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the quark model predicts the existence of heavy baryons composed of single , double and triple quarks . essential improvement has been achieved in heavy baryon spectroscopy in resent years . all baryons with a single charm quark that are predicted by the quark model have been observed in experiments . moreover , heavy baryons with a single bottom quark , such as @xmath2 , @xmath3 , @xmath4 and @xmath5 have also been discovered ( for a review see @xcite ) .    these progresses in experiments stimulated future investigation for the properties of these baryons at lhc , as well as further theoretical studies on this subject . remarkable information about the internal structure of baryons can be gained by studying their magnetic moments . magnetic moments of the heavy baryons have long been under the focus of theoretical physicists , and they have been studied in framework of various approaches . so far , magnetic moments of charmed heavy baryons have been calculated in framework of the naive quark model @xcite , relativistic quark model @xcite , chiral perturbation model @xcite , hypercentral model @xcite , soliton model @xcite , skyrmion model @xcite , bag model @xcite , qcd sum rules method @xcite , nonrelativistic quark model @xcite , phenomenological relativistic model @xcite , quark model with confinement law potential @xcite , and chiral constituent quark model , respectively . magnetic moments of heavy hadrons have also been studied in numerous works within the qcd sum rules method . magnetic moments of the @xmath6 and @xmath7 baryons have been calculated in framework of the traditional qcd sum rules method in @xcite ; of the @xmath8 and @xmath9 @xmath10 or @xmath11 baryons within the light version of the qcd sum rules method in @xcite , respectively . it should be noted here that magnetic moments of the spin-3/2 heavy baryons have already been analyzed within the same approach in @xcite . the goal of the present work is calculation of the magnetic moments of heavy @xmath12 , @xmath13 and @xmath14 baryons within the light cone qcd sum rules method . the paper is organized as follows . in section 2 , sum rules for the magnetic moments of the above - mentioned baryons are constructed . numerical results of our calculations are presented in section 3 . this section further contains comparison of our results with the predictions of other approaches , and concluding remarks . we start this section by giving a brief summarizing of the classification of heavy baryons in su(3 ) symmetry . according to su(3 ) symmetry , heavy baryons with single heavy quark belong to either symmetric sextet or antisymmetric anti - triplet flavor representations . as has already been noted , magnetic moments of the @xmath8 and @xmath9 baryons belonging to anti - symmetric flavor representations of su(3 ) are calculated within the light qcd sum rules method in @xcite and @xcite , respectively . in the present work we calculate magnetic moments of the heavy baryons belonging to sextet representation of su(3 ) group .    in order to calculate magnetic moments of the heavy sextet baryons , we start by considering the following correlation function : [ enil01 ] ( p , q ) = i d^4x e^ipx ( q ) \ { _ q ( x ) |_q(0 ) } 0  , where @xmath15 is the interpolating current of the heavy spin-1/2 baryon . the main task in constructing the sum rules for magnetic moments of the heavy sextet baryons is the calculation of the correlation function in terms of the photon distribution amplitude by using the operator product expansion ( ope ) over twist from one side , and in terms of the hadrons from the other side , and then equating both representations . calculation of the correlation function from the hadronic side