of the heavy hadron in the infinite mass limit. 1 Since the chromomagnetic field is produced by the light cloud inside the heavy hadron, it is clear that σ · G is proportional to S Q · S ℓ , where S Q ( S ℓ ) is the spin operator of the heavy quark (light cloud). The parameter d H is given by Therefore, d H = 3 for B and D mesons, d H = −1 for B * and D * mesons, d H = 0 for the antitriplet baryon T Q , d H = 4 for the spin-1 2 sextet baryon S Q and d H = −2 for the spin-3 2 sextet baryon S * Q . It follows from eq. (2.6) that Numerically (in units of GeV 2 ), It is interesting to note that the large-N c relation [28,29] λ meson 2 ∼ N c λ baryon 2 (2.10) is fairly satisfied especially for bottom hadrons. As for the kinetic energy parameter λ 1 , we shall use [30] λ meson Summing over the contributions from b → ccs, b → ccd, b → cūd and b → cūs processes, we have [1][2][3][4] x, x, 0)) −8c 1 c 2 (I 2 (x, 0, 0) + I 2 (x, x, 0)), (2.12) JHEP11(2018)014

Dimension-6 operators
Defining the dimension-six four-quark operators in eq. (2.3) responsible for spectator effects in inclusive decays of heavy baryons (denoted by B Q ) are given by [5][6][7] T B Q ,q 1 where (q 1 q 2 ) ≡q 1 γ µ (1 − γ 5 )q 2 , α, β are color indices and ξ is the relevant CKM matrix element for the quark-mixing-favored decay. Note that for charm decay, Q = c, q 1 = d, q 2 = u and q 3 = s and for bottom decay, Q = b, q 1 = u, q 2 = d, q 3 = s. In the baryon sector, the first term T B Q ,q 1 6,ann corresponds to a W -exchange (or generically weak annihilation) contribution (see figure 1(a)), the rest to contributions from Pauli interference. For example, T B Q ,q 2 6,int− arises from the destructive interference of the q 2 quark produced in the heavy quark Q decay with the q 2 quark in the wave function of the heavy baryon B Q ( figure 1(b)). The last term T In the heavy meson sector, the W -exchange contribution to the heavy meson corresponds to the Pauli interference term T B Q 6,int− in eq. (2.20) in heavy baryon decays, while the Pauli interference in inclusive nonleptonic decays of heavy mesons corresponds to the annihilation term T B Q 6,ann in heavy baryon decays. This will be discussed in section 3.
It is clear from eqs. (2.3) and (2.20) that there is a two-body phase-space enhancement factor of 16π 2 for spectator effects relative to the three-body phase space for the heavy quark decay. This implies that spectator effects, being of order 1/m 3 Q , are comparable to and even exceed the 1/m 2 Q terms. Note that the Wilson coefficients and four-quark operators in eq. (2.20) are renormalized at the heavy quark mass scale. Sometimes the so-called hybrid renormalization [6,33] is performed to evolve the four-quark operators (not the Wilson coefficients!) from m Q down to a low-energy scale, say, a typical hadronic scale µ had . The evolution from m Q down to µ had will in general introduce new structures such as penguin operators. Nevertheless, in the present paper we will follow [12] to employ (2.3) and (2.20) as our starting point for describing inclusive weak decays since it is equivalent to first evaluating the four-quark matrix elements renormalized at the m Q scale and then relating them to the hadronic matrix elements renormalized at µ had through the renormalization group equation, provided that the effect of penguin operators is neglected.
For inclusive semileptonic decays, apart from the heavy quark decay contribution there is an additional spectator effect in charmed-baryon semileptonic decay originating from the Pauli interference of the s quark [34]; that is, the s quark produced in c → sℓ + ν ℓ has an interference with the s quark in the wave function of the charmed baryon (see figure 2). It is now ready to deduce this term from T q 3 6,int+ in eq. N c = 1 and q 3 = s: Obviously, this term occurs only in the semileptonic decays of Ξ c and Ω c baryons.

Dimension-7 operators
To the order of 1/m 4 Q in the heavy quark expansion in eq. (2.3), we need to consider dimension-7 operators. For our purposes, we shall focus on the 1/m Q corrections to the spectator effects discussed in the last subsection and neglect the operators with gluon fields. As mentioned in the Introduction, the relevant dimension-7 terms are either the four-quark operators times the spectator quark mass or the four-quark operators with an additional derivative [23,24]. We shall follow [26] to define the following dimension-7 four-quark operators: and the color-octet operators S q i (i = 1, . . . , 6) obtained from P q i by inserting t a in the two currents of the respective color singlet operators, for example, Following the prescription outlined in [26], one can derive the dimension-7 operators relevant to heavy baryon decays. Explicitly (see appendix A for details), However, we shall see later that in order to evaluate the baryon matrix elements, it is more convenient to express dimension-7 operators in terms of P q i andP q i ones, whereP i denotes the color-rearranged operator that follows from the expression of P i by interchanging the color indices of the q i andq j Dirac spinors. For example, For the dimension-7 operators relevant to heavy meson decays, see the next section.

