P -wave charmed-strange mesons

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  • PHYSICAL REVIEW C 72, 065202 (2005)

    P-wave charmed-strange mesons

    Yukiko Yamada, Akira Suzuki, and Masashi KazuyamaDepartment of Physics, Tokyo University of Science, Shinjuku, Tokyo, Japan

    Masahiro KimuraDepartment of Electronics Engineering, Tokyo University of Science, Suwa, Nagano, Japan

    (Received 7 August 2005; published 9 December 2005)

    We examine charmed-strange mesons within the framework of the constituent quark model, focusing on thestates with L = 1. We are particularly interested in the mixing of two spin states that are involved in Ds1(2536)and the recently discovered DsJ (2460). We assume that these two mesons form a pair of states with J = 1.These spin states are mixed by a type of spin-orbit interaction that violates the total-spin conservation. Withoutassuming explicit forms for the interactions as functions of the interquark distance, we relate the matrix elementsof all relevant spin-dependent interactions to the mixing angle and the observed masses of the L = 1 quartet.We find that the spin-spin interaction, among various types of spin-dependent interactions, plays a particularlyinteresting role in determining the spin structure of Ds1(2536) and DsJ (2460).

    DOI: 10.1103/PhysRevC.72.065202 PACS number(s): 12.38.Bx, 12.39.Jh, 12.39.Pn, 14.40.Lb


    Recently a new charmed-strange meson, DsJ (2317), wasdiscovered by the BaBar Collaboration [1] and confirmedby the CLEO Collaboration [2]. The CLEO reported anothercharmed-strange meson called DsJ (2460). Both these mesonswere confirmed by the Belle Collaboration [3,4]. The massesand decay properties of DsJ (2317) and DsJ (2460) have beeninvestigated with two types of particular structures assumed forthem. One type is the ordinary qQ structure, and the other is anexotic structure such as the KD molecule [57,9] or tetra-quarkconfiguration [1013]. We will work with the former structurein this paper. Then, these new entries together with Ds1(2536)and Ds2(2573), which were discovered earlier, are expected toform a quartet with L = 1 (P states) of the cs (or sc) system.Given this expectation, Godfrey studied various propertiesof DsJ (2317) and DsJ (2460) [14,15], following the workdone prior to the discoveries of these mesons [16,17]. Also,decay modes of DsJ (2317) and DsJ (2460) were analyzed byColangero and De Fazio [18], Bardeen et al. [19], Mehen andSpringer [7], and Close and Swanson [8].

    With respect to the spin structure of these mesons, there arefour states, 1P1, 3P0, 3P1, and 3P2, in terms of the JLS bases.1

    While DsJ (2317) and Ds2(2573) can probably be assignedto 3P0 and 3P2, respectively, Ds1(2536) and DsJ (2460) areprobably mixtures of 1P1 and 3P1. The extent of the mixing canbe parametrized by a mixing angle [1417,20,21]. In additionto the masses of the mesons, the branching fractions for B

    Present address: Department of Physics, Kyushu University,Fukuoka, Japan.

    Present address: Department of Physics, Nagoya University,Nagoya, Japan.

    1We use the ordinary spectroscopic notation 2S+1LJ that is usedfor a two-particle system, where S,L, and J are total spin, orbitalangular momentum, and total angular momentum quantum numbers,respectively.

    DDsJ followed by the electromagnetic (EM) decays of DsJhave also been measured [3]. The mixing angles are closelyrelated to the EM decay rates of DsJ [15].

    The purpose of this paper is to examine the spin structureof the four mesons. We use the constituent quark model withthe interquark interactions that arise from the nonrelativisticexpansion of the QCD-inspired Fermi-Breit interaction. Wehave five types of interactions in the following sense. Inaddition to the spin-independent interaction that consists ofa confining potential and the color Coulomb interaction, wehave four types of spin-dependent interactions. They are thespin-spin, tensor, and two types of spin-orbit interactions, onwhich we elaborate in the next paragraph. The model is thesame as the one used by Godfrey et al. [16,17,20] except thatwe do not assume any explicit forms for the interactions asfunctions of the distance between the two quarks. We treat allspin-dependent interactions perturbatively.

    By the two types of spin-orbit interactions, we mean theones that are symmetric and antisymmetric with respect tothe interchange of the two quarks. We refer to the former asSLS and the latter as ASLS interactions. The SLS interactioncommutes with the total spin of the two quarks, whereasASLS interaction does not. The ASLS interaction violatesthe conservation of the total spin. This is the agent thatinduces the mixing of 1P1 and 3P1. The ASLS interaction isproportional to the mass difference between the quarks. Hence,its effect can be substantial when the mass difference is large,leading to a specific amount of mixing in the heavy quarklimit. This is indeed the case with the cs (or sc) system aswe will see. Historically, ASLS interaction effects were firstexamined for the -N interaction and hypernuclei [2224].Regarding the particular roles of spin-orbit interactions in qQsystems, we refer to a series of works by Schnitzer [25] andthe work by Cahn and Jackson [26] in addition to those citedalready [16,17,20].

