Measurement of the shape of the Λ 0 b → Λ + c µ − µ differential decay rate

: A measurement of the shape of the differential decay rate and the associated Isgur-Wise function for the decay Λ 0 b → Λ + c µ − µ is reported, using data corresponding to 3 fb 1 collected with the LHCb detector in proton-proton collisions. The Λ + c µ − µ (+ anything ) final states are reconstructed through the detection of a muon and a Λ + c baryon decaying into pK − π + , and the decays Λ 0 b → Λ + c π + π − µ − µ are used to determine contributions from Λ 0 b → Λ ∗ + c µ − µ decays. The measured dependence of the differential decay rate upon the squared four-momentum transfer between the heavy baryons, q 2 , is compared with expectations from heavy-quark effective theory and from unquenched lattice QCD predictions. A measurement of the shape of the differential decay rate and the associated Isgur-Wise function for the decay Λ 0 b → Λ þ c μ − ¯ ν μ is reported, using data corresponding to 3 fb − 1 collected with the LHCb detector in proton-proton collisions. The Λ þ c μ − ¯ ν μ ðþ anything Þ final states are reconstructed through the detection of a muon and a Λ þ c baryon decaying into pK − π þ , and the decays Λ 0 b → Λ þ c π þ π − μ − ¯ ν μ are used to determine contributions from Λ 0 b → Λ (cid:2)þ c μ − ¯ ν μ decays. The measured dependence of the differential decay rate upon the squared four-momentum transfer between the heavy baryons, q 2 , is compared with expectations from heavy-quark effective theory and from unquenched lattice QCD predictions.

Measurement of the shape of the Λ 0 b → Λ + c μ −ν μ differential decay rate A measurement of the shape of the differential decay rate and the associated Isgur-Wise function for the decay Λ 0 b → Λ þ c μ −ν μ is reported, using data corresponding to 3 fb −1 collected with the LHCb detector in proton-proton collisions. The Λ þ c μ −ν μ ðþanythingÞ final states are reconstructed through the detection of a muon and a Λ þ c baryon decaying into pK − π þ , and the decays Λ 0 b → Λ þ c π þ π − μ −ν μ are used to determine contributions from Λ 0 b → Λ Ãþ c μ −ν μ decays. The measured dependence of the differential decay rate upon the squared four-momentum transfer between the heavy baryons, q 2 , is compared with expectations from heavy-quark effective theory and from unquenched lattice QCD predictions. DOI

I. INTRODUCTION
In the Standard Model (SM) of particle physics, quarks participate in a rich pattern of flavor-changing transitions. The relevant couplings form a complex 3 × 3 matrix, known as the Cabibbo-Kobayashi-Maskawa (CKM) matrix, characterized by just four independent parameters [1]. A vast body of measurements of individual CKM elements exists, and thus the overall consistency of the SM picture of charged current interactions is highly overconstrained. Decades of experimental work have demonstrated the impressive consistency of experimental data with the CKM paradigm [2,3]; nonetheless, the motivation to probe the CKM matrix remains strong. Effects of physics beyond the SM may be subtle; thus, more precise measurements are necessary to unveil them. Semileptonic decays of heavyflavored hadrons are commonly used to measure CKM parameters, as they involve only one hadronic current, parametrized in terms of scalar functions known as form factors. The number of form factors needed to describe a particular decay depends upon the spin of the initial-and final-state hadrons [4,5]. A precise calculation of these form factors has been elusive for many years as it is not possible in perturbative QCD. Heavy-Quark Effective Theory (HQET) provides the framework to systematically include nonperturbative corrections in computations involving hadrons containing heavy quarks. In particular, in the limit of infinite heavy-quark mass, all the form factors describing the semileptonic decay of a heavyflavored hadron are proportional to a universal function, known as the Isgur-Wise (IW) function [6]. Lattice QCD, namely the use of lattice formulations of QCD in large scale numerical simulations, has emerged in recent years as a technique with well-defined and systematically improvable uncertainties which can be applied to a wide range of processes and physical quantities [7]. Predictions from the infinite heavy-quark mass limit are useful as a check of several lattice QCD calculations [8].