Lifetime ratio
In order to compare the HQE predictions with the experimental results, we often consider the lifetime ratio of two heavy hadrons H 1 and H 2 , which reads where use of eqs. (2.3) and (2.16) has been made, c 3,Q ≡ c NL 3,Q + c SL 3,Q and likewise for c 5,Q . Note that the lifetime ratio computed in this manner is valid for B mesons and bottom baryons where the HQE in 1/m b converges nicely, but not for charmed hadrons where the inclusive rates are not dominated by the c 3,c term.

Lifetimes of bottom mesons
We shall first fix the b quark mass from the measured inclusive semileptonic decay rate. Experimentally [13],

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Theoretically, eq. (2.16) leads to 2 where we have included the radiative corrections to order α s characterized by the parameters a and b. The order α s corrections alone without µ 2 π /m 2 b or µ 2 G /m 2 b terms were first calculated in [36][37][38]. Corrections of order α s µ 2 π /m 2 b have been calculated in [39,40], while the O(α s µ 2 G /m 2 b ) terms in [41,42]. The analytic expression of the coefficient a can be found in [38] and the b term in [42].
The inclusive rate is very sensitive to the quark mass m b . The reliability of the calculation depends on the ability to control the higher order contributions in the double series expansion in α s and Λ QCD /m b . The pole mass definition for heavy quark masses does not converge very well and moreover it is plagued by the renormalon ambiguity [43,44]. For the short-distance MS massm b (m b ), it is not under good control for the smaller scale µ ∼ 1 GeV. Two different schemes commonly used to define the short-distance b-quark mass are the kinetic [45,46] and the 1S [47] schemes. We follow [30] for a recent global fit of inclusive semileptonic B decays in the kinetic scheme. This analysis includes higher power corrections O(1/m 4 b ) and O(m 5 b ) and next-to-leading order QCD (NLO-QCD) corrections O(α 2 s ). In this scheme, it is conventional to constrain the charm quark mass to be the MS onem c (3 GeV) = 0.987 ± 0.013 GeV which yields a better convergence of the perturbative series. The results of the fit are [30]: is close to the usual one. To the leading-order QCD (LO-QCD), the definition of the quark mass is very arbitrary. If everything is calculated consistently to NLO-QCD, the dependence of the final result on the quark mass definition will be considerably weak when the relations between different quark mass schemes are used consistently at the NLO accuracy. 3 Although dimension 3, 4 and 6 Wilson coefficients up to NLO-QCD are available for heavy B and D mesons, they are still absent for heavy baryons. Dimension-7 Wilson coefficients are known only to the LO level for both heavy mesons and baryons. For this reason, in this work we shall focus on the LO-QCD study. In the bottom hadron sector, we use the quark masses m b = 4.546 GeV and m c = 0.987 GeV obtained in eq. (3.3). The reason is that the calculated inclusive semileptonic rate to LO, Γ(B → X c e + ν e ) = 4.59 × 10 −14 GeV using the kinetic b quark mass is very close to the experimental measurement: Corrections to inclusive semileptonic B decays have been calculated to order O(α 2 s ) and O(1/m 5 b ) [35]. 3 Besides the above-mentioned inclusive semileptonic B decays, another example is given in [48] for inclusive nonleptonic decay rates to NLO which are calculated in various quark mass schemes. The numerical results are similar for different short-distance quark masses.