is accomplished by inserting a complete set of hadrons carrying the same quantum numbers of the interpolating current @xmath15 . isolating the the ground state s contribution , we obtain , [ enil02 ] = 0 _ q b_q ( p_2 ) p_2 ^ 2-m_b_q^2 b(p_2 ) ( q ) b_q ( p_1 ) _ + , where dots correspond to the contributions of higher states and continuum , @xmath16 . in further analysis we shall make the replacement @xmath17 . the matrix elements in eq . ( [ enil02 ] ) are determined as , [ enil03 ] 0 _ q b_q ( p ) _ q u_b_q(p )  , + [ enil04 ] b_q(p ) b_q ( p_1 ) _ ^|u_b_q ( p ) u_b_q(p_1 )  , where @xmath18 is the photon polarization vector , @xmath19 and @xmath20 are the form factors . using the equation of motion , eq . ( [ enil04 ] ) can be written as , [ enil05 ] b_q(p ) b_q ( p_1 ) _ = |u_b_q ( p ) u_b_q ( p_1 ) ^  . since the photon involved in these transitions is a real photon , we set @xmath21 , and hence in calculation of the magnetic moments of the heavy sextet baryons the values of the form factors are needed only at @xmath21 .    substituting eqs . ( [ enil03 ] ) and ( [ enil05 ] ) in eq . ( [ enil02 ] ) , and performing summations over spins of the heavy baryons , for the hadronic of the correlation function we get , [ enil06 ] = _ b_q^2 ^  . we observe from eq . ( [ enil06 ] ) that the correlation function contains many structures , any of them can be chosen in calculating magnetic moments of the sextet baryons , and in this respect we choose the structure @xmath22 . this structure envelopes the magnetic form factor @xmath23 , and at @xmath21 it gives the magnetic moment @xmath24 of the heavy baryons in units of @xmath25 . as a result , the correlation function can be written in terms of the magnetic moment of heavy baryons as , [ enil07 ] = _ b_q^2 1m_b_q^2 - p^2 _ b_q 1m_b_q^2 - ( p+q)^2  .    in order to calculate the correlation function in terms of quark and gluon degrees of freedom and photon distribution amplitudes , the expressions of the interpolating currents of the heavy baryons are needed . the general form of the interpolating currents of the heavy spin-1/2 positive parity baryons is given as ( see for example @xcite ) , [ enil08 ] _ b_q - 1 ^abc \ { ( q_1^at c q^b ) _ 5 q_2^c + t ( q_1^at c _ 5 q^b ) q_2^c - ( q^at c q_2^b ) _ 5 q_1^c - t ( q^at c _ 5 q_2^b ) q_1^c }  , where @xmath26 are the color indices , @xmath27 is the charge conjugation operator , and @xmath28 is an arbitrary parameter whose value at @xmath29 gives the so - called ioffe current . the quark contents of the sextet heavy sextet baryons are given in table 1 . @xmath30    using the expression for the interpolating current and wick s theorem , the theoretical part of the correlation function for the @xmath31 can be written as , [ enil09 ] ^_b^0 -3 \ { _ 5 s_d(x ) s_b^(x ) s_u(x ) _ 5 + _ 5 s_u(x ) s_b^(x ) s_d(x ) _ 5 + _ 5 s_u(x ) _ 5 tr + _ 5 s_d(x ) _ 5 tr + t ( _ 5 s_d(x ) _ 5 s_b^(x ) s_u(x ) + _ 5 s_u(x ) _ 5 s_b^(x ) s_d(x ) + s_d(x ) s_b^(x ) _ 5 s_u(x ) _ 5 + s_u(x ) s_b^(x ) _ 5 s_d(x ) _ 5 + _ 5 s_u(x ) tr + s_u(x ) _ 5 tr + _ 5 s_d(x ) tr + s_d(x ) _ 5 tr ) + t^2 ( s_d(x ) _ 5 s_b^(x ) _ 5 s_u(x ) + s_u(x ) _ 5 s_b^(x ) _ 5 s_d(x ) + s_d(x ) tr + s_u(x ) tr ) }  , where @xmath32 , @xmath33 symbolizes transposition operator , and @xmath34 is the quark ( light or heavy ) propagator . the corresponding expressions of the correlation functions for the other members of the sextet baryons can be found from the @xmath35 by making the following replacements : [ nolabel95 ] ^_c^0 ^_c^+(u d )  , + ^_c^++ ^_c^+(d u )  , + ^_b^- ^_b^0(u d )  , + ^_b^+ ^_b^0(d u )  , + ^_c^+ ^_c^+(d s )  , + ^_c^0 ^_c^+(u d , d s )  , + ^_b^0 ^_b^0(d s )  , + ^_b^- ^_b^0(u d , d s )  , + ^_c^0 ^_c^+(u s , d s )  , + ^_b^- ^_b^0(u s , d s )  .    