The decay Λ 0 b → Λ þ c μ −ν μ is described by six form factors corresponding to the vector and axial-vector components of the flavor-changing charged current [9]. In HQET, Λ 0 b decays are particularly simple, as the light ud quark pair has total spin j ¼ 0, and thus the chromomagnetic corrections, which are of the order of a few percent for B mesons, are not present [10]. In the static approximation of infinite heavy-quark masses, the six form factors characterizing the baryonic semileptonic decay 1 Λ 0 b → Λ þ c μ −ν μ can be expressed in terms of the elastic heavybaryon Isgur-Wise function ξ B ðwÞ [11]. The scalar invari- c is related to the squared four-momentum transfer between the heavy baryons, q 2 , by where v Λ 0 b and v Λ þ c are the four-velocities of the Λ 0 b and Λ þ c baryons, respectively, and m Λ 0 b and m Λ þ c are the corresponding invariant masses. Nonperturbative corrections to the static limit can be expressed in terms of an expansion in powers of 1=m c and 1=m b , where m c and m b represent the cand b-quark masses, respectively. It has been shown in Ref. [12] that the 1=m c term can be expressed in terms of ξ B ðwÞ and one dimensionful constant. Moreover, partial cancellations lead to small first-order corrections near w ¼ 1 [13].
In the static approximation, the differential decay width of the Λ 0 b → Λ þ c μ −ν μ decay is given by where the constant factor G is given by where G F represents the Fermi coupling constant [14], jV cb j is the magnitude of the matrix element describing the coupling of the c quark to the b quark, and the kinematic factor KðwÞ is given by The function ξ B ðwÞ cannot be determined from first principles in HQET, but calculations based on a variety of approaches exist. The kinematic limit w ¼ 1 is special in HQET, as only modest corrections in the (1=m b , 1=m c ) expansion are expected, due to the absence of hyperfine corrections [15]. Thus, it is interesting to express ξ B as a Taylor series expansion where ρ 2 is the magnitude of the slope of ξ B and σ 2 is its curvature at w ¼ 1. Sum rules provide constraints on ρ 2 and σ 2 . In particular, they require the slope at the zero recoil point to be negative and give bounds on the curvature and higher-order derivatives [16,17]. In addition, they predict σ 2 ≥ 3=5½ρ 2 þ ðρ 2 Þ 2 [18] and ρ 2 ≥ 3=4. Table I summarizes theoretical predictions for ρ 2 from quenched lattice QCD, QCD sum rules, and a relativistic quark model. Recently, state-of-the-art calculations of the six form factors describing the decay Λ 0 b → Λ þ c μ −ν μ have been obtained using lattice QCD with 2 þ 1 flavors of dynamical domain-wall fermions [19]. These form factors are calculated in terms of q 2 . More details on this formalism are given in Appendix A. The resulting theoretical uncertainty attached to a measurement of jV cb j using this form-factor prediction is about 3.2%. The precision of this calculation makes this approach an appealing alternative to the ones currently used, all based on B-meson semileptonic decays such asB 0 → D Ãþ μ −ν μ . Thus, it is important to examine the model's agreement with measured quantities such as the shape of the dΓ=dq 2 spectrum.
The experimental knowledge of Λ 0 b semileptonic decays is quite sparse, as this baryon is too heavy to be produced at the e þ e − B-factories. The only previous experimental study of ξ B ðwÞ was performed by the DELPHI experiment at LEP, which obtained ρ 2 ¼ 2.03 AE 0.46ðstatÞ þ0.72 −1.00 ðsystÞ, with an overall uncertainty of the order of 50% [20].