    As we said above, we have five types of interactions. Onthe other hand, there are five pieces of experimental data now

    0556-2813/2005/72(6)/065202(7)/$23.00 065202-1 2005 The American Physical Society



    TABLE I. Summary of observed charmed-strange mesons.

    Label Mass (MeV) Assignment Year of(2S+1LJ ) discovery

    Ds 1968.3 0.5 1S0 1983 [28]Ds 2112.1 0.7 Probably 3S1 1987 [29]DsJ (2317)

    2317.4 0.9 Probably 3P0 2003 [3]DsJ (2460) 2459.3 1.3 ? 2003 [3]Ds1(2536) 2535.35 0.34 ? 1989 [30]Ds2(2573) 2572.4 1.5 Probably 3P2 1994 [31]

    available, which are the masses of the four mesons and thebranching ratio of the EM decays. [See Eq. (29).] The matrixelements of the five interactions (within the P-state sector) canbe determined such that the five pieces of the experimental dataare reproduced. At the same time, the spin structure of the fourmesons can be determined. In doing so, we do not have to knowthe radial dependence of the interactions. As it turns out, thespin-spin interaction, among the four types of spin-dependentinteractions, plays a particularly interesting role in relation tothe spin structure of Ds1(2536) and DsJ (2460).

    We begin Sec. II by defining a nonrelativistic model Hamil-tonian that incorporates relativistic corrections as variousspin-dependent interactions and proceed to determining thematrix elements of the interactions by using the mass spectraof the L = 1 quartet of charmed-strange mesons and the EMdecay widths of DsJ (2460). In Sec. III, we remark on theapproximations that we use. Discussions and a summary aregiven in the last section. In Table I we list the observedcharmed-strange mesons that we consider in this paper [27].


    We assume that the nonrelativistic scheme is appropriatefor the system, and relativistic corrections can be treatedas first-order perturbation. The nonrelativistic expansion ofthe Fermi-Breit interaction gives us the Hamiltonian for acharmed-strange meson in the form of

    H = H0 + Ss ScVS(r) + S12VT (r)+L SV (+)LS (r) + L (Ss Sc)V ()LS (r), (1)

    where Si is the spin operator of the strange quark when i = sand of the charmed quark when i = c, S = Ss + Sc, S12 is thetensor operator, and L the orbital angular momentum operator.The lowest-order terms in the nonrelativistic expansion are allin H0 which also contains a phenomenological potential toconfine the quarks. More explicitly, H0 reads as

    H0 = ms +mc + p2s

    2ms+ p


    2mc+ VC(r) + Vconf(r), (2)

    where mi and pi are the mass and momentum of quark i,respectively, VC is the color Coulomb interaction, and Vconfis the confinement potential. The last two terms of Eq. (1)are the SLS and ASLS interactions, respectively. The spatialfunctions attached to the operators in Eq. (1) can be expressedin terms of VC and Vconf [17,32]. However, we do not need

    such explicit expressions of these functions, as it will becomeclear shortly.

    We start with the eigenstates of H0 such that

    H0nJLS(r) = E(0)nLnJLS(r), (3)where

    nJLS(r) = RnL(r)J

    M=JCMYMJLS(, ). (4)

    Here CM are constants such that

    M |CM |2 = 1 and can bechosen as (2J + 1)1/2 since there is no preferable direction.We concentrate on the P states ofn = 1 with no radial node. Wedenote each of theL = 1 states with single index according to



    corresponding to


    . (5)

    Next we calculate the matrix elements of H in terms ofthe bases defined by Eqs. (3) and (4). Nonvanishing matrixelements are

    H11 = M0 34vS,H22 = M0 + 14vS 2vLS 4vT ,H33 = M0 + 14vS vLS + 2vT ,H44 = M0 + 14vS + vLS 25vT ,H13 = H31 =




    M0 =

    d3r J1S(r)H0J1S(r) = E(0)1 , (7)

    vS =


    21(r), (8)

    vLS =


    (+)LS (r)R

    21(r), (9)

    vT =

    0drr2VT (r)R

    21(r), (10)



    ()LS (r)R

    21(r). (11)

    We choose the phases of the wave functions involved inEq. (11) such that is positive. Here we have suppressedsuffix n = 1 of the wave functions and the unperturbed P-stateenergy. We have ignored the tensor coupling of the 3P2 state tothe 3F2 state. We will remark on this point in the next section.Note that the ASLS interaction gives rise to = 0, whichcauses the mixing of 1P1 and 3P1.

    All of the matrix elements of the Hamiltonian that we needare parametrized in terms M0, vS, vLS, vT , and . These fiveparameters can be determined by the four observe