the correlation function described by eq . ( [ enil09 ] ) contains three different parts : a ) perturbative part , when a photon is radiated from short distance ( perturbative contribution ) ; b ) a photon is radiated from short distance from the quark propagators , and light quarks form a condensate ; c ) a photon is radiated from long distance ( nonperturbative contribution ) .    in order to calculate the perturbative contribution of the correlation function , it is enough to make the replacement [ nolabel01 ] s d^4y s^free(x - y ) ( y ) s^free(y )  , for one of the quark propagator , where @xmath36 is the free quark operator ; and the other two are being the free propagators . the expressions of the free light and heavy quarks in coordinate representation are given as , [ nolabel02 ] s_q^free - m_q 4 ^2 x^2  , + s_q^free + i m_b_q^2 4 ^2 k_2 ( m_b_q ) ( ) ^2  , where @xmath37 are the bessel functions .    the contribution of part ( c ) can easily be calculated by replacing one of the light quark operator with , [ nolabel03 ] ( s_q^ab ) _ - 14 ^ab |q^a _ i q^b ( _ i ) _  , where @xmath38 are the full set of dirac matrices , and other quark operators that involve perturbative , as well as nonperturbative terms . the explicit forms of the  full " quark propagators can be found in @xcite and @xcite . nonperturbative contribution is realized as the matrix element of the nonlocal operator @xmath39 between the vacuum and one - photon states.these matrix elements are described in terms of photon distribution amplitudes , as are given below ( see @xcite ) :    [ nolabel04 ] & & ( q ) |q(x ) _ q(0 ) 0 = -i e_q |q q ( _ q_- _ q _ ) _ 0 ^ 1 du e^i |u qx ( _ ( u ) + ( u ) ) + & & - e_q _ 0 ^ 1 du e^i |u q x h_(u ) + & & ( q ) |q(x ) _ q(0 ) 0 = e_q f_3 ( _ - q _ ) _ 0 ^ 1 du e^i |u q x ^v(u ) + & & ( q ) |q(x ) _ _ 5 q(0 ) 0 = - e_q f_3 _ ^q^x^_0 ^ 1 du e^i |u q x ^a(u ) + & & ( q ) | |q(x ) g_s g _ ( v x ) q(0 ) 0 = -i e_q ( _ q_- _ q _ ) _ i e^i ( _ |q + v _ g ) q x s(_i ) + & & ( q ) | |q(x ) g_s g _ i _ 5 ( v x ) q(0 ) 0 = -i e_q ( _ q_- _ q _ ) _ i e^i ( _ |q + v _ g ) q x ( _ i ) + & & ( q ) |q(x ) g_s g_(v x ) _ _ 5 q(0 ) 0 = e_q f_3 q_(_q_- _ q _ ) _ i e^i ( _ |q + v _ g ) q x a(_i ) + & & ( q ) |q(x ) g_s g_(v x ) i _ q(0 ) 0 = e_q f_3 q_(_q_- _ q _ ) _ i e^i ( _ |q + v _ g ) q x v(_i ) + & & ( q ) |q(x ) _ g_s g_(v x ) q(0 ) 0 = e_q \ { _ i e^i ( _ |q + v _ g ) qx t_1(_i ) + & & + _ i e^i ( _ |q + v _ g ) qx t_2(_i ) + & & + ( q_x_- q_x _ ) ( _ q_- _ q _ ) _ i e^i ( _ |q + v _ g ) qx t_3(_i ) + & & + . ( q_x_- q_x _ ) ( _ q_- _ q _ ) _ i e^i ( _ |q + v _ g ) qx t_4(_i ) } . in the definitions given above , @xmath40 is the magnetic susceptibility of the quarks , @xmath41 is the leading twist-2 , @xmath42 , @xmath43 , @xmath44 and @xmath45 are the twist-3 , and @xmath46 , @xmath47 , @xmath48 ( @xmath49 ) are the twist-4 photon das , respectively , whose explicit expressions are given in appendix a. the measure @xmath50 is defined as [ nolabel05 ] _ i = _ 0 ^ 1 d _ |q _ 0 ^ 1 d _ q _ 0 ^ 1 d _ g ( 1-_|q-_q-_g ) .    in constructing the sum rules for the magnetic moments of heavy sextet baryons it is necessary to equate the coefficients of the structure @xmath22 to from the phenomenological and theoretical representations of the correlation function . the following steps in obtaining the final form of the sum rules for the magnetic moment are : fourier transformation , borel transformation over the variables @xmath51 and @xmath52 variables , and continuum subtraction in order to suppress the contribution of the higher states and continuum . after these procedures we get the sum rules for the magnetic moment of the sextet heavy baryons , which can schematically be written in the following form , [ nolabel06 ] _ b_q_i e^m_b_q_i^2/m^2 = ^b , theor  , where the function @xmath53 contain perturbative and nonperturbative contributions . the expression for @xmath53 is quite lengthy , and for this reason we do not present it here .    