In this paper, we describe a determination of the shape of the w or q 2 spectrum of the decay Λ 0 b → Λ þ c μ −ν μ and compare it with functional forms related to a single form factor, inspired by HQET, and the lattice QCD prediction of Ref. [19]. Section II presents the experimental procedure and simulated samples, while Sec. III describes the method employed to reconstruct Λ 0 b → Λ þ c μ −ν μ candidates and to estimate the corresponding kinematic variables w and q 2 . Section IV describes the method adopted to isolate the signal, the unfolding procedure used to account for experimental resolution effects, and the efficiency corrections. The fit results for ξ B ðwÞ corresponding to different functional forms are summarized in Sec. V. The same analysis procedure is used in Sec. VI to derive the shape of the differential decay width dΓ=dq 2 ðΛ 0 b → Λ þ c μ −ν μ Þ and compare with the predictions of Ref. [19]. These data are also fitted with a single form-factor parametrization that corresponds to the HQET infinite heavy-quark mass limit.

II. EXPERIMENTAL METHOD
The data used in this analysis were collected with the LHCb detector at the Large Hadron Collider at CERN and correspond to 1 fb −1 of integrated luminosity collected at a center-of-mass energy of 7 TeV in 2011 and 2 fb −1 collected at a center-of-mass energy of 8 TeV in 2012.
The LHCb detector [24,25] is a single-arm forward spectrometer designed for the study of particles containing b or c quarks. The detector covers the pseudorapidity range 2 < η < 5, where η is defined in terms of the polar angle θ with respect to the beam direction as − lnðtan θ=2Þ. The detector includes a high-precision tracking system consisting of a silicon-strip vertex detector surrounding the pp interaction region [26], a large-area silicon-strip detector located upstream of a dipole magnet with a bending power of about 4 Tm, and three stations of silicon-strip detectors and straw drift tubes [27] placed downstream of the magnet. The tracking system provides a measurement of the momentum, p, of charged particles with a relative uncertainty that varies from 0.5% at low momentum to 1.0% at 200 GeV. 2 The minimum distance of a track to a primary vertex, the impact parameter (IP), is measured with a resolution of ð15 þ 29=p T Þ μm, where p T is the component of the momentum transverse to the beam, in GeV. Different types of charged hadrons are distinguished using information from two ring-imaging Cherenkov detectors (RICH) [28]. Photons, electrons, and hadrons are identified by a calorimeter system consisting of scintillating-pad and preshower detectors, an electromagnetic calorimeter, and a hadronic calorimeter. Muons are identified by a system composed of alternating layers of iron and multiwire proportional chambers [29]. The online event selection is performed by a trigger [30], which consists of a hardware stage, based on information from the calorimeter and muon systems, followed by a software stage, which applies a full event reconstruction. Muon candidates are first required to pass the hardware trigger that selects muons with a transverse momentum p T > 1.6 (1.8) GeV for the 2011 (2012) data taking period. In the subsequent software trigger, events with one particle identified as a muon are selected if at least one of the final-state particles has both p T > 0.8 GeV and IP larger than 100 μm with respect to all of the primary pp interaction vertices (PVs) in the event. In the offline selection, trigger signals are associated with reconstructed particles. Selection requirements can therefore be made on the trigger selection itself and on whether the decision was due to the signal candidate, other particles produced in the pp collision, or a combination of both. This classification of trigger selections can be used for data-driven efficiency determination. Finally, the tracks of two or more of the final-state particles are required to form a vertex that is significantly displaced from the PVs.
Our study makes use of simulated semileptonic decays, where pp collisions are generated using PYTHIA [31] with a specific LHCb configuration [32]. Decays of hadronic particles are described by EVTGEN [33], in which final-state radiation is generated using PHOTOS [34]. The interaction of the generated particles with the detector, and its response, are implemented using the GEANT4 toolkit [35] as described in Ref. [36].