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where the average lifetime τ (B + /B 0 /B s /b−baryon admixture) = (1.566±0.003) ps [13] and branching fraction (3.1) have been made. If the running quark massesm b (m b ) = 4.248 GeV andm c (m c ) = 1.277 GeV are employed, the obtained Γ(B → X c e + ν e ) to LO will be too small by 47% compared to experiment. It should be stressed that to the NLO-QCD, the dependence of the inclusive semileptonic rate on the quark mass definition is considerably weak.
We next turn to the spectator effects of order 1/m 3 b . The W -exchange contributions to B d and B s correspond to the Pauli interference terms T B Q ,q 2 6,int and T B Q ,q 3 6,int , respectively, in eq. (2.20) for heavy baryon decays, while the Pauli interference in inclusive nonleptonic B − decay corresponds to the annihilation term T B Q ,q 1 6,ann in heavy baryon decays: where (q 1 t a q 2 ) ≡q 1 γ µ (1 − γ 5 )t a q 2 with t a = λ a /2 and we have applied the relation to the transition operators so that they are more suitable for the matrix element evaluation in the meson case. Likewise, dimension-7 operators relevant for heavy meson decays can be read from eq. (2.23): For the meson matrix elements of four-quark operators, we follow [12] to define the bag parameters B i and ε i to parametrize the hadronic matrix elements in a model-independent way: Under the vacuum-insertion approximation, bag parameters are given by B i = 1 and ε i = 0, but they will be treated as free parameters here. In the large-N c limit, it is expected that B i ∼ O(1) and ε i ∼ O(1/N c ). Likewise, the matrix elements of dimension-7 four-quark operators read [26] and similar parametrization for the color-octet operators with the replacement of P → S and ρ i → σ i . Under the vacuum-insertion approximation, ρ q i = 1 and all σ's vanish. Applying eqs. (3.8) and (3.9) to evaluate the B-meson matrix elements of dimension-6 and dimension-7 four-quark operators, (3.5) and (3.7), respectively, the spectator effects , it is evident that contributions from dimension-7 operators are suppressed by Λ/m b relative to the dimension-6 ones. As stressed in [12], the coefficients of B i in Γ ann (B d ) are one to two orders of magnitude smaller than that of ε i . Therefore, contributions of B i can be safely neglected at least in Γ ann (B d ). There exist several estimates of the bag parameters B i and ε i based on sum rules [49][50][51][52] and lattice QCD [53,54]. On the basis of HQET sum rules, 4 these parameters have been updated recently to be [22] For the parameters ρ q i and σ q i we shall use the vacuuminsertion estimates, namely ρ q i = 1 and σ q i = 0. To compute the nonleptonic decay rate we apply the Wilson coefficient functions which are evaluated at µ = 4.4 GeV to the leading logarithmic approximation (see table XIII of [57]). The total rate reads where the decay rate of the heavy quark b of the B meson is given by The calculated lifetimes of B mesons shown in table 1 are longer than the free b quark lifetime for two reasons: (i) 1/m 2 b effects characterized by λ 1 and λ 2 will suppress the nonleptonic rate slightly, and (ii) inclusive semileptonic rate is slightly suppressed by QCD corrections, the a and b terms in eq. (3.2).
Eq. (3.11) implies a constructive W -exchange to B d and B s and a destructive Pauli interference to B u . From eq. (2.26) we obtain model-independent expressions for the lifetime ratios where we have decomposed the lifetime ratios in terms of dimension-6 and dimension-7 contributions and dropped the superscripts of ρ q i and σ q i by assuming their flavor independence JHEP11(2018)014 for simplicity. Using eq. (3.12) for dimension-6 bag parameters and the vacuum-insertion approximation for dimension-7 ρ q i and σ q i , 5 we obtain = 0.9994 ± 0.0025 found in [22]. The theoretical uncertainties in (3.18) arise mainly from the bag parameters given in eq. (3.12). Our results are in excellent agreement with experiment. If we apply naive vacuum-insertion approximation also to dimension-6 bag parameters, we will have This implies that the main contribution to the B u − B d lifetime ratio arises from the coloroctet terms −0.57ǫ 1 + 0.15ǫ 2 + · · · in eq. (3.17). The predicted ǫ 1 and ǫ 2 from HQET sum rules given in eq. (3.12) yield an excellent description of lifetime ratios. Note that ǫ 1 ≈ 3ǫ 2 here rather than ǫ 1 ≈ 0.3ǫ 2 as originally argued in [12]. Several remarks are in order. (i) Weak annihilation contributions to B d and B s are suppressed relative to the Pauli interference due to a large cancelation between the bag parameters B 1 and B 2 and the partial cancelation between ǫ 1 and ǫ 2 , see eq. (3.11) and table 1. (ii) The annihilation contribution to B s is larger than that of B d owing to SU(3) breaking in the decay constants and masses. This explains why the lifetime B s is slightly shorter than B d . (iii) To order 1/m 3 c , we obtain τ (B + )/τ (B 0 d ) = 1.0945, which can be checked from eq. (3.17). Hence, it is necessary to introduce dimension-7 operators in order to improve the agreement with experiment.

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where x = (m s /m c ) 2 , d D = 3 and the Wilson coefficients c SL 3,c and c SL 5,c are given by eq. (2.18). In the above equation we have included the radiative correction η(x, 0, 0) given by the (1 + aα s /π) term in eq. (3.2). We find that the experimental values for D + and D 0 semileptonic widths can be fitted by the charm quark mass m c = 1.56 GeV. 6 For the Wilson coefficients, we shall use the lowest order values where z = m 2 µ /m 2 c . We have followed [26] to derive the expression for the inclusive rate of D + s . Note that the contributions involving the z terms arise from the leptonic intermediate states.

