2+\left( 1-\frac{3\alpha }{l^{2}}\right) ^{1/3}\right] ^{2}},  \label{Leff}$$

It is notable that the effective $l_{\mathrm{eff}}$ reduces to $l$ as $%
\alpha $ goes to zero. Having the finite action and using the Brown–York method of a quasilocal definition [@BY] with Eq. (\[Ibulk\])-(\[Ict\]), one can introduce a divergence-free stress-energy tensor as follows $$T^{ab}=\frac{2}{{\sqrt{-\gamma }}}\frac{{\partial (\mathcal{I}_{G}+\mathcal{I%
}_{\mathrm{ct}})}}{{\partial \gamma {_{ab}}}}=\frac{1}{8\pi }\left[
(K^{ab}-K\gamma ^{ab})+2\alpha (3J^{ab}-J\gamma ^{ab})+\frac{n-1}{l_{\mathrm{%
eff}}}\gamma ^{ab}\right] .  \label{Tab}$$The quasilocal conserved quantities associated with the stress-energy tensor of Eq. (\[Tab\]) can be defined as $$Q(\xi )=\int_{\mathcal{B}}d^{n-1}\varphi \sqrt{\gamma }T_{ab}n^{a}\xi ^{b},
\label{Conserved}$$where the the timelike unit vector $n^{a}$ is normal to the boundary $B$ and $\xi ^{b}$ is the Killing vector. Regarding temporal Killing vector $\xi
=\partial /\partial t$ and taking into account Eqs. (\[Conserved\]) and (\[Tab\]), we can calculate the mass per unit volume $V_{n-1}$ as $$M=\frac{\left( n-1\right) }{16\pi }m.  \label{Massk0}$$We should note that the parameter $m$ can be calculated by using of the fact that the metric function vanishes at the event horizon, $r_{+}$. Although one can check that the form of Eq. (\[Massk0\]) is valid for $k=\pm 1,0$, we should indicate that, unlike $k=\pm 1$ cases, the mass parameter, $m$, does not depend on the Lovelock parameter for the boundary flat solutions.

Although we 