III. EVENT RECONSTRUCTION
where X represents the undetected particles produced with the Λ þ c in the c-quark hadronization, we combine Λ þ c → pK − π þ candidates with tracks identified as muons. We consider candidates where a well-identified muon passing the hardware and software trigger algorithms with momentum greater than 3 GeV is found. Charmed baryon candidates are formed from hadrons with momenta greater than 2 GeV and transverse momenta greater than 0.3 GeV. In addition, we require that the average of the magnitudes of the transverse momenta of the hadrons forming the Λ þ c candidate be greater than 0.7 GeV. Kaons, pions, and protons are identified using the RICH system. Each track's IP significance with respect to the associated primary vertex is required to be greater than 9. 3 Moreover, the selected tracks must be consistent with coming from a common vertex: the χ 2 per degree of freedom (χ 2 =DOF) of the vertex fit must be smaller than 6. In order to ensure that the direction of the parent Λ 0 b is well measured, the Λ þ c vertex must be distinct from the primary pp interaction vertex. To this end, we require that the flight-distance significance of the Λ þ c candidate (defined as the measured flight distance divided by its uncertainty) with respect to the associated PV be greater than 100.
Partially reconstructed Λ 0 b baryon candidates are formed combining μ − and Λ þ c candidates that are consistent with coming from a common vertex, and we require that the angle between the direction of the momentum of the Λ þ c μ − candidate and the line from the associated PV to the Λ þ c μ − vertex be less than 45 mrad. As the Λ þ c baryon is a Λ 0 b decay product with a small but significant lifetime, we require that the difference in the component of the decay vertex position of the charmed hadron candidate along the beam axis and that of the beauty candidate be positive. We explicitly require that the Λ 0 b hadron candidate pseudorapidity be between 2 and 5. We measure η using the line defined by connecting the associated PV and the vertex formed by the Λ þ c and the μ − lepton. Finally, the invariant mass of the Λ þ c μ − system must be between 3.3 and 5.3 GeV. These selection criteria ensure that the Λ þ c candidates are decay products of Λ 0 b semileptonic decays. In particular, the background from directly produced Λ þ c (prompt Λ þ c ) is highly suppressed. This is quantified by an unbinned extended maximum likelihood fit to the two-dimensional pK − π þ invariant mass and ln(IP/mm) distributions of the Λ þ c candidates, where "/mm" refers to the length unit used to measure the IP. The ln(IP/mm) component allows us to determine the small prompt Λ þ c background. The parameters of the IP distribution of the prompt sample are found by examining directly produced charm hadrons, as described in Ref. [37]. An empirical probability density function (PDF) derived from simulation is used and we determine the prompt Λ þ c → pK − π þ fraction to be 1.5%, which can be neglected. The corresponding fit is shown in Fig. 1.
Our goal is the study of the ground-state semileptonic [38,39]. The residual contribution is expected to be accounted for by 3 The associated primary vertex to a Λ 0 b → Λ þ c μ −ν μ X candidate is selected as the primary vertex which minimizes the IP significance of the Λ þ c μ − system.
, are suppressed in the static limit and to order 1=m Q , where m Q represents the heavy-quark mass (m c or m b ) [40], with an additional stronger suppression factor of the order ðm d − m u Þ=m c rather than ðm d − m u Þ=m Λ QCD [9]. We candidates are combined with pairs of oppositecharge pions that satisfy criteria similar to those used to select the pions from the Λ þ c decay. The minimum transverse momentum of these pions is required to be 0.2 GeV, and the transverse momentum of the Λ þ c π þ π − system is required to be greater than 1.5 GeV. Lastly, the χ 2 per degree of freedom of the vertex fit for the Λ þ c π þ π − system must be smaller than 6.