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It is well known that D + has a longer lifetime than D 0 because of destructive Pauli interference [5,59,60]. To a good approximation to 1/m 3 c expansion, we have For the decay constant f D of order 205 MeV (see [58] for a review), it is easily seen that the Pauli interference Γ int (D + ) to order 1/m 3 c overcomes the c quark decay rate so that Γ(D + ) becomes negative no matter which charmed quark mass is employed, the MS massm c (m c ) = 1.279 GeV or the fit mass m c = 1.56 GeV. This remains to be true even if other sets of the bag parameters are used so long as they are not far from the vacuum insertion expectation.
In the literature, the lifetime ratio is often computed using the relation 7 where the experimental value of τ (D + ) is utilized on the r.h.s. of the above equation. However, it is important to keep in mind that the calculated D + lifetime is negative to order 1/m 3 c . Hence, it does not make sense to apply the HQE to O(1/m 3 c ) to predict a "positive" lifetime ratio τ (D + )/τ (D 0 ) in spite of a negative D + lifetime predicted by the HQE at this level. Therefore, we should also consider the ratio to ensure that R ′ D = 1/R D . Their experimental values are given by [13] τ (D + ) τ (D 0 ) expt = 2.536 ± 0.019, τ (D 0 ) τ (D + ) expt = 0.394 ± 0.003 .
We can use the experimental values of R D and R ′ D to constrain the bag parameters. To order 1/m 3 c , we find R D = 3.98 and R ′ D = −0.18 for B i = 1 and ǫ i = 0. This implies a negative D + lifetime. Indeed, the calculated τ (D + ) is −8.4 × 10 −13 s. The subleading 1/m c 7 It is not meaningful to apply eq. (2.26) to compute the lifetime ratio RD because (i) the Γ(D + ) rate is not dominated by the c3 term, and (ii) when eq. (2.26) is applied to the ratio R ′ D , it will lead to R ′ D = 2−RD which is negative.

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corrections to the Pauli interference term, namely, Γ int 7 obtained from dimension-7 fourquark operators at 1/m 4 c level, contributes constructively to the D + width (see eq. (3.23)). Hence, it is conceivable that the 1/m c corrections to the Pauli interference will be able to render Γ(D + ) positive in certain rages of the bag parameters. With m c = 1.56 GeV, we find R D = 2.06 and R ′ D = 0.58 in the presence of 1/m 4 c corrections with ρ i = 1 and σ i = 0. For the D + s meson, we follow [26] to define a substracted D + s lifetime bȳ as the decay D + s → τ + ν τ cannot be properly described by HQE due to its small energy release. In analogue to the D + meson, we consider the lifetime ratios We obtain In principle, if the vacuum-insertion expectation for ρ's and σ's is assumed, the four unknown parameters B 1,2 and ǫ 1,2 can be obtained by solving the four equations for R D , R ′ D , R Ds and R ′ Ds given in eqs. (3.28) and (3.32). In practice, the solutions are very sensitive to the experimental values within errors. We pick up the solutions not far from the vacuum-insertion expectation. 8 For example, one of the solutions is at the scale µ = m c . They reproduce the experimental values of R D , R ′ D , R Ds and R ′ Ds . Note that in order to accommodate the experimental values of R Ds and R ′ Ds , it is necessary to have B 2 > B 1 . To see this, we take vacuum-insertion values for ρ's and σ's and find from eq. (3.32) that

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It is clear that if B 2 ≈ B 1 and ǫ 2 ≈ ǫ 1 , the value of R Ds (R ′ Ds ) will be too large (small) compared to the data. Hence, one needs B 2 > B 1 and |ǫ 1 | > |ǫ 2 | in order to suppress R Ds and enhance R ′ Ds simultaneously. Our results are to be compared with the recent estimates based on HQET sum rules by Kirk, Lenz and Rauh (KLR) [22]

Lifetimes of bottom baryons
The spectator effects in inclusive heavy bottom baryon decays arising from dimension-6 and dimension-7 operators are given by eqs. (2.20) and (2.25), respectively. We shall rely on the quark model to evaluate the baryon matrix elements of four-quark operators. In [18] we have studied the matrix elements in the MIT bag model [61][62][63][64] and the nonrelativistic quark model (NQM). In analogue to eq. (3.8), we parameterize the four baryon matrix elements in a model-independent manner: 9 where B b stands for the antitriplet bottom baryon T b (Λ b or Ξ b ) or the sextet bottom baryon Ω b , f Bq and m Bq are the decay constant and the mass of the heavy meson B q , respectively. The four hadronic parameters L 1 , · · · , L 4 are not all independent.
First, since the color wavefunction for a baryon is totally antisymmetric, the matrix element of (bb)(qq) is the same as that of (bq)(qb) except for a sign difference. Thus we follow [12] to define a parameterB and where a q , b q and c q are the four-quark overlap integrals used in the MIT bag model: (4.5) which are expressed in terms of the large and small components u(r) and v(r), respectively, of the quark wavefunction (see e.g., ref. [66] for the technical detail of the bag model evaluation). In deriving eq. (4.4), use of has been made. The first relation in eq. (4.6) is a model-independent consequence of heavy quark spin symmetry [12]. It follows from eqs. (4.2), (4.3) and (4.4) that where the second relation for the Ω b is exact in the NQM but only an approximation in the MIT bag model.

