This was determined by fitting CAM-B3LYP orbital energies to those obtained using the short-range corrected SRC1 functional (see Fig. ), because that functional was specifically parameterized to obtain corelevel spectra with experimental accuracy, via TD-DFT calculations. In other words, rather than shifting spectra with respect to experiment, as is required in TD-DFT calculations using B3LYP or CAM-B3LYP, we shift the core orbital energies obtained from CAM-B3LYP to match the corresponding SRC1 values, in the ground state. Our aim is to reduce the inherent error in core-level eigenvalues obtain from CAM-B3LYP that, when left uncorrected, tend to be higher (less bound) than SRC1 values due to self-interaction error (SIE). Note that SRC1 uses a large fraction of exact exchange only a length scale < 1 Å, in order to reduce SIE in the core states. For elements through Ne, the shift introduced in Eq. ( ) for |ε| ≤ 102 E h is essentially the same as what is used Grimme's B3LYP-based implementation, because core-level eigenvalues from both B3LYP and CAM-B3LYP underestimate excitation energies for xray absorption by approximately the same amount. The present work extends the parameterization to third-row elements (|ε| > 102 E h ). Our choice for the modifications in Eqs. ( ) and ( ) is motivated by the observation that the majority of the correction in B3LYP/CIS comes from the c 1 parameter. The exponential correction in Eq. ( ) that is used in B3LYP/CIS was introduced by Grimme in order to deal with Rydberg and charge-transfer states where the exchange integral K ia is much smaller than it is compared for localized valence excitations, but the de-pendence on the Coulomb integral J in Eq. ( ) is inconvenient from an implementation perspective. Range separation in the CAM-B3LYP functional equips this method to better account for charge-separated states, as compared to B3LYP, so the more complicated form of ∆J(ε) was avoided in our re-parameterization.