The resulting spectrum, measured as the mass difference mðpK − π þ π − π þ Þ − mðpK − π þ Þ added to the known Λ þ c mass [14], is shown in Fig. 2. We see peaks corresponding to the Λ c ð2595Þ þ , Λ c ð2625Þ þ , Λ c ð2765Þ þ , and Λ c ð2880Þ þ resonances. The Λ c ð2595Þ þ is only a few MeV above the kinematic threshold, and thus it is not well described by a Breit-Wigner function. The baseline fit for this resonance uses a PDF consisting of the sum of two bifurcated Gaussian functions. As a check, we use an S-wave relativistic Breit-Wigner convolved with a Gaussian function with standard deviation σ ¼ 2 MeV that accounts for the detector resolution. While the second parametrization is more accurate, the fits to the invariant mass spectra in different kinematic bins are more stable with the baseline parametrization. We fit the Λ c ð2625Þ þ signal with a double Gaussian PDF with shared mean, as the natural width is expected to be well below the measured detector resolution. The shape of the combinatoric background PDF is inferred from wrong-sign (WS) candidates, where a π þ π þ or π − π − pair is combined with Λ þ c instead of π þ π − . In addition, we observe peaks corresponding to two higher-mass resonances, with masses and widths consistent with the Λ c ð2765Þ þ and Λ c ð2880Þ þ baryons [14]. In order to determine their yields, we fit the two signal peaks with single Gaussian PDFs with unconstrained masses and widths. The measured yields for the four Λ þ c final states, as well as the Λ þ c μ −ν μ X final state, are presented in Table II. The mass difference mðpK − π þ π þ π − Þ − mðpK − π þ Þ added to the known Λ þ c mass, m PDG ðΛ þ c Þ [14], for candidates with pK − π þ invariant mass within AE20 MeV of the known Λ þ c mass in candidate semileptonic decays for the entire w range: data are shown as black dots, the combinatoric background is shown as a blue solid line, and the gray histogram shows the WS spectrum, obtained by combining a π þ π þ or π − π − pair with Λ þ c instead of π þ π − . The signal fits are identified as follows: (a) for m < 2700 MeV, the Λ c ð2595Þ þ as a magenta dashed line and the Λ c ð2625Þ þ as a green long-dashed line; (b) for m > 2700 MeV, the Λ c ð2765Þ þ as a magenta dashed line and the Λ c ð2880Þ þ as a green long-dashed line.
The measured contributions from the two heavier Λ Ãþ c final states, shown in Table II, are smaller than those exists, but we estimate systematic uncertainties due to the subtraction of this component with an alternative semileptonic decays, where we derive both the yield and shape of the combinatoric background from the WS sample. The kinematical quantities q 2 and w in the momentum is known. The Λ 0 b flight direction can be inferred from the primary and secondary vertex locations, and this input, combined with the constraints from energy and momentum conservation, implies the following relationship for is the nominal mass of the Λ 0 b baryon, and Λ þ c identifies the pK − π þ combination. This is a quadratic equation, reflecting the lack of knowledge of the neutrino orientation in the Λ 0 b rest frame with respect to the Λ 0 b direction in the laboratory. The solution corresponding to the lower value of p Λ 0 b , which is correct between 50% and 60% of the time depending upon the kinematics of the final state, is chosen in the q 2 and w determination as simulation studies have shown that this choice introduces the smallest bias. The w resolution is estimated from simulated data in different w intervals. The distributions of differences between reconstructed and generated w are fitted with double-Gaussian functions, and the effective standard deviations are found to be between 0.01 and 0.05. The overall w resolution is estimated with a fit with a triple-Gaussian function and has an effective standard deviation σ equal to 0.028.
candidates are separated into 14 equal-size bins of reconstructed w in the full kinematic range 1 ≤ w ≤ 1.43. The parameters of the PDFs describing the signal and background components are determined from the fit to the overall pK − π þ mass spectrum. The contributions from semileptonic decays including higher-mass baryons in the final state is evaluated by fitting the Λ þ c π þ π − mass spectra with two different methods. In the first, we fit for the four resonances shown in Fig. 2 using a PDF derived from the WS sample to model the background and then use the simulation to correct for efficiency. In the second, we determine the signal yields of the Λ Ãþ c states by subtracting the WS background and treating the residual smooth component of the spectrum as originating from a semileptonic decay The second method provides an estimate of the systematic uncertainty introduced by the contribution from nonresonant Λ þ c π þ π − components of the hadron spectrum, as the smooth component of this spectrum is likely to comprise also the combinatoric background.