in order to determine the magnetic moments of heavy sextet baryons , the value of the overlap amplitude is needed , which can be found from the analysis of the two - point correlation function . the residues of the heavy sextet baryons are calculated in @xcite , and their expressions can be found in this work . having obtained the sum rules for the magnetic moments of the heavy sextet spin-1/2 baryons , we are now ready to perform the numerical analysis . the main input parameters of the light cone qcd sum rules for the magnetic moments are the photon distribution functions das @xcite . their explicit expressions are presented in appendix a. the values of the other input parameters are : @xmath54 , @xmath55 @xcite , @xmath56 @xcite , @xmath57 @xcite @xmath58 @xcite , @xmath59 @xcite . few words about the magnetic susceptibility involved in the numerical analysis are in order . its value is estimated to have the value @xmath60 in @xcite . in @xcite , using the vector dominance model ansatz and qcd sum rules its value is predicted to be @xmath61 . furthermore , from an analysis of the radiative decays of heavy mesons its value is found to be @xmath62 @xcite . in numerical analysis we have used all these predicted values of the magnetic susceptibility . it should also be remembered that , the sum rules for the magnetic moments involve the following auxiliary parameters : the arbitrary parameter @xmath28 appearing in the expressions of the interpolating currents , borel mass parameter @xmath63 , and the continuum threshold @xmath64 . the magnetic moment must be independent of these parameters . in order to find  regions " of these parameters where magnetic moment exhibits good stability with respect to their variations we proceed as follows . firstly , we try to find the upper and lower bounds of borel mass parameter at fixed values of @xmath64 and @xmath28 . the upper bound of @xmath63 can be determined by requiring that the contribution due to the continuum threshold should be less than half of the contribution coming from the perturbative part . the lower bound of @xmath63 can be found by demanding that the higher powers of @xmath65 contribute less than the leading twist contributions . our numerical analysis shows that these two conditions are satisfied simultaneously if @xmath63 ranges in the following regions : [ nolabel09 ] & & 2.0  gev^2 m^2 3.0  gev^2  _ c + & & 2.2  gev^2 m^2 3.4  gev^2  _ c^ + & & 2.5  gev^2 m^2 4.0  gev^2  _ c + & & 5.0  gev^2 m^2 6.0  gev^2  _ b + & & 5.0  gev^2 m^2 6.4  gev^2  _ b^ + & & 5.2  gev^2 m^2 7.0  gev^2  _ b    in regard to the continuum threshold @xmath64 appearing in the sum rules , it is known that the values of this arbitrary parameter is related to the energy of first excited state . the difference @xmath66 , where @xmath67 is the ground state mass of the baryon , is the energy needed to excite the particle to its first energy state . this quantity usually varies between @xmath68 and @xmath69 . analysis of the mass sum rules shows that , in order to reproduce the experimental mass of the sextet baryons the continuum threshold should vary in the following domain : [ nolabel10 ] = \ {    c ( 3.10.1 )  gev  _ c + ( 3.20.1 )  gev  _ c^ + ( 3.30.1 )  gev  _ c + ( 6.60.2 )  gev  _ b + ( 6.70.2 )  gev  _ b^ + ( 6.80.2 )  gev  _ b    . having determined the sum rules , input parameters , and working regions of all auxiliary parameters , we perform numerical analysis to calculate the magnetic moment @xmath24 of the heavy sextet spin-1/2 baryons , whose results we can summarize as follows . as examples , in figs . 