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Since the small component v(r) is negligible in the NQM, baryon matrix elements of four-quark operators in the NQM and MIT models are the same except for the replacement: Hence, in the NQM a q is nothing but the baryon wave function at the origin squared |ψ bq (0)| 2 . In general, the strength of destructive Pauli interference and W -exchange is governed by a q + b q in the bag model and |ψ(0)| 2 in the NQM. However, the bag model calculation of a q + b q generally gives a much smaller value than the nonrelativistic estimate of |ψ(0)| 2 . As argued in [18], the difference between a q + b q and |ψ(0)| 2 is not simply attributed to relativistic corrections; it arises essentially from the distinction in the spatial scale of the wavefunction especially at the origin. As a consequence, both models give a quite different quantitative description for processes sensitive to |ψ(0)| 2 . It turns out that the NQM works better for heavy baryon decays. Hence, we will follow [18] to consider the NQM estimate of baryon matrix elements.
To estimate the bottom baryon wave function in the center, consider |ψ Λ b bq (0)| 2 as an example. A calculation of hyperfine splittings between Σ b and Λ b as well as between B * and B based on the mass formula given in [67] yields [68] where the equality |ψ Σ b bq (0)| 2 = |ψ Λ b bq (0)| 2 has been assumed. As a consequence, the wave function of a bottom baryon at the origin can be related to that of a B meson. Another approach proposed by Rosner [69] is to consider the hyperfine splittings of Σ b and B separately so that This method is presumably more reliable as |ψ bq (0)| 2 thus determined does not depend on m b and the constituent quark mass m q directly. Defining the wave function ratio 12) and noting that |ψ B bq (0)| 2 = 1 12 f 2 B m B , we see from eqs. (4.3), (4.4) and (4.6) that the parameters L 1 , · · · , L 4 for bottom baryons now read Hence, the baryon matrix elements are expressed in terms of two independent parameters r Bc andB.

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For dimension-7 four-quark operators, the baryon matrix elements are given by where m diq is the mass of the scalar diquark of T b and the parameters η q i are expected to be of order unity. We shall follow [70] so thatβ q i = 1 under the valence quark approximation. Two remarks are in order. First, unlike the meson matrix elements B q |P q 1,2 |B q in eq. (3.9) which are explicitly of order m q /m b because of the definition of the operators P q 1,2 , the baryon matrix elements B b |P q 1,2 |B b in eq. (4.14) are not explicitly proportional to m q /m b . Nevertheless, it is easily seen that (m 2 T b − m 2 diq )/m 2 b − 1, for example, is indeed of order m q /m b . Second, unlike the meson case we do not know how to evaluate the baryon matrix elements of P q 5,6 . Since the operators P q 5,6 arise from by expressing the QCD four-quark operators in terms of HQET operators we shall follow [23,24] to assume that dimension-7 operators contain full QCD b quark fields. Therefore, to evaluate the baryon matrix elements of dimension-7 operators given in eq. (2.25), we will drop the operators P q 5,6 andP q 5,6 . To estimate the hadronic parameter r B Q in the NQM, we find from eq. (4.11) that and likewise for r Λc , r Ξc and r Ωc . Notice that the heavy-quark spin-violating mass relation [28] holds very accurately for Q = b, c. Numerically, we obtain 10 r Λc = 0.610, r Ξc = 0.656, r Ωc = 0.664, 10 For a summary of the earlier estimates of r B Q , see [8].