Next, we correct the raw Λ þ c μ −ν μ X and Λ þ c π þ π − μ −ν μ X signal yields for the corresponding software trigger efficiencies, which are derived with a data-driven method [30], based on the determination of Λ þ c μ −ν μ X events where a positive trigger decision is provided by the signal candidates and events where the trigger decision is independent of the signal. Then, we subtract the raw yields reported in Table II, scaled by the corresponding efficiency ratios simulations. The higher-mass yields are scaled by an average of these two corrections, as no model for these semileptonic decays is available. These corrections account for the efficiency loss due to the reconstruction of the additional pion pairs, as well as for the unseen Λ 0 b → Λ þ c π 0 π 0 μ −ν μ X decay, and are only mildly dependent upon the invariant mass of the final state. The expectation is that Λ 0 b → Λ þ c π þ π − μ −ν μ accounts for two-thirds of the inclusive dipion final state. We have checked this prediction by studying the inclusive final states Σ þþ where NðΣ þþ c Þ and NðΣ 0 c Þ are the detected yields for the final states Σ þþ c π − μν and Σ 0 c π þ μν, NðΣ þ c Þ is the detected yield for

Final state Yield
the final state Σ þ c μνX, and εðΛ þ c π þ π − μÞ=εðΛ þ c π 0 μÞ is the ratio between the reconstruction efficiencies of these final states calculated with simulation. A simulation study gives εðΛ þ c π þ π − μÞ=εðΛ þ c π 0 μÞ ¼ 25.9 AE 2.7, where the uncertainty reflects the limited sample size of the simulation. We obtain R ¼ 0.63 AE 0.14, where the statistical uncertainty is due to limited π 0 reconstruction efficiency, consistent with the expectation R ¼ 2=3, and a negligible Σ þ c μ −ν μ component in the denominator of Eq. (7).
is then unfolded to account for the detector resolution and other w smearing effects such as the possible choice of the wrong solution of Eq. (6). The procedure adopted is based on the single value decomposition (SVD) method [41] using the ROOUNFOLD package [42]. We choose to divide the unfolded spectrum dN u =dw into seven w bins, to be consistent with the recommendation of Ref. [43] to divide the measured spectrum into a number of bins at least twice as many as the ones in the corrected spectrum. The SVD method includes a regularization procedure that depends upon a parameter k [41], ranging between unity and the number of degrees of freedom, in our case 14. Simulation studies demonstrate that k ¼ 4 is optimal in our case. Variations associated with different choices of k have been studied and are included in the systematic uncertainties. We have performed closure tests with different simulation models of the Λ 0 b → Λ þ c μ −ν μ dynamics and verified that this unfolding procedure does not bias the reconstructed distribution. The spectra before and after unfolding are shown in Fig. 3. Finally, using simulated samples of signal events, we correct the unfolded spectrum for w-dependent acceptance and selection efficiency to obtain the distribution dN corr =dw. Various kinematic distributions have been studied in simulation and data, and we find that they are all in good agreement.
In order to determine the shape of the Isgur-Wise function ξ B ðwÞ, we use the square root of dN corr =dw divided by the kinematic factor KðhwiÞ, defined in Eq. (4), evaluated at the midpoint in the seven unfolded w bins. We derive the IW shape with a χ 2 fit, where the χ 2 is formed using the full covariance matrix of dN corr =dw.
We use various functional forms to extract the slope, ρ 2 , and curvature, σ 2 , of ξ B ðwÞ. The first functional form is motivated by the 1=N c expansion [44], where N c represents the number of colors, and has an exponential shape parametrized as The latter spectrum is then corrected for acceptance and reconstruction efficiency and fitted to the IW function ξ B ðwÞ with the procedure discussed in the text. The correlation between slope ρ 2 and curvature σ 2 =2; the three ellipses correspond to the 1σ, 2σ, and 4σ contours.