1 and 2 we present the dependence of @xmath70 on @xmath63 at several fixed values of @xmath28 and at the fixed value of @xmath64 listed above for the baryons @xmath71 and @xmath72 , respectively . we observe from these figures that the magnetic moments of @xmath12 show good stability with respect to the variation of the borel mass parameter in aforementioned domains . the next step in finding the values of the magnetic moments of the baryons under consideration is to determine working region of the arbitrary parameter @xmath28 , where @xmath24 is practically independent of its variation . for this purpose , in figs . 3 and 4 the dependence of @xmath70 on @xmath73 , where @xmath74 for the @xmath71 and @xmath72 baryons , at several fixed values of the borel mass parameter @xmath63 and at the predetermined value of the continuum threshold @xmath64 , are presented , respectively . it follows from these figures that the magnetic moments of the heavy sextet spin-1/2 baryons seem to be practically independent of the arbitrary parameter @xmath28 in the domain @xmath75 , and insensitive to the the chosen values of @xmath64 . our final results on the magnetic moments of the heavy sextet spin-1/2 baryons are presented in table 2 . for comparison , in the same table we present the predictions of other approaches on the magnetic moments of the relevant baryons , such as nonrelativistic quark model @xcite , bag model @xcite , phenomenological relativistic quark model @xcite , quark model with confinement law potential @xcite , relativistic quark model @xcite , hypercentral model @xcite , chiral constituent model @xcite , and qcd sum rules method @xcite . @xmath76    we observe from this table that almost all approaches give , more or less , similar predictions , except the results of @xcite and @xcite ( especially for the charmed baryons ) , which are smaller .    using our results one can easily deduce the following relations among the magnetic moments of heavy baryons . [ nolabel11 ] _ _ c^++ + _ _ c^0 2 _ _ c^+  , + _ _ c^++ + _ _ c^0 2 _ _ c^+  , + _ _ c^++ + 2 _ _ c^0 _ _ c^0 + 2 _ _ c^+  , + _ _ b^+ + _ _ b^- 2 _ _ b^0  , + _ _ b^+ + _ _ b^- 2 _ _ b^0  , + _ _ b^+ + 2 _ _ b^- _ _ b^- + 2 _ _ b^0  ,    the direct measurement of the magnetic moments of heavy baryons are unlikely in the near future . therefore , any indirect estimations of the magnetic moments of the heavy baryons could be very useful . for example , it could help extracting information about the mass spectrum of the heavy baryons . as is well known , experimentally measured mass difference is attributed to the hyperfine splitting . moreover , the magnetic moments of quarks are proportional to the chromomagnetic moments , which determine the hyperfine splitting in the baryon spectrum . following this reasoning , the magnetic moments of the @xmath6 and @xmath2 baryons are estimated in @xcite . hence , this approach could be an essential tool in estimating the magnetic moments of the heavy baryons .    in conclusion , the magnetic moments of the heavy sextet @xmath77 baryons are calculated in framework of the light cone qcd sum rules method . empirically , linearly independent relations among the magnetic moments of the sextet baryons are obtained . comparison of our results with the predictions of other approaches is presented . explicit forms of the photon das @xcite .    [ nolabel27 ] _ ( u ) 6 u |u  , + ^v(u ) 3 [ 3 ( 2 u - 1)^2 -1 ] + ( 15 w^v_- 5 w^a _ ) [ 3 - 30 ( 2 u - 1)^2 + 35 ( 2 u -1)^4 ]  , + ^a(u ) ( 1 + w^v_- w^a _ )  , + a(_i ) 360 _ q _ |q _ g^2  , + v(_i ) 540 w^v_(_q - _ |q ) _ q _ |q _ g^2  , + h_(u ) - 10 ( 1 + 2 ^+ ) c_2^(u - |u )  , + ( u ) 40 u^2 |u^2 ( 3 - ^+ + 1 ) + 8 ( _ 2^+ - 3 _ 2 ) [ u |u ( 2 + 13 u |u ) + 2 u^3 ( 10 -15 u + 6 u^2 ) ( u ) + 2 |u^3 ( 10 - 15 |u + 6 |u^2 ) ( |u ) ]  , + t_1(_i ) -120 ( 3 _ 2 + _ 2^+)(_|q - _ q ) _ |q _ q _ g  , + t_2(_i ) 30 _ g^2 ( _ |q - _ q ) [ ( - ^+ ) + ( _ 1 - _ 1^+)(1 - 2_g ) + _ 2 ( 3 - 4 _ g ) ]  , + t_3(_i ) - 120 ( 3 _ 2 - _ 2^+)(_|q -_q ) _ |q _ q _ g  , + t_4(_i ) 30 _ g^2 ( _ |q - _ q ) [ ( + ^+ ) + ( _ 1 + _ 1^+)(1 - 2_g ) + _ 2 ( 3 - 4 _ g ) ]  , + s(_i ) 30_g^2\{(+ ^+)(1-_g)+(_1 + _ 1^+)(1 - _ g)(1 - 2_g ) + _ 2 [ 3 ( _ |q - _ q)^2-_g(1 - _ g ) ] }  , + ( _ i ) -30_g^2\{(- ^+)(1-_g)+(_1 - _ 1^+)(1 - _ g)(1 - 2_g ) + _ 2 [ 3 ( _ |q - _ q)^2-_g(1 - _ g)]}. the parameters entering the above da s are borrowed from @xcite whose values are @xmath78 , @xmath79 , @xmath80 , @xmath81 , @xmath82 , @xmath83 , @xmath84 , @xmath85 , and @xmath86 . 99    k. olive _ et . al _ , particle data group , chin . c * 38 * , 090001 ( 2014 ) . a. l. choudry , v. joshi , phys . d * 13 * , 3115 ( 1976 ) . d. b. lichtenberg , phys . d * 15 * , 345 ( 1977 ) . a. faessler _ et . al _ , phys . d * 73 * , 094013 ( 2006 ) . m. savage , phys . b * 326 * , 303 ( 1994 ) . b. patel , a. k. rai , p.c . vinodkumar , j. phys . g * 35 * , 065001 ( 2008 ) . d. o. riska , nucl . inst . method . b * 119 * , 259 ( 1996 ) . y. oh , d. p. min , m. rho , n. n. scoccola , nucl . phys . a * 534 * , 493 ( 1991 ) . a. bernotas , and v. simonis , lithuanian journal of phys . * 53 * , 84 ( 2013 ) . s. l. zhu , w. y. hwang , and z. s. yang , phys . d * 56 * , 7273 ( 1997 ) . j. franklin , d. b. lichtenberg , w. mamgung , and d. c. carydas , phys . d * 24 * , 2910 ( 1981 ) . b. julia - diaz , and d. o. riska , nucl . a * 739 * , 69 ( 2004 ) . m. barik , and h. das , phys . d * 29 * , 2823 ( 1983 ) . n. sharma , p. k. chatley , and m. gupta , phys . d * 81 * , 073001 ( 2010 ) . t. m. aliev , a. zpineci , m. savci , phys . d * 65 * , 096004 ( 2002 ) . t. m. aliev , k. azizi , m. savci , phys . d * 77 * , 114006 ( 2008 ) . t. m. aliev , k. azizi , a. zpineci , nucl . b * 808 * , 137 ( 2009 ) . e. bagan , m. chabab , h. g. dosch , s. narison , phys . b * 278 * , 369 ( 1992 ) . i. i. balitsky , v. m. braun , nucl . phys . b * 311 * , 541 ( 1998 ) . v. m. braun , j. e. filyanov , z. phys . c * 48 * , 239 ( 1990 ) . p. ball , v. m. braun , and n. kivel , nucl . b * 649 * , 263 ( 2003 ) . t. m. aliev , k. azizi , a. zpineci , phys . d * 79 * , 056005 ( 2009 ) . v. m. belyaev , b. l. ioffe , jetp * 56 * , 493 ( 1982 ) . k. g. chetyrkin , a. khodjamirian , a. a. pirovarov , phys . b * 661 * , 250 ( 2008 ) .    c. a. dominguez , n. f. nasrallah , r. rontisch , k. schilcher , j. high energy phys . * 05 * 020 , ( 2008 ) . v. m. belyaev , and y. i. kogan , yad . fiz . * 40 * , 1035 ( 1984 ) . j. rohrwild , j. high energy phys . * 09 * , 073 ( 2007 ) . m. karliner , h. lipkin , phys . b * 660 * , 539 ( 2008 ) . * fig . ( 1 ) * the dependence of the magnetic moment of the @xmath71 baryon on @xmath63 , at several fixed values of @xmath28 , and at @xmath87 . +   + * fig . ( 2 ) * the same as fig . ( 1 ) , but for the @xmath72 baryon , at @xmath88 . +   + * fig . ( 3 ) * the dependence of the magnetic moment of the @xmath71 baryon on @xmath73 , at several fixed values of @xmath63 , and at @xmath87 . +   + * fig . ( 4 ) * the same as fig . ( 3 ) , but for the @xmath72 baryon , at @xmath88 .
the magnetic moments of heavy sextet @xmath0 baryons are calculated in framework of the light cone qcd sum rules method . 
 linearly independent relations among the magnetic moments of these baryons are obtained . 
 the results for the magnetic moments of heavy baryons obtained in this work are compared with the predictions of the other approaches . 
 # 1#2#3    @xmath1        # 1#2#3    @xmath1        0^*0 5_5 q 5_5    o _ ^0 _    pacs numbers : 11.55.hx , 13.40.em , 14.20.mr , 14.20.lq