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and 20) for f Bq = 186 MeV and f Bs = 230 MeV [58]. Therefore, the NQM estimate of |ψ B b bq (0)| 2 is indeed larger than the analogous bag model quantity: Except for the weak annihilation term, the expression of Pauli interference will be very lengthy if the hadronic parameters η q i andβ q i are all treated to be different from each other. Since in realistic calculations we will setβ q i (µ h ) = 1 under valence quark approximation and put η q i to unity, we shall assume for simplicity that η q i = η andβ q i =β. The spectator effects in nonleptonic decays of bottom baryons are now readily obtained from eqs. (2.20) and (2.25): where use has been made of eqs. (4.13) and (4.14). Note that there is no weak annihilation contribution to the Ξ − b and Ω b and that there are two Cabibbo-allowed Pauli interference terms in Ξ − b decay, and one Cabibbo-allowed as well as one Cabibbo-suppressed interferences in Λ b decay.
To compute the decay widths of bottom baryons, we have to specify the values ofB and r. SinceB = 1 in the valence-quark approximation and since the wavefunction squared ratio r is evaluated using the quark model, it is reasonable to assume that the NQM and the valence-quark approximation are most reliable when the baryon matrix elements are evaluated at a typical hadronic scale µ had . As shown in [12], the parametersB and r renormalized at two different scales are related via the renormalization group equation to bẽ and β 0 = 11 3 N c − 2 3 n f . We consider the hadronic scale in the range of µ had ∼ 0.65 − 1 GeV. Taking the medium scale µ had = 0.825 GeV as an illustration, we obtain α s (µ had ) = 0.59, B(µ) = 0.54B(µ had ) ≃ 0.54 and r(µ) ≃ 1.86 r(µ had ). The parameterβ is treated in a similar way. Using the values of r(µ had ) given in eq. (4.19), the calculated inclusive decay rates of bottom baryons are summarized in table 2. We find that the lifetimes of bottom baryons stay almost constant with variation of µ had .
We see from table 2 that the bottom baryon lifetimes follow the pattern effects and that the destructive Pauli interference Γ int − in Ω b is the largest due to the presence of two valence s quarks in its quark content. The Ξ − b has the second largest Γ int − due to the Pauli interference of identical s quarks and the interference of identical d quarks.
Several remarks are in order. (i) There is a tiny difference between the semileptonic decays of the antitriplet Λ b or Ξ b and the sextet Ω b . It comes from the fact that the chromomagnetic operator contributes to the matrix element of Ω b but not to Λ b or Ξ b as the light degrees of freedom in the latter are spinless. (ii) It is evident from tables 1 and 2 that Wannihilation contribution in B decays is much smaller than that in bottom baryon decays. The W -exchange in B decays is helicity suppressed, while it is neither helicity nor color suppressed in the heavy baryon case. (iii) As pointed out in [65], b-flavor-conserving decays such as Ξ − b → Λ 0 b π − , Λ 0 b e −ν e and Ξ 0 b → Λ 0 b π 0 could affect the total rates of the Ξ b . These heavy-flavor-conserving weak decays were studied more than two decades ago within the framework that incorporates both heavy-quark and chiral symmetries [71,72]. The branching fraction of Ξ b → Λ b π is found to be of order (0.1 ∼ 1)%, consistent with the recent LHCb measurement which lies in the range from (0.57±0.21)% to (0.19±0.07)% [73]. Hence, contributions from b-flavor-conserving decays can be safely neglected for our present purpose.
From eq. (2.26) we obtain the following lifetime ratios 11 They are in good agreement with experiment [13]. The theoretical uncertainties for bottom baryon lifetime ratios can arise from many different places such as the nonperturbative parameters µ 2 π and µ 2 G , where QCD sum rule and lattice calculations are still not available, and the matrix elements of dimension-6 and -7 operators. In the quark model, the unknown matrix elements are expressed in terms of two parameters r B b , the wave function ratio, and B, which is equal to unity under the valence quark approximation. The estimate of the former is quite uncertain in the literature (see [8] for a review). Therefore, it is far more difficult to estimate the uncertainties than the B meson case. Nevertheless, there is one uncertainty which we can estimate reliably, namely, the hadronic scale µ had introduced before. The baryon matrix elements need to be evaluated at a typical hadronic scale µ had in order to comply with the valence quark approximation. We consider the hadronic scale in the range of 0.65−1 GeV and use µ had = 0.825±0.175 GeV to estimate the uncertainties. The theoretical errors in eq. (4.25) we have computed arise solely from the uncertainty of 11 The experimental lifetime ratio τ (Ξ 0 b )/τ (Ξ − b ) = 0.929 ± 0.028 (or τ (Ξ − b )/τ (Ξ 0 b ) = 1.076 ± 0.032) is quoted in the Heavy Flavor Averaging Group [74,75].

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the hadronic scale. The uncertainty in the prediction of τ (Λ + c )/τ (B 0 d ) comes from the bag parameters in (3.12) and the hadronic scale µ had . We see that the current world average of τ (Λ 0 b )/τ (B 0 d ) can be nicely explained within the framework of the HQE.