The second functional form, the so-called dipole IW function, which is more consistent with sum-rule bounds [17], is given by Finally, we can use a simple Taylor series expansion of the Isgur-Wise function and fit for the slope and curvature parameters using the Taylor series expansion introduced in Eq. (5). Figure 4 shows the measured ξ B ðwÞ and the fit results with this parametrization. Table III summarizes the slope and curvature at zero recoil obtained with the three fit models. Note that the curvature is an independent parameter only in the last fit, while in the first two models, it is related to the second derivative of the IW function.
As the slope of the IW function is the most relevant quantity to determine jV cb j in the framework of HQET [13], we focus our studies on the systematic uncertainties on this parameter. We consider several sources of systematic uncertainties, which are listed in Table IV. The first two are determined by changing the fit models for Λ þ c and Λ c ð2595Þ þ and Λ c ð2625Þ þ signal shapes in the corresponding candidate mass spectra. The software trigger efficiency uncertainty is estimated by using an alternative procedure to evaluate this efficiency using the trigger emulation in the LHCb simulation. In order to assess systematics associated with the bin size, we perform the analysis with different binning choices. The sensitivity to the Λ 0 b → Λ þ c μ −ν μ form-factor modeling is assessed by reweighting the simulated w spectra to correspond to different ξ B functions with slopes ranging from 1.5 to 1.7. The "phase space averaging" sensitivity is estimated by comparing the fit to the expression for dN corr =dw with the fit to 1=KðhwiÞ ffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffi ffi dN corr =dw p . The uncertainty associated with the Λ 0 b → Λ Ãþ c μ −ν μ modeling is evaluated by changing the relative fraction of Λ þ c π þ π − versus Λ þ c π 0 π 0 of the Λ Ãþ c spectrum by AE20%. Finally, we use the alternative evaluation of the fraction of Λ 0 b → Λ þ c π þ π − μ −ν μ which includes the maximum possible nonresonant component to assess the sensitivity to residual Λ Ãþ c components in the subtracted spectrum. The total systematic uncertainty in ρ 2 is 0.08.

VI. COMPARISON WITH UNQUENCHED LATTICE PREDICTIONS
The lattice QCD calculation in Ref. [19] uses a helicitybased description of the six form factors governing Λ 0 b → Λ transitions introduced in Ref. [45]. The calculation uses state-of-the-art techniques encompassing the entire q 2 region. The stated uncertainties on the predicted width are therefore larger than what is expected in a high-q 2 region but remain rather small, namely 6.3%. This corresponds to a 3.2% theoretical uncertainty on jV cb j, thus raising the prospect of an additional precise independent determination of jV cb j.
The simplest check on this theoretical prediction consists of a comparison of the predicted shape of dΓ=dq 2 and the measured data. Thus, we measure the distribution dN corr =dq 2 with the same procedure adopted to derive dN corr =dw, including efficiency corrections and the unfolding procedure, with the same number of bins used to determine the raw and unfolded yields. We produce seven corrected yields and their associated covariance matrix, where the nondiagonal terms are related to the unfolding procedure. We then perform a χ 2 fit to the seven experimental dN corr =dq 2 data points using the theoretical functional shape given in Eq. (85) of Ref. [19], which also provides the nominal values of the form-factor parameters, and thus we leave only the relative normalization floating. This fit uses a covariance matrix that combines experimental and theoretical uncertainties, which yields a χ 2 equal to 1.32 for 6 degrees of freedom and a corresponding p-value of 97%. This shows that the predicted shape is in good agreement with our measurement. The form-factor decomposition in Ref. [19] does not allow a straightforward extrapolation to the HQET limit of infinite heavy-quark masses. However, we know that in the static limit all the form factors are proportional to a single universal function. In order to assess how well our data are consistent with the static limit, we perform a second χ 2 fit assuming that all the form factors are proportional to a single z-expansion function [46]. Fits with different pole masses used in the six form factors determined in Ref. [19] are performed. The overall shape does not change appreciably; the pole mass of 6.768 GeV is preferred. The two fit parameters are the coefficients a 0 and a 1 , giving the strength of the first two terms in the z-expansion. The resulting fitted shape is shown in Fig. 5. This fit has a χ 2 equal to 1.85 for 5 degrees of freedom, with a corresponding p-value of 87%. Note that the shape obtained with a single form factor is very similar to the one predicted in Ref. [19]. This is consistent with the HQET prediction [15] that the shape of the differential distribution is well described by the static approximation, modulo a scale correction of the order of 10%, reflecting higher-order contributions. Further details of this fit and the fit using the lattice QCD calculation can be found in the Appendix.

