Case 1, 3 Case 2 y 16 κ 2 ω 2 − 1 64 κ 2 3 ν 2 − 3 Δ √$_{6(}$$_{y}$$_{+1)}$$_{/y}$ 8 π K ′ √$_{6(}$$_{y}$$_{+3)}$$_{/y}$ 8 π K ′ R 0 0 Q$_{3}$ 0 3 √ 2 y 32 π ( 3+ y y K ′ − E ′ ) Q$_{8}$ 0 0 J$_{3}$ √ 6 y 16 π ( y +1 y K ′ − E ′ ) 0 Since the unitarity bound Δ ≥ | R | is not saturated asymptotically, the dual operators are not expected to be holomorphic. To help the identification, we quote here the dictionary of gauge/membrane correspondence. All we can say about the dual operators is that their composition is such that the vanishing global charges cancel. For instance, R → 0 implies we should have the same number of X ’s as ¯ X ’s for infinitely long operators. Thus these states are far from supersymmetric, and it will be highly nontrivial to verify the correspondence by comparing the spectrum of the quiver Chern-Simons theory. In this paper we have studied the classical membrane action in a nontrivial 11 dimensional background, AdS$_{4}$ × M 1 , 1 , 1 . The AdS/CFT correspondence implies classical solutions with large energy give an approximate description of dual field theory operators which are very long. A rigid configuration is required to rotate to satisfy the equation of motion, and the angular momenta in the internal space M 1 , 1 , 1 correspond to some global charges on the field theory side. V. DISCUSSION 16 TABLE III. Conserved charges for toroidal membranes. K ′ ≡ K (1 /y ) , E ′ ≡ E (1 /y ). R = 2 $^{[}$#( XXX ) − #( ¯ X ¯ X ¯ X ) $^{]}$, (53) Q$_{3}$ = 1 2 $^{[}$#( X $^{1}$) + #( ¯ X $^{2}$) − #( ¯ X $^{1}$) − #( X $^{2}$) $^{]}$, (54) Q$_{8}$ = 1 2 √ 3 $^{[}$#( X $^{1}$) + #( X $^{2}$) − 2#( X $^{3}$) − #( ¯ X $^{1}$) − #( ¯ X $^{2}$) + 2#( ¯ X $^{3}$) $^{]}$, (55) J$_{3}$ = #( X$_{12}$X$_{23}$X$_{23}$ ) − #( X$_{12}$X$_{31}$X$_{31}$ ) − #( ¯ X$_{12}$ ¯ X$_{23}$ ¯ X$_{23}$ ) + #( ¯ X$_{12}$ ¯ X$_{31}$ ¯ X$_{31}$ ) . (56)