Lifetimes of charmed baryons
We first summarize the spectator effects relevant to charmed baryon decays derived from eqs. (2.20) and (2.25): whereB, η andβ are the hadronic parameters defined in eqs. (4.2), (4.14) and (4.15), respectively, and the wavefunction ratio r Bc defined in analog to eq. (4.12) with values given in eq. (4.19). As stated before, we follow [70]  For the semileptonic inclusive decay of the charmed baryons meson, the semileptonic decay rate has the same expression as eq. (3.21) except that the parameter d D is replaced by d Bc , which is equal to 0 for the antitriplet charmed baryons Λ c , Ξ c and 4 for the Ω c . For charmed baryons Ξ c and Ω c , there is an additional contribution to the semileptonic width coming from the Pauli interference of the s quark [34] (figure 2). The dimension-6 contribution Γ SL 6,int (B c ) is given before by eq. (2.21). As for the dimension-7 four-quark operator for semileptonic decays, it can be written as with the coefficients given by [26] g νµ We shall see later that, depending on the parameter r, the spectator effect in semileptonic decay of Ξ c and Ω c can be very significant, in particular for the latter.
To proceed the hadronic decay rates, we employ the Wilson coefficients given in eq. (3.22). As before, we consider the hadronic scale in the range of µ had ∼ 0.65 − 1 GeV and obtainB(µ) = 0.70B(µ had ) ≃ 0. 70  We see from table 3 the lifetime pattern is in accordance with experiment (for early studies of charmed baryon lifetimes, see [2-4, 7, 79-84]). This lifetime hierarchy is understandable qualitatively but not quantitatively. The Ξ + c baryon is longest-lived among charmed baryons because of the smallness of Wexchange and partial cancellation between constructive and destructive Pauli interferences, while Ω c is shortest-lived due to the presence of two s quarks in the Ω c that renders the contribution of Γ int + largely enhanced. It is also clear from table III that, although the qualitative feature of the lifetime pattern is comprehensive, the quantitative estimates of charmed baryon lifetimes and their ratios are still rather poor. For example, R 1 ≡ τ (Ξ + c )/τ (Λ + c ) and R 2 ≡ τ (Ξ + c )/τ (Ξ 0 c ) are calculated to be 1.03 and 1.90, respectively, while experimentally R 1 = 2.21 ± 0.15 and R 2 = 3.95 ± 0.47.
It is evident that, contrary to B meson and bottom baryon cases where the HQE in 1/m b leads to the lifetime ratios in excellent agreement with experiment, the heavy quark expansion in 1/m c does not work well for describing the lifetime pattern of charmed baryons. Since the charm quark is not heavy enough, it is perhaps sensible to consider the subleading 1/m c corrections to spectator effects as depicted in eq. (4.27). The numerical results are shown in table 4. By comparing table 4 with table 3, we see that Γ(Λ + c ) is enhanced while Γ(Ξ + c ) is suppressed so that the resulting lifetime ratio R 1 is enhanced from 1.03 to 1.84. This means that 1/m c corrections to spectator effects described by dimension-7 operators are in the right direction. However, the calculated Ω c lifetime becomes entirely unexpected: the shortest-lived Ω c turns out to be the longest-lived one to O(1/m 4 c ). This is because the dimension-7 contributions Γ int +,7 (Ω c ) and Γ SL 7 (Ω c ) are destructive and their size are so large that they overcome the dimension-6 ones and flip the sign. Of course, a negative Γ SL (Ω c ) does not make sense as the subleading corrections are too large to justify the validity of the HQE.
In order to allow a description of the 1/m 4 c corrections to Γ(Ω c ) within the realm of perturbation theory, we introduce a parameter α so that Γ int +,7 (Ω c ) and Γ SL 7 (Ω c ) are multiplied by a factor of (1 − α); that is, α describes the degree of suppression. The origin of this suppression is unknown, but it could be due to the next-order 1/m c correction. 12 The lifetime of Ω 0 c is plotted as a function of α in figure 3. For the two extreme cases that α = 0 (no suppression on dimension-7 effects) and α = 1 (no corrections to Γ int + (Ω c ) and Γ SL (Ω c ) from dimension-7 operators), we have τ (Ω 0 c ) = 6.10×10 −13 s and 0.97×10 −13 s, respectively (see table 5). Our guidelines for the parameter α are (i) both Γ int + (Ω c ) and Γ SL (Ω c ) should be positive (at least, a negative Γ SL (Ω c ) does not make sense), and (ii) Γ SL (Ω c ) is comparable to that of Λ + c or Ξ c . Under these guidelines, we get α > 0.16 to ensure positive Γ SL (Ω c ) and Γ int + (Ω c ) and α ∼ 0.22 (0.32) for Γ SL (Ω c ) to be comparable to that of Λ + c (Ξ c ). We see from table 5 that a reasonable range of α lies in 0.16 < α < 0.32 and the corresponding Ω c lifetimes lies in the range 2.3 × 10 −13 s < τ (Ω 0 c ) < 3.3 × 10 −13 s. It should be stressed that this is our conjecture as we do not have rigorous statements on the unknown parameter α. At any rate, the Ω 0 c lifetime is very different from the current world average of τ (Ω 0 c ) = (0.69 ± 0.12) × 10 −13 s [13] from fixed target experiments. We suggest the new lifetime pattern  Table 5. Various contributions to the decay rates (in units of 10 −12 GeV) of the Ω 0 c after including subleading 1/m c corrections to spectator effects. However, the dimension-7 contributions Γ int +,7 (Ω 0 c ) and Γ SL 7 (Ω 0 c ) are multiplied by a factor of (1 − α) with α varying from 0 to 1.
0.24 ± 0.10 ± 0.02) × 10 −13 s [85], using the semileptonic decay Ω − b → Ω 0 c µ −ν µ X with Ω 0 c → pK − K − π + . This value is nearly four times larger than the current world-average value. 13 Finally, we would like to remark on the semileptonic widths. We see from table 3 that to order 1/m 3 c , the constructive Pauli interference is sizeable for the Ξ c and becomes overwhelming for the Ω c . However, this interference effect will be partially washed out by the next-order 1/m c correction, in particular for the latter (see table 5). Nevertheless, the interference effect in semileptonic inclusive decays can be tested by measuring the ratio of semileptonic branching fractions B semi (Ξ + c )/B semi (Λ + c ), where B semi (B c ) = B(B c → Xe + ν e ). This ratio naively of order 1.8 will be enhanced to O (3.2) in the presence of Pauli interference.