VII. CONCLUSIONS
A precise measurement of the shape of the Isgur-Wise function describing the semileptonic decay Λ 0 b → Λ þ c μ −ν μ has been performed. The measured slope is consistent with theoretical models and the bound ρ 2 ≥ 3=4 [16]. The measured curvature σ 2 is consistent with the lower-bound constraint σ 2 ≥ 3=5½ρ 2 þ ðρ 2 Þ 2 [18]. The shape of dΓ=dq 2 is studied and found to be well described by the unquenched lattice QCD prediction of Ref. [19], as well as by a single form-factor parametrization. Further studies with a suitable normalization channel will lead to a precise independent determination of the CKM parameter jV cb j.

ACKNOWLEDGMENTS
We express our gratitude to our colleagues in the CERN accelerator departments for the excellent performance of the LHC. We thank the technical and administrative staff at the LHCb institutes. We acknowledge support from CERN and from the national agencies: CAPES, CNPq, FAPERJ, and This Appendix describes the formalism used in the dΓ=dq 2 fits. In particular, we give the expression of dΓ=dq 2 in terms of the form-factor basis chosen in Ref. [19], the so-called helicity form factors. In addition, we show the corresponding expression used to model the static limit.
The lattice QCD calculations reported in Ref. [19] predict the differential decay width dΓðΛ 0 b → Λ þ c μ −ν μ Þ=dq 2 as follows, Comparison between the fit to the seven experimental data points using either the lattice QCD calculation of Ref. [19], shown as gray points with a shaded area corresponding to the binned 1σ theory uncertainty, or a single form-factor fit in the zexpansion, shown as the solid blue curve. The data points, modulo a scale factor, are shown as black points with error bars.
where g ⊥ , f ⊥ , g þ , f þ , g 0 , and f 0 represent the six form factors necessary to describe this decay, X ≡ Λ c denotes the final-state baryon, m l represents the mass of the muon, q 2 is the squared four-momentum transfer between the heavy baryons, and The six form factors are cast in terms of the z-expansion [46] up to first order and have the functional form where z f ðq 2 Þ is given by and t f þ is given by and the pole masses used in the calculations are shown in Table V. The parameters a f 0 and a f 1 for the six form factors describing this decay are given in Table VIII of Ref. [19].
In the static limit, all the helicity form factors are proportional to a single universal function. Thus, we use a common z-expansion parametrization where the choice of g ⊥ reflects the choice of the pole mass used in the single z-expansion fit given in Sec. VI. We performed the fits with various choices of pole masses and examined the effects on the shape dΓ=dq 2 and found the shape did not vary significantly, though it was found that the parameters defining g ⊥ yielded the optimal fit. In this case, the fit parameters are the coefficients a 0 and a 1 in the z-expansion parametrization of g ⊥ ðq 2 Þ, which has the form shown in Eq. (A3).
APPENDIX B: MEASURED NORMALIZED SPECTRA dN corr =dq 2 AND ASSOCIATED COVARIANCE MATRIX In this Appendix, we report the seven measured data points dN corr =dq 2 and the corresponding covariance matrix, shown in Tables VI and VII, respectively. TABLE V. Masses of the relevant form-factor poles in the physical limit (in GeV).