x_i v_i \right)^2} \left[v_j + v_k - \frac{\sum_i x_i
    v_i^2}{\left(1+ \sum_i x_i v_i \right) } \right]~.$$ The Eq. (\[pjk\]) for $j=k$ leads to the following result for $\omega_j$, $$\begin{aligned}
\label{omega-j-vdw}
\omega_j ~=~ 1~ +~
\lambda_j~ \frac{\partial^2 p}{\partial \lambda_j^2 }  ~ \times
~\left(   \frac{\partial p}{\partial
  \lambda_j} \right)^{-1}
  ~=~1~-~\frac{x_j}{1~+~\sum_iv_ix_i}~~\left(2v_j~-~\frac{\sum_i
v_i^2 x_i} {1~+~\sum_i v_ix_i}\right)~.\end{aligned}$$ The Eq. (\[omega-j-vdw\]) is reduced to Eq. (\[omegavdw\]) for the one-component VDW gas. For an ‘almost‘ ideal gas when all proper volumes come to zero, $v_i \rightarrow 0$, one finds the ideal gas results, $\langle N_j \rangle \cong V\phi_j$ and $\omega_j \cong 1$, from Eqs. (\[Nmvdw\]) and (\[omega-j-vdw\]), respectively. The above equations are simplified if the proper volumes of different hadron species are equal to each other, $v_i=v$. The scaled variance (\[omega-j-vdw\]) becomes then equal to: $$\begin{aligned}
\label{omega-j-vdw-a}
\omega_j
  ~=~1~-~v~\frac{x_j~(2~+~v~\sum_ix_i)}
 {(1~+~v~\sum_i x_i)^2}~.\end{aligned}$$ The Eq. (\[omega-j-vdw-a\]) demonstrates a suppression of the particle number fluctuations for all hadron species ($\omega_j <
1$). At small total particle number density, $v\sum_ix_i\ll 1$, it behaves as, $\omega_j\cong 1- 2v\phi_j$, similar to the one-component VDW gas. In the opposite limiting case, $v\sum_ix_i\gg 1$, one finds, $\omega_j\cong 1-
\phi_j/\sum_i\phi_i=1-n_j^{id}/n_{tot}^{id}$. In a dense VDW gas the particle number fluctuations are suppressed, and the suppression for $j$th species 