Discussions and conclusions
In this work we have analyzed the lifetimes of bottom and charmed hadrons within the framework of the heavy quark expansion. It is well known that the lifetime differences stem from spectator effects such as weak annihilation and Pauli interference. We list the dimension-6 four-quark operators responsible for various spectator effects and derive the corresponding dimension-7 ones. The hadronic matrix elements of four-quark operators are parameterized in a model-independent way.
The main results of our analysis are as follows.
• Since in this work we focus on the LO-QCD study for reason of consistency, the inclusive rate to LO is sensitive to the quark mass definition. For the b quark mass, we use the kinetic mass m kin b = 4.546 GeV obtained from a recent global fit to the inclusive semileptonic B decay to X c e + ν e in the kinetic scheme. Using the dimension-6 bag parameters recently determined from HQET sum rules and the vacuum-insertion approximation for meson matrix elements of dimension-7 operators, the calculated B 13 Our early conjecture of τ (Ω 0 c ) of order 2.3 × 10 −13 s first presented in [86] is indeed consistent with the LHCb measurement. • Baryon matrix elements of four-quark operators parametrized in a model-independent way in terms of four parameters, but only two of them are independent. They are evaluated using the NQM and the bag model. The hadronic parameter r defined in eq. (4.12) is estimated in the NQM to be in the range 0.60 to 0.66 for both bottom and charmed baryons.
• The lifetime pattern of bottom baryons is found to be τ ( Spectator effects due to W -exchange and destructive Pauli interference account for their lifetime differences. The calculated lifetime ratios τ • It is found that W -annihilation contribution in B decays is much smaller than that in bottom baryon decays (see tables 1 and 2). The W -exchange in B decays is helicity suppressed, while it is neither helicity nor color suppressed in the heavy baryon case.
• Contrary to the bottom hadron sector where the HQE in 1/m b works well, the HQE to 1/m 3 c fails to give a satisfactory description of the lifetimes of both charmed mesons and charmed baryons. This calls for the subleading 1/m Q corrections to spectator effects.
• We have employed the experimental values for D + and D 0 semileptonic widths to fix the charmed quark mass to be m c = 1.56 GeV. For the charmed meson decay constant of order 200 MeV, the destructive Pauli interference leads to a negative D + width irrespective of which charmed quark mass is employed. We showed that 1/m c corrections to the Pauli interference arising from dimension-7 four-quark operators will be able to render Γ(D + ) positive. We use the measured lifetime ratios of τ (D + )/τ (D 0 ) and τ (D + s )/τ (D 0 ) to constrain the bag parameters and find that B 2 > B 1 .
• The calculated lifetimes for heavy baryons depend on the low normalization point. We considered the hadronic scale in the range of µ had ∼ 0.65 − 1 GeV and found that the lifetimes of bottom baryons stay almost constant with variation of µ had , while the charmed baryon lifetimes increase by around 10% when the hadronic scale varies from 0.65 to 1.0 GeV. Nevertheless, the charmed baryon lifetime ratios remain nearly constant.
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